2.1 Forces acting upon dust particles

The dynamics of charged dust particles is governed by the various forces acting on them in the plasma medium. A brief overview of these dust forces is given.

1. (i) Gravitation force. The dust grains have finite mass; therefore, they will experience the force due to the Earth's gravity. For a spherical dust grain of mass $M_d$, the gravitation force $F_g$ is (Nitter Reference Nitter1996; Shukla & Mamun Reference Shukla and Mamun2002a)

   (2.1)\begin{equation} \boldsymbol{F_g} = M_d \boldsymbol{g} = \frac{4}{3} {\rm \pi}r^3_d \rho_d \boldsymbol{g} , \end{equation}
   where $g$ is the acceleration due to gravity, $r_d$ is the radius of the dust grain and $\rho _d$ is the mass density of the dust grain.

2. (ii) Electrostatic force. The dust grains undergo various charging mechanisms in the plasma background and acquire a large amount of charge ($Q_d \sim 10^2$–$10^5 e^{-}$) on their surface. The amount of charge on the dust-grain surface is decided by the surface potential of particles ($V_s$) with respect to the plasma potential and the size of dust particles (Goree Reference Goree1994) ($Q_d = 4 {\rm \pi}\epsilon _0 r_d V_s$). This shows that the net charge on the dust-grain surface scales linearly with the radius of the dust particle for a given discharge. In laboratory discharges, the charged dust particles experience an electrostatic force $F_E$ due to the electric field $E$. This force is (Nitter Reference Nitter1996; Shukla & Mamun Reference Shukla and Mamun2002a)

   (2.2)\begin{equation} \boldsymbol{F_E} = Q_d \boldsymbol{E} ={\pm} e Z_d \boldsymbol{E} , \end{equation}
   where $Q_d = \pm e Z_d$ is the dust charge.

3. (iii) Ion drag force. The dust grains are confined in an electrostatic potential well. The streaming ions in the electric field exert a force on the dust grains in two ways. The ions transfer momentum to dust particles through direct impacts ($F_{ic}$). Secondly, the ions transfer momentum through Coulomb collisions with the charged dust particles ($F_{io}$). The formulations of both forces (Barnes et al. Reference Barnes, Keller, Forster, O'Neill and Coultas1992; Nitter Reference Nitter1996; Shukla & Mamun Reference Shukla and Mamun2002b) under the approximation $\lambda _D/l_i\ll 1$, where $\lambda _D$ is the dust Debye (screening) length and $l_i$ is the ion mean free path, are given as

   (2.3)\begin{equation} F_{ic} = n_i v_s m_i v_i {\rm \pi}b^2_c, \end{equation}
   where $n_i$ is the plasma number density, $m_i$ is the ion mass, $v_s$ is the mean speed and $b_c$ is the collection impact parameter, and
   (2.4)\begin{equation} F_{io} = n_i v_s m_i v_i 4 {\rm \pi}b^2_{{\rm \pi}/2} \varGamma, \end{equation}
   where $b^2_{{\rm \pi} /2}$ is the impact parameter whose asymptotic angle is ${\rm \pi} /2$ and $\varGamma$ is the Coulomb logarithm integrated over the interval from $b_c$ to $\lambda _D$. So the net ion drag force acting on a charged grain is $F_i = F_{ic} + F_{io}$. Since $\boldsymbol {F_I}$ is acting in the direction of the electric field, it can be written in terms of local electric field vector $\boldsymbol {F_I} = F_i \hat {E}$. For a collisional dusty plasma, an updated formulation to estimate the ion drag force is required (Khrapak et al. Reference Khrapak, Ivlev, Morfill and Thomas2002; Patacchini & Hutchinson Reference Patacchini and Hutchinson2008).

4. (iv) Neutral drag force. The neutral drag force is a kind of resistance experienced by the dust grains if they have relative velocity or motion with respect to the background neutral gas. For dust particles of size ($r_d$) smaller than the collision mean free path ($\lambda _{mpf})$, i.e. $r_d\ll \lambda _{mpf}$, and velocities much smaller than the thermal velocity of the gas, i.e. $v_d\ll v_{tn}$, the neutral drag force experienced by the dust particles is estimated using the Epstein expression (Epstein Reference Epstein1924):

   (2.5)\begin{equation} \boldsymbol{F_n} ={-}M_d \nu_{dn} \boldsymbol{v_d}, \end{equation}
   where $\nu _{dn}$ is the dust–neutral collision frequency and $\boldsymbol {v_d}$ is the relative velocity of dust particles to that of the neutral gas atoms. An expression for $\nu _{dn}$ is
   (2.6)\begin{equation} \nu_{dn} = \delta \frac{4 {\rm \pi}}{3} r_d^2 n_g \frac{m_n}{M_d} v_n, \end{equation}
   where $n_g$ is the neutral number density, $m_n$ is the mass of the neutral atoms and $v_n$ is the average thermal speed of the gas atoms. The estimated value of $\delta$ is $1.44 \pm 0.19$ (Liu et al. Reference Liu, Goree, Nosenko and Boufendi2003).

5. (v) Thermophoretic force. The thermophoretic force arises due to a temperature gradient in the background neutral gas. The gas atoms present in the high-temperature zone exert more momentum on the confined dust particles than those present in the lower-temperature zone. Consequently, a thermophoretic force is established opposite to the temperature gradient. The magnitude of this force (Shukla & Mamun Reference Shukla and Mamun2002a) is written as

   (2.7)\begin{equation} \boldsymbol{F_{th}} ={-} \frac{32}{15} \frac{r^2_d}{v_{th,n}} \left(1 + \frac{5 {\rm \pi}}{32} (1 - \alpha)\right)\kappa_T \boldsymbol{\nabla} T_n, \end{equation}
   where $\kappa _T$ is the translation thermal conductivity of the gas and $T_n$ is the neutral gas temperature. The spatial scale of the temperature gradient is greater than the size (diameter) of the dust grains (Zheng Reference Zheng2002). The value of $\alpha$ is $\approx$1 for dust particles and neutral gas atoms having temperatures below 500 K.

2.2 Physics of the driven vortices

The observed vortices/coherent structures in a dusty plasma can be categorized as externally driven and instability-driven vortices. In the externally driven vortices, dust grains behave as trace particles in the plasma background. Since the dynamics of the dust-grain medium is associated with the background plasma species (electrons, ions and neutrals), any internal and/or external electromagnetic or non-electromagnetic perturbation alters the dynamics of ambient plasma species and sets the dust cloud into rotational motion.

In the fluid description of a dusty plasma, the transport/motion of charged dust particles in the background of ambient plasma is understood by solving the equation of motion of dust particles under the action of driving and friction forces. The fluid equation of motion for the dust-grain medium, which is assumed to be incompressible in nature, is (Akdim & Goedheer Reference Akdim and Goedheer2003; Bockwoldt et al. Reference Bockwoldt, Arp, Menzel and Piel2014)

(2.8)\begin{equation} M_d n_d \left(\frac{{\rm d}\boldsymbol{v_d}}{{\rm d}t}\right) = n_d (\boldsymbol{F_g} + \boldsymbol{F_E} + \boldsymbol{F_i} + \boldsymbol{F_n} + \boldsymbol{F_{th}}) -\boldsymbol{\nabla} P_E + \eta \nabla^2 \boldsymbol{v_d}, \end{equation}

where $\boldsymbol {F_g}, \boldsymbol {F_E}, \boldsymbol {F_i}, \boldsymbol {F_n}$ and $\boldsymbol {F_{th}}$ are the gravitational force, electric force, ion drag force, neutral drag force and thermophoretic force acting on a single dust grain; $n_d$ is the dust number density; $\boldsymbol {v_d}$ is the dust fluid element velocity; $\boldsymbol {\nabla } P_E$ is the pressure force arising due to the dust–dust interactions and confinement of dust particles in an electrostatic potential well; $\eta$ is the kinetic viscosity of the dust-grain medium; and the whole term ($\eta \nabla ^2 \boldsymbol {v_d}$) represents a viscous force acting between layers of flowing dust grains. If dusty plasma experiments are performed at higher pressure ($P > 15\,{\rm Pa}$), then the contribution of viscous friction can be ignored compared with the friction due to background neutral gas. In normal radio-frequency (RF) discharges and low-power direct-current (DC) discharges, the magnitude of the thermophoretic force acting on dust grains is a few orders lower than that of other dominant forces. Therefore, the contribution of thermophoresis force can also be dropped in the equation of motion (2.8). Equation (2.8) takes the form

(2.9)\begin{equation} \left(\frac{{\rm d}\boldsymbol{v_d}}{{\rm d}t}\right) = \frac{1}{M_d}(\boldsymbol{F_g} + \boldsymbol{F_E} + \boldsymbol{F_i} + \boldsymbol{F_n}) -\frac{n_d}{M_d n_d^2}\boldsymbol{\nabla} P_E. \end{equation}

The vortex motion of dust grains in a two-dimensional (2-D) plane can be described by the vorticity equation. After taking the curl of (2.9), we get the vorticity equation for the dust-grain medium:

(2.10)\begin{gather} \frac{{\rm d}\boldsymbol{\omega}}{{\rm d}t} = \frac{1}{M_d} \left(\boldsymbol{\nabla} \times \boldsymbol{F_g} + \boldsymbol{\nabla} \times \boldsymbol{F_E} + \boldsymbol{\nabla} \times \boldsymbol{F_i} + \boldsymbol{\nabla} \times \boldsymbol{F_n}\right) \nonumber\\ - \frac{1}{M_d n^2_d}\boldsymbol{\nabla} n_d \times \boldsymbol{\nabla} P_E, \end{gather}

where $\boldsymbol {\omega } = \boldsymbol {\nabla } \times \boldsymbol {v_d}$ is the angular frequency or vorticity vector. Since the gravitational field is curl-free, $\boldsymbol {\nabla } \times \boldsymbol {F_g} = 0$. It is also observed in many experiments that a dusty plasma is nearly homogeneous in a 2-D plane. In the case of a large-aspect-ratio dusty plasma (Choudhary, Mukherjee & Bandyopadhyay Reference Choudhary, Mukherjee and Bandyopadhyay2018) the dusty plasma is expected to be inhomogeneous. However, the dust-grain medium is normally homogeneous to the length scale of the size of the vortex structure. Therefore, $\boldsymbol {\nabla } n_d \approx 0$ for such a nearly homogeneous dusty plasma. With all these approximations, the vorticity equation (2.10) takes the form

(2.11)\begin{equation} \frac{{\rm d}\boldsymbol{\omega}}{{\rm d}t} = \frac{1}{M_d}\left(\boldsymbol{\nabla} \times \boldsymbol{F_E} + \boldsymbol{\nabla} \times \boldsymbol{F_i} + \boldsymbol{\nabla} \times \boldsymbol{F_n}\right). \end{equation}

It is clear from (2.11) that vortex generation in a dusty plasma is possible if electrostatic or ion drag force is non-conservative in the background of neutral atoms having random motion. In such a dusty plasma system, the neutral drag force has only a dissipative effect on dust-grain motion. Coherent or vortex structures in dusty plasmas indeed have a finite lifetime; therefore, steady-state solutions of the vorticity equation (2.11) would describe the onset of such dynamic structures. For the steady-state condition, (2.11) transforms to

(2.12)\begin{equation} 0 = \left(\boldsymbol{\nabla} \times \boldsymbol{F_E} + \boldsymbol{\nabla} \times \boldsymbol{F_i} + \boldsymbol{\nabla} \times \boldsymbol{F_n}\right). \end{equation}

For a given discharge configuration, we can write the electric field force in terms of the plasma potential ($\varPhi$) and charge ($Q_d$): $\boldsymbol {F_E} = -Q_d \boldsymbol {\nabla } \varPhi$. The ion drag force is directed along the electric field and flow of ions. Therefore, the ion drag force vector can be written as $\boldsymbol {F_i} = F_i \hat {E}$, where $F_i$ is an ion drag force function (magnitude) and $\hat {E}$ represents the direction of ion drag force. The neutral drag force is $\boldsymbol {F_n} = -M_d \nu _{dn} \boldsymbol {v_d}$.

Once substituting the value of forces in (2.12), we have

(2.13)\begin{gather} M_d \nu_{dn} \boldsymbol{\nabla} \times \boldsymbol{v_d} = \boldsymbol{\nabla} Q_d \times \boldsymbol{E} + \boldsymbol{\nabla} F_i \times \hat{E}, \end{gather}

(2.14)\begin{gather} \boldsymbol{\nabla} \times \boldsymbol{v_d} = \frac{1}{M_d \nu_{dn}}\left(\boldsymbol{\nabla} Q_d \times \boldsymbol{E} + \boldsymbol{\nabla} F_i \times \hat{E}\right). \end{gather}

There are two possible driving forces or free energy sources, $\boldsymbol {\nabla } Q_d \times \boldsymbol {E}$ and $\boldsymbol {\nabla } F_i \times \hat {E}$, to sustain the vortex motion of a homogeneous and incompressible dust cloud against frictional losses. In other words, the stable vortex motion of charged microparticles in the dusty plasma medium can only occur in the presence of free energy sources, compensating for the energy losses.

The first term, $\boldsymbol {\nabla } Q_d \times \boldsymbol {E}$, will be non-zero if $\boldsymbol {\nabla } Q_d \neq 0$. This is the case when there is a finite dust charge gradient. Similarly, the second term, $\boldsymbol {\nabla } F_i \times \hat {E}$, will be non-zero if $\boldsymbol {\nabla } F_i \neq 0$. This means that the gradient in ion drag force, which is not parallel to the electric field, can also excite the vortex motion of the dust cloud. The values of these vortex driving terms strongly depend on the discharge configuration used to produce the dusty plasma.

In most experimental dusty plasmas (finite systems), there are two electric field ($\boldsymbol {E}$) components. One is required to hold dust grains against gravity and the other helps compensate for the repulsive forces of dust grains. The ion drag force can have a gradient vertically (along gravity) as well as horizontally (in plane) or along an arbitrary direction near the power electrode/wall of the chamber. Whenever the value of the driving force term $\boldsymbol {\nabla } F_i \times \hat {E}$ is non-zero, dust grains experience a force that rotates them in the given plane. These dust grains rotating about a common axis passing through an origin (centre of the vortex structure) form the stationary vortex structures in that plane. A schematic representation of the rotational motion in the presence of an ion drag gradient orthogonal to the electric field is depicted in figure 1(a).

Figure 1.

A schematic representation of the rotational motion in a 2-D plane due to (a) ion drag gradient along with orthogonal electric field and (b) dust charge gradient ($\beta$) along with orthogonal non-electrostatic force (gravity). The blue curved line with an arrow presents the direction of rotating particles in this $Y$–$Z$ plane.

In RF capacitively coupled discharge dusty plasmas, it is possible to estimate the curl of ion drag force ($\boldsymbol {\nabla } \times \boldsymbol {F_i}$) in terms of ion density gradient ($\boldsymbol {\nabla } n_i$) and velocity gradient ($\boldsymbol {\nabla } v_i$) (Chai & Bellan Reference Chai and Bellan2016):

(2.15)\begin{equation} \boldsymbol{\nabla} \times \boldsymbol{F_i} = G\boldsymbol{\nabla} v_i \times \boldsymbol{\nabla} n_i, \end{equation}

where $v_i$ and $n_i$ are the ion drift velocity and density, respectively. Parameter $G$ depends on the grain potential, the radius of the dust particles, the ion density and the ambipolar diffusion coefficient (Chai & Bellan Reference Chai and Bellan2016). The finite curl of ion drag force on dust grains ($\boldsymbol {\nabla } \times \boldsymbol {F_i} \neq 0$) is possible if the gradient of $v_i$ is not parallel to the gradient of $n_i$. It should be noted that the formulation (expression) of $\boldsymbol {\nabla } \times \boldsymbol {F_i}$ could be slightly different for different dusty plasma systems, but a finite value of $\boldsymbol {\nabla } \times \boldsymbol {F_i}$ can set the dust grains into rotational motion, resulting in the formation of vortices or coherent structures in the dust cloud.

We consider a free energy source, $\boldsymbol {\nabla } Q_d \times \boldsymbol {E}$, that can excite the vortex motion of dust particles. The spatial dependence of dust-grain charge in a dusty plasma system can convert the potential energy of the electric field into the kinetic energy of dust particles (Vaulina et al. Reference Vaulina, Nefedov, Petrov and Fortov2000, Reference Vaulina, Samarian, Petrov, James and Melandso2004). The presence of a dust charge gradient ($\boldsymbol {\nabla } Q_d$) in the dust–plasma system could be due to non-uniform charging mechanisms because of the inhomogeneity in plasma density and temperature, dispersion of the shape and size of dust grains, etc.

Apart from the fluid description, the onset of vortex motion due to spatial dependence of dust charge in the presence of non-electrostatic force $\boldsymbol {F}_{{\rm non}}$ such as gravitational force ($\boldsymbol {F}_g$) or ion drag force ($\boldsymbol {F}_i$) can be explained by considering a dust system of finite particles having spatial charge dependence (Vaulina et al. Reference Vaulina, Nefedov, Petrov and Fortov2000, Reference Vaulina, Samarian, Petrov, James and Fortov2003). In the presence of a free energy source, the dust particles in a dust cloud start to move in the direction of $F_{{\rm non}}$ where the dust particles have their maximum charge value and form a stable vortex structure. In figure 1(b), a schematic representation of dust rotation in a 2-D plane in the presence of a dust charge gradient and orthogonal non-electrostatic forces is displayed. The frequency ($\omega$) of the steady-state rotation of particles in a vortex structure can be estimated by the formula (Vaulina et al. Reference Vaulina, Nefedov, Petrov and Fortov2000, Reference Vaulina, Samarian, James, Vladimirov and Cramer2001a, Reference Vaulina, Samarian, Petrov, James and Melandso2004)

(2.16)\begin{equation} \omega = \left|\frac{F_{{\rm non}}}{M_d} \frac{\beta}{e Z_0 \nu_{dn}} \right|, \end{equation}

where $\boldsymbol {\beta } = \boldsymbol {\nabla } Q_d = e\boldsymbol {\nabla } Z_d$, $Z_0 = Q_{d0}/e$ is the charge on the dust particle at an equilibrium position in the rotating plane and $\nu _{dn}$ is the dust–neutral collision frequency.

It should be noted that the discussed theoretical models (§ 2) help to explore the driving mechanism for vortex formation in finite dusty plasma systems where the boundary and continuity are dominant effects. Therefore, such a theoretical description may not be of help in understanding the driving mechanism of vortex formation in extended dusty plasma systems.

The vortices in dusty plasmas can also arise due to instabilities such as Kelvin–Helmholtz (KH) instability, Rayleigh–Taylor (RT) instability, dust acoustic wave instability, etc. The RT instability is a buoyancy-driven fluid instability that occurs in the presence of gravitational acceleration ($g$). Whenever a light fluid or dusty plasma supports a heavy fluid or dusty plasma (high mass density) in the presence of gravity and a perturbation occurs at the boundary separating both fluids (Sen, Fukuyama & Honary Reference Sen, Fukuyama and Honary2010; Das & Kaw Reference Das and Kaw2014; Avinash & Sen Reference Avinash and Sen2015), the perturbation grows with time and long-lived mushroom-like vortex structures are formed (Banerjee Reference Banerjee2020; Wani et al. Reference Wani, Mir, Batool and Tiwari2022). A single-fluid description of a dusty plasma helps in formulating the growth rate of RT instability. The stability of a dust–plasma system, in either a strongly coupled or weakly coupled state, can be understood by the dispersion relation. We consider a strongly coupled inhomogeneous 2-D dusty plasma (in the $X$–$Y$ plane), as shown in figure 2(a), where dust density increases with height (along the $y$ direction, which is opposite to $\boldsymbol {g}$) in comparison with the perturbation scale length. The dispersion relation for such a dusty plasma system is (Das & Kaw Reference Das and Kaw2014; Avinash & Sen Reference Avinash and Sen2015)

(2.17)\begin{equation} \omega^2 = \frac{\eta}{\tau_m} k^2 - \frac{g}{\rho_{mo}} \frac{{\rm d}\rho_{m0}}{{\rm d} y} \frac{k^2_x}{k^2}, \end{equation}

where $k_x$ is a perturbation length scale along the $x$ axis, $\rho _{m0}$ is the mass density of the fluid (dusty plasma) and $\eta$ and $\tau _m$ characterize the nature of the dusty plasma. If $\eta \rightarrow 0$ and $\tau _m \rightarrow$ 0 then the dusty plasma is considered as a simple hydrodynamic fluid (weakly coupled state). For the RT unstable dusty plasma system, the gradient in mass density or dust density gradient should be opposite to gravity, i.e. ${{\rm d}\rho _{m0}}/{{\rm d} y} > 0$ (as per figure 2). The growth rate strongly depends on the strength of the density gradient opposite to the gravitational force acting on the fluid/dust-grain medium. The value of the ratio ${\eta }/{\tau _m} = {p_d \varGamma }/{\rho _{mo}}$ demonstrates that the growth rate of RT instability reduces with increasing coupling strength ($\varGamma$) amongst dust grains.

Figure 2.

A schematic diagram of 2-D fluid (dusty plasma) having (a) inhomogeneous density variation opposite to the gravitational force and (b) sharp density variation at the separating boundary of two fluids of different densities/mass densities. The arrows indicate the direction of the flow of fluids during the evolution of RT instability.

If there is a sharp boundary separating two fluids of different densities ($\rho _{m1}$ and $\rho _{m2}$) as shown in figure 2(b), then the dispersion relation is (Avinash & Sen Reference Avinash and Sen2015)

(2.18)\begin{equation} \omega^2 = \frac{\eta}{\tau_m} k^2 - g k \left(\frac{\rho_{m2}-\rho_{m1}}{\rho_{m1} + \rho_{m2}}\right ). \end{equation}

In this case, the growth rate of RT instability depends on the wavelength of the initial perturbation ($k^{-1}$) as well as the coupling effects. The perturbation grows rapidly for shorter wavelength. It should be noted that the occurrence of RT instability in either case of dust–plasma system is possible above a critical wavenumber or initial perturbation wavelength (Avinash & Sen Reference Avinash and Sen2015).

The KH instability occurs at the interface of two fluids flowing with different velocities (Banerjee, Janaki & Chakrabarti Reference Banerjee, Janaki and Chakrabarti2012; Johnson, Wing & Delamere Reference Johnson, Wing and Delamere2014). Such shear flow can lead to the generation of vortices, which is a result of the nonlinear stage of the KH instability. As per the schematic diagram in figure 3, two dust-grain mediums (fluids) of different mass densities ($\rho _{01}$ and $\rho _{02}$) have a continuous velocity shear in the $Y$ direction at the boundary of medium (fluid), while flowing in either horizontal direction (${\pm }X$). A set of singly charged fluid equations are solved using the linear stability analysis technique along with some boundary conditions and initial values (incompressible perturbation, variation of perturbed quantities along the $y$ axis) (Krall & Trivelpiece Reference Krall and Trivelpiece1986; Dolai & Prajapati Reference Dolai and Prajapati2022). The dispersion relation is

(2.19)\begin{equation} \omega = k_x (\alpha_1 U_1 + \alpha_2 U_2) \pm \sqrt{-k^2_x \alpha_1 \alpha_2 (U_1 -U_2)^2}, \end{equation}

where $\alpha _1 = {\rho _{01}}/({\rho _{01} + \rho _{02}})$, $\alpha _2 = {\rho _{02}}/({\rho _{01} + \rho _{02}})$ and $k_x$ is the length scale of the perturbation. Velocities $U_1$ and $U_2$ are the equilibrium flow velocities of the charged fluid (dusty plasma) in $Y>0$ and $Y<0$ regions, respectively, as per the schematic representation in figure 3.

Figure 3.

A schematic diagram of 2-D fluid flow geometry for KH instability. (a) Fluids flowing in the same direction but a finite shear in the velocity at the boundary separating both flowing fluids. (b) Fluids flowing in opposite directions with a finite shear in the velocity at the boundary separating both flowing fluids. The length and direction of the arrows indicate the magnitude of equilibrium flow velocity and direction of flow, respectively. The dotted curve represents a small linear perturbation at the interface of either flowing fluid.

In most dusty plasma experiments, $\rho _{01} = \rho _{02}$; therefore, the dispersion relation will be

(2.20)\begin{equation} \omega = \frac{k_x}{2} (U_1 + U_2) \pm {\rm i}\, \frac{k_x}{2} (U_1 -U_2). \end{equation}

If $\omega$ is real, then the linear perturbation at the interface (see figure 3) will not grow with time, as it makes the dusty plasma a stable system. This is the case when there is no shear in the transverse direction at the separating boundary, i.e. $U_1 = U_2$. The dusty plasma system is KH unstable if $\omega$ is an imaginary or complex quantity. This is only possible when there is a finite velocity difference or shear in the velocity $(U_1 - U_2 \neq 0)$ at the boundary. Once shear velocity $(U_1 - U_2)$ crosses a critical velocity, either the thermal speed or phase velocity of a dusty acoustic wave, instability starts to grow at the interface. Since the vorticity is non-zero ($\boldsymbol {\nabla } \times \boldsymbol {v_d}$) due to the discontinuity in velocity at the interface, it induces rotational velocity that can amplify the instability growth. As a result of this instability, vortex rolls or vortices are formed at the interface of the flowing dust-grain mediums (hydrodynamic fluids).

It should be noted that the growth rate of KH instability strongly depends on the compressibility in the dusty plasma (compressible dust perturbation). Therefore, the characteristics of vortex structures (shape and size) may become changed while incorporating the compressibility effect of the medium (Tiwari et al. Reference Tiwari, Das, Kaw and Sen2012d). When the dusty plasma is in the strongly coupled state, its elastic nature also alters the characteristics of coherent or vortical structures (Tiwari et al. Reference Tiwari, Das, Angom, Patel and Kaw2012a).

In a dusty plasma, dust-acoustic instability also plays a role in exciting the acoustic wave modes and vortex modes. Such instability arises due to the streaming of plasma ions and neutrals relative to the charged dust particles. The streaming plasma ions/neutrals are assumed to be the free energy sources for the charged dust component against the frictional losses due to the ion–neutral and dust–neutral collisions. The growth of the dust-acoustic instability in dusty plasma experiments (moderate collisional dusty plasma) is possible above a threshold electric field and increases with the electric field in the dusty plasma. However, the ion–neutral and dust–neutral collisions reduce the growth rate of the instability (Rosenberg Reference Rosenberg1993; Merlino Reference Merlino1997; Winske & Rosenberg Reference Winske and Rosenberg1998; Salimullah & Morfill Reference Salimullah and Morfill1999). Such low-frequency dust-acoustic instabilities (Rosenberg Reference Rosenberg1993; Salimullah & Morfill Reference Salimullah and Morfill1999) can lead to the formation of vortices (Tsai & Lin Reference Tsai and Lin2014) as the dust plasma system seeks to attain a more stable equilibrium state.

In the presence of an external magnetic field, the dust rotation can be induced by two mechanisms. In the first case, the magnetic field either modifies the existing ion drag gradient and/or dust charge gradient value or induces them by altering the dust-charging processes or confining potential distribution. Section 3 discusses the role of ion drag gradient and dust charge gradient along with electric field in establishing the vortex motion of the dust-grain medium (Choudhary et al. Reference Choudhary, Bergert, Mitic and Thoma2020c).

In the second case, the $\boldsymbol {E}\times \boldsymbol {B}$ drift of plasma particles (mostly ions) in the presence of an external magnetic field sets the dust particles into rotational motion. The schematic diagram in figure 4 represents the direction of ion drag or electric field in a cylindrical geometry where an additional ring against the dust–dust repulsive forces confines dust grains. The ions have radial as well $z$ component of velocities in the cylindrical geometry (see figure 4b). In the presence of magnetic field, the path of the motion of ions (electrons) is changed from radial to azimuthal direction or in the $\boldsymbol {E}\times \boldsymbol {B}$ direction. These $\boldsymbol {E}\times \boldsymbol {B}$ drifted ions (electrons) or neutrals transfer the momentum to dust grains and set them into rotational motion in the plane perpendicular to the magnetic field (Konopka et al. Reference Konopka, Samsonov, Ivlev, Goree, Steinberg and Morfill2000; Kaw, Nishikawa & Sato Reference Kaw, Nishikawa and Sato2002). The dust grains rotating about a particular axis form the vortical structures/vortices.

Figure 4.

A schematic diagram of 2-D dusty plasma in (a) horizontal plane ($X$–$Y$ plane) and (b) vertical plane ($X$–$Z$ plane) in the presence of anexternal magnetic field ($\boldsymbol {B}$). The arrows indicate the direction of the dust forces/motion in the given plane.

2.3 Boundary conditions and vortices

The presence (absence) of boundary layers and the nature of boundary conditions (no slip, partial slip and perfect slip) play a crucial role in determining the dynamics of vortex formation in hydrodynamic fluid flows. A schematic representation of boundary conditions (no slip, partial slip and perfect slip) is depicted in figure 5. These boundary conditions affect the distribution of vorticity, the development of shear layers and, ultimately, the formation and evolution of vortices in the flow field (Sano Reference Sano2015; Vasconcelos & Moura Reference Vasconcelos and Moura2017). The velocity gradient or shear in flowing fluid around the boundary/surface of an object, which arises due to the non-slip or partial-slip boundary (see figure 5), determines the strength of shear stress in the tangential direction of flow. The boundary layer thickness (see figure 5) depends on various factors such as the medium's viscosity, compressibility, velocity of flowing fluid, mass density of fluid, pressure force, etc. If pressure decreases in the direction of fluid flow, the flow is accelerated. This results in a decrease in the boundary layer's thickness in the flow direction. However, the thickness of the boundary layer increases in the flow direction if pressure increases in the direction of fluid flow. In this case, the boundary layer gets separated from the surface of the body, and counter-rotating vortices are formed in the downstream flow or wake region of the object. The thickness of the boundary layer is predicted by the Reynolds number (Fornberg Reference Fornberg1980; Sano Reference Sano2015), which is a ratio of the inertial forces to viscous forces in the boundary layer. No flow separation occurs at a low value of the Reynolds number, formation of steady vortices or a vortex street is possible at an intermediate range of Reynolds number and flow becomes turbulent at a higher value of the Reynolds number (Fornberg Reference Fornberg1980; Thom & Taylor Reference Thom and Taylor1933; Sato & Kobayashi Reference Sato and Kobayashi2012).

Figure 5.

A schematic diagram representing boundary conditions for hydrodynamic fluid (liquid or gas) flowing over a solid surface. Length $L_s$ is the slip length, $u_s$ is the velocity at the surface and $u$ is a constant flow velocity. The boundary layer is very thin or negligible in the perfect slip case.

In the flowing dusty plasma, the boundary layer or Reynolds number has an effective role in the flow characteristics around the virtual boundary (potential barrier) of an object or void or confining electrode (Morfill et al. Reference Morfill, Rubin-Zuzic, Rothermel, Ivlev, Klumov, Thomas, Konopka and Steinberg2004). A typical schematic diagram to understand the physical and potential boundary (or virtual boundary) is shown in figure 6. The magnitude of dust-flow velocity or value of Reynolds number around the potential boundary (in the boundary layer) of the object/void determines the flow characteristics (laminar or turbulent) and vortex formation in the wake region of the obstacle. The existence of velocity gradient in the tangential direction (shear stress) of dust flow (as per the schematic diagram in figure 6) due to the no-slip or partial-slip boundary conditions is responsible for the formation of stable vortices and vortex street in the wake region (Morfill et al. Reference Morfill, Rubin-Zuzic, Rothermel, Ivlev, Klumov, Thomas, Konopka and Steinberg2004; Charan & Ganesh Reference Charan and Ganesh2016). However, there is a velocity or Reynolds number range that favours vortex formation in the wake region of the object (Feng, Goree & Liu Reference Feng, Goree and Liu2012; Bailung et al. Reference Bailung, Chutia, Deka, Boruah, Sharma, Kumar, Chutia, Nakamura and Bailung2020; Bandyopadhyay & Sen Reference Bandyopadhyay and Sen2022).

Figure 6.

A schematic diagram of dusty plasma flow around a solid surface. (a) No slip and (b) partial slip. The potential boundary is separating the plasma and dust-grain medium. Length $L_p$ is the length of the plasma column or sheath dimension or void dimension over the solid surface.

In a bounded dusty plasma, dust grains are confined in an electrostatic potential well created by the biased and floating electrodes/surfaces. The rotating charged dust grains (as per figure 4) do not experience any drag/friction force due to the physical boundaries (surfaces/electrodes). However, the potential boundary could have a finite role in the flow characteristics of the dust-grain medium. In such bounded systems, studying the boundary conditions on the vortex motion/flow is challenging because of the potential boundaries rather than physical boundaries (see figure 6). The potential boundaries are expected to shift or modify on tuning the plasma parameters. If one changes the potential boundaries, the dynamics becomes altered in response. This is possible because of the change in dust parameters (charge, forces) associated with the ambient plasma parameters. Therefore, an explicit role of boundaries in the dynamical dust structures in most dusty plasma experiments (bounded systems) has not been explored.

3.1 External object and force-induced vortices

Past study suggests that the vortex motion of charged particles can be excited by introducing external perturbation with the help of a floating or charged object (rod/probe) in a dusty plasma. The origin of counter-rotating vortices due to a non-uniform field around a biased probe (metal wire), which is shown in figure 7, is reported by Law et al. (Reference Law, Steel, Annaratone and Allen1998). The dust vortex motion in vertical and horizontal planes was also observed in the presence of an external metal electrode in a planar RF discharge (Samarian et al. Reference Samarian, Vaulina, Tsang and James2002). The dissipative instability induced by the dust charge gradient and orthogonal non-electrostatic force was considered as the primary source of vortex formation. Uchida et al. (Reference Uchida, Iizuka, Kamimura and Sato2009) observed 2-D dust vortex flow in a DC discharge near the edge of a negatively biased metal plate introduced externally above the dust-levitating electrode. The numerical calculations conclude that asymmetric ion drag force due to the alteration of the potential distribution of confined dust grains in the presence of the biased metal plate plays a dominant role in forming these symmetric dust vortices. The experimental study by Yan et al. (Reference Yan, Feng, Liu and He2017) suggests that the vortex motion of dust grains can be set up with a modification in confinement electrostatic potential using an insulator saw structure above the conducting lower RF-powered electrode. The asymmetry of the saw-teeth gives rise to a non-zero curl of the total forces ($\boldsymbol {\nabla } \times \boldsymbol {F} \neq 0$) acting on dust particles, which is required for vortex formation. Dai et al. (Reference Dai, Song, Guo, Sun, Guo, Liu and He2020) reported vortex formation in an unmagnetized dusty plasma using a metal saw electrode instead of a disc-shaped planar-powered electrode. The asymmetry in the azimuthal direction, along with the sheath electric field and ion drag, was assumed to be the leading cause of vortex motion in such a configuration. There is also the possibility of generating rotational vortices in co-generated dusty plasma without a saw-like electrode (Mondal et al. Reference Mondal, Sarkar, Mukherjee and Bose2018). The recent experimental work of Bailung et al. (Reference Bailung, Chutia, Deka, Boruah, Sharma, Kumar, Chutia, Nakamura and Bailung2020) suggests that a pair of counter-rotating vortices can be formed in the wake region behind a stationary obstacle (a metal object) in a flowing dusty plasma medium. Images of vortices past an obstacle in a strongly coupled dust-flowing medium are shown in figure 8. They verified the role of the Reynolds number in the formation of vortices behind the obstacle in the wake region.

Figure 7.

Eighteen overlapping video frames, side views, major ticks 2 mm. During experiments, an RF voltage of 90 V (peak-to-peak) at a pressure of 0.5 Torr was fixed. The probe (wire) was biased at 30 V. Three images (i)–(iii) were taken at different heights (8, 7 and 6 mm) of the probe (white circle in image) from the lower electrode. The biased-probe-induced vortex structures are clearly visible in these images. Reproduced with permission from Phys. Rev. Lett., vol. 80, 1998, pp. 4189–4192. Copyright 1998 American Physical Society.

Figure 8.

Particle image velocimetry images of dust-grain medium at different times: (a) 0.63–0.72 s, (b) 0.73–0.82 s and (c) 1.13–1.22 s. The dusty plasma was produced in a low-power ($P = 5\,{\rm W}$) RF (13.56 MHz) discharge at an argon pressure of $10^{-2}$ mbar. Monodispersed silica particles of size $5\pm 0.1\,\mathrm {\mu }{\rm m}$ were used in these experiments. The colour bar shows the value of vorticity in $S^{-1}$. The vector-less region in images is the location of an obstacle (probe). The dust vortices past the obstacle in the wake region can be identified in the displayed images. Reproduced from Phys. Plasmas, vol. 27, 2020, 123702, with the permission of AIP Publishing.

It is possible to modify the dynamical properties of a 2-D equilibrium dust-grain medium by exerting an external radiation pressure force on the dust grains with the help of laser manipulation (Feng et al. Reference Feng, Goree and Liu2012; Melzer et al. Reference Melzer, Schella, Schablinski, Block and Piel2012). The dynamical stability of a 2-D dust cluster with a finite number of dust particles under the action of external torque was investigated in the laboratory by Klindworth et al. (Reference Klindworth, Melzer, Piel and Schweigert2000). Two opposing laser beams were used to create a torque between dust layers by using the concept of radiation pressure. They observed that the whole dust cluster rotates as a solid at low laser torque, but intershell rotation is possible at higher laser torque. A Monte Carlo simulation includes the non-ideal effects to understand the intershell rotation by external laser torque. A recent experimental investigation demonstrates that an energetic electron beam (8–10 keV) can exert a torque on charged particles. The dust particles in a cluster experience torque which is a result of electron drag (Ticoş et al. Reference Ticoş, Scurtu, Williams, Scott, Thomas, Sanford and Ticoş2021). In a large dust cluster (2-D dust crystal), a pair of vortices on either side of the electron beam direction are formed with the passing of it through the dust-grain medium (Ticoş et al. Reference Ticoş, Constantin, Mitu, Scurtu and Ticoş2023). A particle image velocimetry image of the electron-beam-induced vortices is depicted in figure 9.

Figure 9.

Particle image velocimetry image of electron-beam-induced dust flow forming two symmetric vortices relative to the irradiation direction. The streamlines show the geometry of the flow, while the flow speed is inferred from the colour bar. The electron beam of variable acceleration voltage or energy (10–14 keV) is produced in high vacuum ($10^{-4}$ Torr), while the dusty plasma crystal is produced at high pressure ($10^{-1}$ Torr) in a capacitively coupled RF (13.56 MHz) discharge. From Ticoş et al., Sci. Rep., vol. 13, 2023, 940; licensed under a Creative Commons Attribution (CC BY) licence.

3.2 Ion-drag-induced vortex structures

It has been experimentally demonstrated that a dust-grain medium exhibits vortex flow, as depicted in figure 10, in RF discharge under microgravity conditions (Morfill et al. Reference Morfill, Thomas, Konopka, Rothermel, Zuzic, Ivlev and Goree1999). The origin of vortex structures observed in microgravity dusty plasma experiments was explained by considering the combined role of ion drag force, electric force and screened Coulomb force acting on the dust particles (Akdim & Goedheer Reference Akdim and Goedheer2003; Goedheer & Akdim Reference Goedheer and Akdim2003; Bockwoldt et al. Reference Bockwoldt, Arp, Menzel and Piel2014) as discussed in § 2.2. In a novel ice dusty plasma experiment, Chai & Bellan (Reference Chai and Bellan2016) observed the vortex motion of charged ice particles created in a device by cooling down water vapour in a controlled manner. The non-conservative nature of ion drag force due to the non-parallel ion density gradient and ion drift velocity gradient (see figure 11) acting on charged ice particles set them into vortex motion. Kaur et al. (Reference Kaur, Bose, Chattopadhyay, Sharma, Ghosh and Saxena2015a,Reference Kaur, Bose, Chattopadhyay, Sharma, Ghosh, Saxena and Thomasb) have observed dust vortices (in a 2-D plane) in the poloidal plane of a toroidal geometry in a DC discharge configuration. The experimental estimation of forces acting on dust grains in the plasma background confirms the role of the non-conservative nature of the ion drag force in driving vortex motion. The experimental study of Mulsow, Himpel & Melzer (Reference Mulsow, Himpel and Melzer2017) explored the motion of dust grains in a cluster having 50–1000 particles using three-dimensional (3-D) diagnostic techniques (stereoscopy). It was observed that dust grains exhibit vortex motion in a poloidal plane when more particles are added to the cluster. The quantitative analysis confirmed the role of the radial gradient of ion drag force in exciting the vortex flow in the dust-grain medium. Vladimirov et al. (Reference Vladimirov, Deputatova, Nefedov, Fortov, Rykov and Khudyakov2001) reported vortex structures with a large number of dust particles in a nuclear-induced dusty plasma system. It was suggested that the motion of ions in the external electric field set dust particles into vortex rotation through an ion–dust momentum transfer mechanism. A ground-based laboratory experiment with the concept of thermophoretic force against gravity on dust particles by Morfill et al. (Reference Morfill, Rubin-Zuzic, Rothermel, Ivlev, Klumov, Thomas, Konopka and Steinberg2004) confirmed the vortex flow in the wake region of an obstacle (here void) in the flowing dusty plasma. To understand the onset and characteristics of vortices around a void in the dust-grain system under microgravity conditions, Schwabe et al. (Reference Schwabe, Zhdanov, Räth, Graves, Thomas and Morfill2014) conducted a detailed numerical simulation of the 2-D dusty plasma system. The addition of extra dust particles to the equilibrium 2-D dusty plasma medium makes it unstable, and vortices are formed around the void due to the non-zero curl of the combined ion drag and electric forces acting on particles. A vast analytical and numerical study on the origin of vortex structures in dusty plasma fluid was done by Laishram, Sharma & Kaw (Reference Laishram, Sharma and Kaw2014), Laishram & Zhu (Reference Laishram and Zhu2018), Laishram, Sharma & Kaw (Reference Laishram, Sharma and Kaw2015), Laishram et al. (Reference Laishram, Sharma, Chattopdhyay and Kaw2017, Reference Laishram, Sharma, Chattopdhyay and Kaw2018) and Laishram, Sharma & Zhu (Reference Laishram, Sharma and Zhu2020) using 2-D hydrodynamics modelling. The authors explored the role of ion shear flow, nonlinearity, boundary conditions and viscosity of the medium in generating a self-organized vortex or coherent structures in the 2-D dusty plasma medium. Their study also predicts the formation of multiple co-rotating vortices in the extended 2-D dusty plasma medium. In a recent experimental study, Scurtu et al. (Reference Scurtu, Ticoş, Mitu, Udrea and Ticoş2023) have observed the stretching and compression of vortices in a CO$_2$ RF discharge dusty plasma and discussed the results based on ion drag force as discussed in § 2.2.

Figure 10.

Cross-sectional view through the colloidal plasma condensation in microgravity (TEXUS 35 rocket flight). The RF power was 0.075 W, and 150 video images with a total exposure of 1.0 s were combined and colour-coded, thus tracing the particle trajectories (beginning with ‘red’). In the inset, the original video image is shown. Reproduced with permission from Phys. Rev. Lett., vol. 83, 1999, pp. 1598–1601. Copyright 1999 American Physical Society.

Figure 11.

(a) Contour plots of $u_i$ (dashed lines) and $n_i/n_{i0}$ (solid lines). (b) Contour plot of ($\boldsymbol {\nabla } \times F$). (c) Flow velocity $u_d$ obtained from a numerical partial differential equation solver. Reproduced from Phys. Plasmas, vol. 23, 2016, 023701, with the permission of AIP Publishing.

3.3 Dust-charge-gradient-induced vortices

The self-excited dynamical structures (vortices) in a dusty plasma system having an inhomogeneous plasma background were explored by Vaulina et al. (Reference Vaulina, Nefedov, Petrov and Fortov2000, Reference Vaulina, Samarian, James, Vladimirov and Cramer2001a,Reference Vaulina, Samarian, Nefedov and Fortovb, Reference Vaulina, Samarian, Petrov, James and Fortov2003, Reference Vaulina, Samarian, Petrov, James and Melandso2004). The role of dust charge gradient along with orthogonal non-electrostatic force such as gravitational or ion drag force in such a dissipative dusty plasma medium in the formation of vortices was discussed in § 2.2. A typical dust vortex flow pattern in the presence of dust charge gradient ($\beta _r$) along with gravitational force ($mg$) is presented in figure 12. The mathematical model provided in § 2.2 had helped to explain the experimentally observed dust vortices in a planar RF discharge dusty plasma (Vaulina et al. Reference Vaulina, Samarian, Nefedov and Fortov2001b; Samarian et al. Reference Samarian, Vaulina, Tsang and James2002). Agarwal & Prasad (Reference Agarwal and Prasad2003) observed the rotating structures (vortices) in a DC discharge strongly coupled dusty plasma without any external metal electrode. The vortex flow in such a dissipative dusty medium was understood with the help of the theoretical model provided in § 2.2. Ratynskaia et al. (Reference Ratynskaia, Rypdal, Knapek, Khrapak, Milovanov, Ivlev, Rasmussen and Morfill2006) performed an experimental study of dust grains in a 2-D monolayer complex plasma and reported a wide range of vortical flows or structures. One of the causes for the formation of large-scale vortices in the 2-D complex plasma was assumed to be charge inhomogeneity across the dust layer. A recent experimental study by Choudhary, Mukherjee & Bandyopadhyay (Reference Choudhary, Mukherjee and Bandyopadhyay2017) and Choudhary et al. (Reference Choudhary, Mukherjee and Bandyopadhyay2018) has confirmed the dust charge gradient along with ion drag force or gravity as a driving force to excite the vortex motion against dissipative losses in a dusty plasma medium. In this work, a novel experimental configuration using an inductively coupled discharge was proposed to create a large-aspect-ratio dusty plasma with an inhomogeneous plasma background that can accommodate multiple self-sustained vortex structures (Choudhary et al. Reference Choudhary, Mukherjee and Bandyopadhyay2017, Reference Choudhary, Mukherjee and Bandyopadhyay2018) as shown in figure 13.

Figure 12.

Examples of dust vortex motion (trajectories of particles) obtained from numerical simulations for different parameters (given in the original article). Here $\beta _r$ represents the dust charge gradient direction from the centre of the dust cloud, and $mg$ is the gravitationalforce acting on particles. The direction of $\beta _r$ decides the direction of vortex flow. Reproduced with permission from New J. Phys., vol. 5, 2003, pp. 82.1–82.20. Copyright 2003 Institute of Physics (IOP). CC BY-NC-SA.

Figure 13.

Video images of a dust cloud in the $X$–$Y$ plane. All images are obtained by superposing five consecutive images at a time interval of 66 ms. The vortex structures were observed at (a–c) different input RF powers. Yellow solid lines with arrows indicate the direction of the vortex motion of dust grains, and the dashed line corresponds to the axis of the dust cloud. Reproduced from Phys. Plasmas, vol. 24, 2017, 033703, with the permission of AIP Publishing.

3.4 Neutral-drag-driven vortex structures

Mitic et al. (Reference Mitic, Sütterlin, Höfner, Thoma, Zhdanov and Morfill2008) observed for the first time vortex structures (see figure 14) in a dust-grain medium confined in a vertical glass tube due to the thermal creep of background atoms/molecules. In their study, the gas flow driven by thermal creep was anti-parallel to gravity. The background gas atoms driven by thermal creep exert a drag force on dust grains, forming vortices in the dust-grain medium (Schwabe et al. Reference Schwabe, Hou, Zhdanov, Ivlev, Thomas and Morfill2010). The experimental study by Flanagan & Goree (Reference Flanagan and Goree2009) also demonstrated the role of thermal creep flow in setting dust grains into rotational motion. The temperature gradient along a surface in contact with a low-pressure gas creates thermal creep flow, resulting in the formation of 2-D vortex flow due to the easy response of dust particles with ambient gas flow. A recent experimental study under microgravity conditions (Schmitz et al. Reference Schmitz, Schulz, Kretschmer and Thoma2023) also confirms the role of thermal creep in driving the dust grains into rotational motion, resulting in counter-rotating vortices. It has been reported (Kählert et al. Reference Kählert, Carstensen, Bonitz, Löwen, Greiner and Piel2012) that frictional coupling between dust particles and background neutral gas can be used to realize the magnetization of massive charged dust particles. The dust grains behave in a way that is equivalent to being magnetized in the absence of an external magnetic field. The directed flow (rotational flow) of background gas sets dust grains into rotational motion through momentum transfer mechanisms (Kählert et al. Reference Kählert, Carstensen, Bonitz, Löwen, Greiner and Piel2012). If sufficient dust grains are used in the experiment, dust vortices are expected to form in a strongly coupled dusty plasma medium by rotating neutral gas. The role of frictional coupling of dust particles with background neutrals in exciting the large-scale shear modes such as vortices or intershell rotations in Yukawa balls (dusty plasma balls) was explored experimentally by Ivanov & Melzer (Reference Ivanov and Melzer2009). They used singular value decomposition and normal mode analysis to explore the dynamical features of Yukawa balls. Their analysis predicted various modes, but large-scale vortices and intershell rotations were the dominant ones. In computer experiments, it is possible to create a temperature difference between charged dust layers and study the effect of temperature gradient on dust dynamics. With this objective, Charan & Ganesh (Reference Charan and Ganesh2015) performed a molecular dynamics (MD) simulations of a strongly coupled dusty plasma with a temperature difference between charged dust layers and observed the vortex flow.

Figure 14.

Averaged gas flow velocity field (vectors) superimposed with particle trajectories. The vertical dashed line indicates the centre of the tube. Reproduced with permission from Phys. Rev. Lett., vol. 101, 2008, 235001. Copyright 2008 American Physical Society.

3.5 Instability-induced vortices

The role of various instabilities in exciting vortices in finite or extended dusty plasma systems has been discussed in § 2.2. Veeresha, Das & Sen (Reference Veeresha, Das and Sen2005) demonstrated the RT-instability-driven flow patterns or vortices in a dusty plasma. These vortex structures or modes were observed in the saturation state of the RT instability. The numerical work of Chakrabarti & Kaw (Reference Chakrabarti and Kaw1996) also confirmed that the nonlinear evolution of RT instabilities can form coherent vortex structures in dusty plasmas. The stability of such coherent vortex structures depends on the strength of short-range secondary instability, which is excited in the core of the vortex (Jun et al. Reference Jun, Yin-Hua, Bao-Xia, Fei-Hu and Dong2006). Recent numerical simulations by Dharodi & Das (Reference Dharodi and Das2021) also observed the vortex-like structure as shown in figure 15 during the time evolution of RT instability in viscoelastic dusty plasma fluid. However, no experimental work has been reported to confirm the RT instabilities that drive coherent vortex structures in dusty plasmas.

Figure 15.

The growth of RT instability at the sharp interface of two viscoelastic fluids (dusty plasma) of different densities: (a–d) $\eta = 0.1$, $\tau _m = 20$; (e–h) $\eta = 0.1$, $\tau _m = 5$. Reproduced with permission from J. Plasma Phys., vol. 87, 2021, 905870216. Copyright 2021 Cambridge University Press.

Another kind of instability that has been studied for a long time in dusty plasmas is KH instability (Banerjee et al. Reference Banerjee, Janaki and Chakrabarti2012). Ashwin & Ganesh (Reference Ashwin and Ganesh2010) performed MD simulations to explore the KH instability in a strongly coupled dusty plasma. Time evolution of KH instability produces vortex roll in the nonlinear regime depicted in figure 16. Numerical and analytical studies of KH instability-driven flow patterns (vortex structures) in the nonlinear regime in weakly as well as strongly coupled dusty plasmas have been conducted by various research groups (Tiwari et al. Reference Tiwari, Das, Kaw and Sen2012c,Reference Tiwari, Das, Angom, Patel and Kawb, Reference Tiwari, Dharodi, Das, Patel and Kaw2014; Das, Dharodi & Tiwari Reference Das, Dharodi and Tiwari2014; Dharodi, Patel & Das Reference Dharodi, Patel and Das2022). The analytical study by Janaki & Chakrabarti (Reference Janaki and Chakrabarti2010) claimed the existence of dipolar vortex structures in a 2-D dusty plasma medium in the presence of sheared dust-grain flow. Gupta & Ganesh (Reference Gupta and Ganesh2018) and Gupta, Ganesh & Joy (Reference Gupta, Ganesh and Joy2018) performed computational fluid dynamics and MD simulations of a dusty plasma medium with Kolmogorov shear flows and observed the coherent vortex structures along with other flow patterns as a result of the sheared-flow-induced instabilities. A recent experimental study by Krishan et al. (Reference Krishan, Bandyopadhyay, Singh, Dharodi and Sen2023) confirmed the KH instability-driven vortex structures in a DC discharge flowing dusty plasma. They generated shear at the interface of the moving and stationary layers of the dust-grain medium that excites the KH instability, and evolution of it gives vortex structures, as is shown in figure 17.

Figure 16.

Blue-coloured fluid moves in the ${+}x$ direction and green-coloured fluid moves in the ${-}x$ direction. Inverse cascading of mode $m_n = 6$ starting from an initial state with a coupling constant of 50. The formation of vortices and their evolution due to KH instability can be seen in the images. Reproduced with permission from Phys. Rev. Lett., vol. 104, 2010, 215003. Copyright 2010 American Physical Society.

Figure 17.

The velocity vector field with the magnitude of the velocity (${\rm cm}\,{\rm s}^{-1}$) for double-layer flow with the input pressure of the pulse valve being 300 Pa. The vortex pattern in the displayed image arises due to the KH instability. From Kumar et al., Sci. Rep., vol. 13, 2023, 3979; licensed under a Creative Commons Attribution (CC BY) licence.

4.1 The ${E}\times {B}$ drift-induced vortex motion

In the presence of an external magnetic field, $\boldsymbol {E}\times \boldsymbol {B}$ drifted ions (electrons) exert force on dust grains and set them into rotational motion (Konopka et al. Reference Konopka, Samsonov, Ivlev, Goree, Steinberg and Morfill2000; Sato et al. Reference Sato, Uchida, Kaneko, Shimizu and Iizuka2001; Kaw et al. Reference Kaw, Nishikawa and Sato2002; Dzlieva et al. Reference Dzlieva, Karasev, Mashek and Pavlov2016; Abdirakhmanov et al. Reference Abdirakhmanov, Moldabekov, Kodanova, Dosbolayev and Ramazanov2019) or background neutral atoms are set into rotation by azimuthal ion flow, and then dust particles start to rotate via this neutral gas flow (Shukla Reference Shukla2002; Carstensen et al. Reference Carstensen, Greiner, Hou, Maurer and Piel2009). The trajectories of the rotating dust grains can be rigid rotation (Reichstein, Pilch & Piel Reference Reichstein, Pilch and Piel2010; Wilms, Reichstein & Piel Reference Wilms, Reichstein and Piel2015) or shear rotation (Konopka et al. Reference Konopka, Samsonov, Ivlev, Goree, Steinberg and Morfill2000; Choudhary et al. Reference Choudhary, Bergert, Moritz, Mitic and Thoma2021) or vortex rotation (Vasiliev et al. Reference Vasiliev, D'Yachkov, Antipov, Huijink, Petrov and Fortov2011; Choudhary et al. Reference Choudhary, Bergert, Mitic and Thoma2020c). Huang et al. (Reference Huang, Ye, Wang and Liu2007) observed the various vortex patterns of dust grains in magnetized dusty plasma experiments (see figure 18) where the external magnetic field was 0.2 T. They observed the gathering and dispersive vortex structures in a 2-D plane after tuning the input RF power. The MD simulation and analysis of forces acting on dust grains confirmed the role of confining electric potential and strong magnetic field in the transition of circular rotating dust particles to vortex structures. To understand dust vortex patterns, Nebbat & Annou (Reference Nebbat and Annou2010, Reference Nebbat and Annou2023) did calculations using a time-dependent nonlinear model for such a dusty plasma system and highlighted the role of magnetized ions having azimuthal velocity component in driving vortex motion. Vasiliev et al. (Reference Vasiliev, D'Yachkov, Antipov, Huijink, Petrov and Fortov2011) presented experimental results on rotating dust structure (vortex) in a horizontal plane of a cylindrical device with DC discharge configuration under the action of a strong magnetic field up to 0.25 T. The rotation of dust grains in the structure was explained by calculating the ion drag force acting on particles against friction force arising due to the background neutrals. In a strong magnetic field ($B > 0.5\,{\rm T}$), dust clusters in the 2-D horizontal plane also exhibit vortex-like motion that was confirmed in an MDPE dusty plasma device (Jaiswal et al. Reference Jaiswal, Hall, LeBlanc, Mukherjee and Thomas2017). Saitou & Ishihara (Reference Saitou and Ishihara2013) studied the dynamics of a dust-grain medium in a strong magnetic field. They observed the transition from horizontal rotational motion to vortex motion in the vertical plane of a cylindrical system once the strength of the external magnetic field is increased. The disturbance of the magnetohydrodynamic equilibrium of the dust-grain medium at a higher value of magnetic field was considered the leading cause of the vortex motion of dust grains in the vertical plane. It should be noted that dust clouds that rotate as a whole at low to moderate magnetic fields in a horizontal plane break up into smaller vortices at high magnetic fields ($B > 1\,{\rm T}$). Schwabe et al. (Reference Schwabe, Konopka, Bandyopadhyay and Morfill2011) performed experiments in a low-pressure dusty plasma and observed small-scale rotating or vortex structures in a 2-D dusty plasma at strong magnetic field ($B > 1\,{\rm T}$). The breaking up of the rotating 2-D dust medium into multiple rotating structures is a result of the plasma filamentation at a strong magnetic field (Schwabe et al. Reference Schwabe, Konopka, Bandyopadhyay and Morfill2011; Thomas et al. Reference Thomas, Lynch, Konopka, Menati, Williams, Merlino and Rosenberg2019).

Figure 18.

Experimental spiral vortex pattern (power = 40–50 W, $p = 120$ Pa). Reproduced with permission from Plasma Sci. Technol., vol. 9, 2007, pp. 11–14. Copyright 2007 IOP Sciences.

4.2 Sheared-flow- and dust-charge-gradient-driven vortices

The analytical study using a fluids model conducted by Bharuthram & Shukla (Reference Bharuthram and Shukla1992) of a non-uniform dusty plasma in the presence of a magnetic field predicted dipolar vortices as a result of the stationary solution of nonlinear equations. Their study demonstrates that shear in ion flow excites low-frequency electrostatic modes, which interact with and give rise to vortex structures in dusty plasma systems. In an external magnetic field, the equilibrium sheared plasma flow or non-uniform plasma is considered a free energy source (as discussed in § 2.2) to excite various linear and nonlinear modes in the medium. The saturation state of nonlinear coupling of excited modes gives various vortex structures such as vortex chain, tripolar vortices (see figure 19) and global vortices in a magnetized dusty plasma system (Vranješ, Petrović & Shukla Reference Vranješ, Petrović and Shukla2001). It is also possible to excite dipolar vortices in a magnetized dusty plasma because of the nonlinear saturation of KH instability (Rawat & Rao Reference Rawat and Rao1993; Shukla & Rao Reference Shukla and Rao1993; Ijaz, Mirza & Azeem Reference Ijaz, Mirza and Azeem2007). The role of the sheared magnetic field that can produce sheared plasma flow perpendicular to the magnetic field in a dusty plasma was examined by Jovanović & Shukla (Reference Jovanović and Shukla2001). The authors observed the formation of dipolar and tripolar vortices depending on the initial plasma density profiles in the non-uniform magnetized dusty plasma.

Figure 19.

The tripolar vortex for given perturbed potential and other parameters (see the original paper (Vranješ et al. Reference Vranješ, Petrović and Shukla2001)). Two lateral vortices have opposite direction of rotation with respect to the central vortex. Reproduced with permission from Phys. Lett. A, vol. 278, 2001, pp. 231–238. Copyright 2001 Elsevier.

Dasgupta & Maitra (Reference Dasgupta and Maitra2021) investigated the dust dynamics numerically in the presence of an external magnetic field and predicted vortices in the dust plasma system by considering the role of dust–dust interactions, dust diffusion and ion drag force in the formation of vortex structures. A recent numerical simulation by Kumar & Sharma (Reference Kumar and Sharma2020) examined the dynamics of a dusty plasma medium in a weakly non-uniform magnetic field. The non-uniformity in the external magnetic field induces $\boldsymbol {E} \times \boldsymbol {B}$ drift flow of plasma particles. The sheared $\boldsymbol {E} \times \boldsymbol {B}$ drift ions play a major role in driving the vortex motion as discussed in § 2.2 in a magnetized dusty plasma system. Laishram (Reference Laishram2021) further extended the study of a dusty plasma in a non-uniform external magnetic field and observed the shear between electrons and ions due to $\boldsymbol {E} \times \boldsymbol {B}$ and $\boldsymbol {\nabla } B \times \boldsymbol {B}$ drifts in the presence of magnetic field. The sheared nature of these drifts was considered as the vorticity source to establish the vortex structures in the dusty plasma. It was also found from numerical investigation that temperature gradient in background ions plays a dominant role in forming vortices in a magnetized dusty plasma (Haque & Saleem Reference Haque and Saleem2006). In recent experimental work, Choudhary et al. (Reference Choudhary, Bergert, Mitic and Thoma2020c) reported the existence of a pair of counter-rotating vortices, as shown in figure 20, in the vertical plane of a 3-D dusty plasma in the presence of a strong magnetic field ($B > 0.05$ T). The vortex structures originating in the dust-grain medium were explained by the combined effect of dust charge gradient and iron drag force gradient along with gravitational force/electric force in the cylindrical system. An analytical work by Shukla & Mamun (Reference Shukla and Mamun2003) reported the electrostatic and electromagnetic vortices in a non-uniform magnetoplasma containing immobile dust grains. The evolution of nonlinear dispersive solitary modes (electrostatic and electromagnetic) explains the origin of dipolar vortices in such dusty plasma systems.

Figure 20.

Video images of a dust cloud (aluminium ring) in the vertical ($Y$–$Z$) plane. Images at different magnetic fields are obtained by a superposition of five consecutive images at a time interval of 65 ms. The edge vortex and central region vortex are represented by V-I and V-II, respectively. The vortex structures at different strengths of the magnetic field are observed at a fixed input RF power, $P = 3.5\,{\rm W}$, and argon pressure, $p = 35$ Pa. The dotted yellow line represents the axis of symmetry. The yellow solid line with an arrow indicates the direction of the vortex flow in the vertical plane of the 3-D dusty plasma. Reproduced from Phys. Plasmas, vol. 27, 2020, 063701, with the permission of AIP Publishing.