2.1 Model of electric charging of the plasma

The model of EMP emission proposed in this paper consists of a phase of plasma charging, followed by a discharge and antenna emission process. Firstly, the plasma is formed, and the charge is lost as hot electrons escape the potential barrier. This charge supplies the electrostatic energy that is later radiated as an EMP. The mechanism of EMP emission, where the plasma is discharged through the nozzle and radiates as a dipole antenna, is similar to the solid-target model already examined in various publications^[ Reference Dubois, Lubrano-Lavaderci, Raffestin, Ribolzi, Gazave, La Fontaine, D’Humières, Hulin, Nicolaï, Poyé and Tikhonchuk^2, Reference Consoli, Tikhonchuk, Bardon, Bradford, Carroll, Cikhardt, Cipriani, Clarke, Cowan, Danson, Angelis, Marco, Dubois, Etchessahar, Garcia, Hillier, Honsa, Jiang, Kmetik, Krasa, Li, Lubrano, McKenna, Poye, Prencipe, Raczka, Smith, Vrana, Woolsey, Zemaityte, Zhang, Zhang, Zielbauer and Neely^3, Reference Poyé, Dubois, Lubrano-Lavaderci, D’Humières, Bardon, Hulin, Bailly-Grandvaux, Ribolzi, Raffestin, Santos, Nicolaï and Tikhonchuk^7, Reference Minenna, Poyé, Bradford, Woolsey and Tikhonchuk^27].

Following the available observations and numerical simulations^[ Reference Debayle, Mollica, Vauzour, Wan, Flacco, Malka, Davoine and Gremillet^28– Reference Willingale, Mangles, Nilson, Clarke, Dangor, Kaluza, Karsch, Lancaster, Mori, Najmudin, Schreiber, Thomas, Wei and Krushelnick^31], we assume that the plasma in the laser channel is fully ionized. The absorbed laser energy ${\eta}_{\mathrm{L}}{E}_{\mathrm{L}}$ is transferred to electrons with an energy distribution approximated by a two-temperature relativistic distribution:

(1) $$\begin{align}{f}_{\mathrm{e}}\left(\gamma \right)={n}_{\mathrm{e}}{f}_{\mathrm{MJ}}\left(\gamma, {\Theta}_{\mathrm{e}}\right)+{n}_{\mathrm{h}}{f}_{\mathrm{MJ}}\left(\gamma, {\Theta}_{\mathrm{h}}\right),\end{align}$$

where ${f}_{\mathrm{MJ}}\left(\gamma, \Theta \right)$ is the Maxwell–Jüttner function^[ Reference Passoni, Bertagna and Zani^32]:

$$\begin{align*}{f}_{\mathrm{e}}\left(\gamma, \Theta \right)=\left(\gamma /\Theta \right)\kern0.1em {K}_2\left(1/\Theta \right)\sqrt{\gamma^2-1}\exp \left(-\gamma /\Theta \right),\end{align*}$$

depending on the dimensionless temperature $\Theta =T/\left({m}_{\mathrm{e}}{c}^2\right)$ , the modified Bessel function $K$ of the second kind and the electron relativistic factor $\gamma =1+\varepsilon /\left({m}_{\mathrm{e}}{c}^2\right)$ . A fraction ${\eta}_{\mathrm{las}\to \mathrm{h}}$ of the absorbed laser energy is transferred to a population of hot electrons with density ${n}_{\mathrm{h}}$ and temperature ${T}_{\mathrm{h}}$ , while the remaining energy goes to electrons in the plasma bulk, with density ${n}_{\mathrm{e}}$ and temperature ${T}_{\mathrm{e}}$ . Here, we use subscripts ‘h’ and ‘e’ to refer to the hot and thermal electron populations, respectively.

The bulk electron density is defined by the gas density ( ${n}_{\mathrm{e}}={Zn}_{\mathrm{at}}$ ) and the bulk temperature is defined by the plasma volume and deposited energy via the following:

(2) $$\begin{align}{C}_{\mathrm{e}}\left({T}_{\mathrm{e}}\right){n}_{\mathrm{e}}{T}_{\mathrm{e}}=\left(1-{\eta}_{\mathrm{las}\to \mathrm{h}}\right){\eta}_{\mathrm{L}}{E}_{\mathrm{L}}/{V}_{\mathrm{p}},\end{align}$$

where ${C}_{\mathrm{e}}\left({T}_{\mathrm{e}}\right)=3-\left[1-{K}_1\left(1/{\Theta}_{\mathrm{e}}\right)/{K}_2\left(1/{\Theta}_{\mathrm{e}}\right)\right]/{\Theta}_{\mathrm{e}}$ is the heat capacitance of a relativistic electron gas.

The hot electron density can then be defined knowing the fraction of energy transferred to hot electrons ${\eta}_{\mathrm{las}\to \mathrm{h}}$ :

$$\begin{align*}{C}_{\mathrm{e}}\left({T}_{\mathrm{h}}\right){n}_{\mathrm{h}}{T}_{\mathrm{h}}={\eta}_{\mathrm{las}\to \mathrm{h}}{\eta}_{\mathrm{L}}{E}_{\mathrm{L}}/{V}_{\mathrm{p}}.\end{align*}$$

The electric potential of the plasma channel is determined by how many hot electrons can overcome the plasma potential barrier. Although electrons from the plasma bulk will also contribute to the ejected charge, their contribution is less than $10\%$ because a significant fraction of the available laser energy is transferred to hot electrons. The electric potential ${\Phi}_{\mathrm{p}}$ at the surface of the plasma cylinder with respect to the grounded nozzle can be estimated as follows:

(3) $$\begin{align}{\Phi}_{\mathrm{p}}=Q/C,\end{align}$$

where $Q$ is the charge of the plasma and $C=2\pi {l}_{\mathrm{p}}{\epsilon}_0/\ln \left(h/{r}_{\mathrm{p}}\right)$ is the capacitance. The capacitance follows from the potential of a charged cylinder, radius ${r}_{\mathrm{p}}$ , length ${l}_{\mathrm{p}}$ , situated a distance $h$ from an infinite conducting plane. Only electrons with energies ${\varepsilon}_{\mathrm{e}}>e{\Phi}_{\mathrm{p}}$ can escape plasma to the ground. Assuming, as mentioned above, that hot electrons have an exponential distribution in energy with a temperature ${T}_{\mathrm{h}}$ , the fraction of escaped hot electrons is as follows^[ Reference Chen^33]:

(4) $$\begin{align}\frac{\delta {n}_{\mathrm{h}}}{n_{\mathrm{h}}}={\int}_{1+\psi}^{\infty } \mathrm{d}\gamma \kern0.1em {f}_{\mathrm{MJ}}\left(\gamma, {\Theta}_{\mathrm{h}}\right),\end{align}$$

where $\psi =e{\Phi}_{\mathrm{p}}/\left({m}_{\mathrm{e}}{c}^2\right)$ is the dimensionless potential. The plasma charge is then $Q= e\delta {n}_{\mathrm{h}}{V}_{\mathrm{p}}$ and, substituting this expression into Equation (3), we have the following equation for the dimensionless potential $\psi$ :

(5) $$\begin{align}\psi =\frac{r_{\mathrm{p}}^2{\omega}_{\mathrm{ph}}^2}{2{c}^2}\kern0.1em \frac{\delta {n}_{\mathrm{h}}}{n_{\mathrm{h}}}\kern0.1em \ln \frac{h}{r_{\mathrm{p}}},\end{align}$$

where ${\omega}_{\mathrm{ph}}={\left({e}^2{n}_{\mathrm{h}}/{m}_{\mathrm{e}}{\varepsilon}_0\right)}^{1/2}$ is the hot electron plasma frequency.

The total energy of escaped electrons is split between the electrostatic energy of the charged plasma ${\mathcal{E}}_{\mathrm{es}}={Q}^2/2C$ and the kinetic energy of the escaped electrons:

(6) $$\begin{align}{\mathcal{E}}_{\mathrm{esc}}={V}_{\mathrm{p}}{n}_{\mathrm{h}}{m}_{\mathrm{e}}{c}^2{\int}_{1+\psi}^{\infty } \mathrm{d}\gamma \kern0.1em \left(\gamma -1\right){f}_{\mathrm{MJ}}\left(\gamma, {\Theta}_{\mathrm{h}}\right).\end{align}$$

2.2 Ion acceleration in the expanding plasma

The number of ions in the laser plasma and their energy are important factors for determining the extent of damage to the gas nozzle, as well as for placing a lower limit on the speed of the plasma discharge. When the expanding thermal ions reach the nozzle surface they deposit their kinetic energy and can cause the nozzle to melt. Contact between the plasma and the nozzle also establishes an electrical path to the ground, triggering a plasma discharge and the emission of EMP radiation.

The ion spectrum can be separated into two broad populations^[ Reference Ospina-Bohórquez, Salgado-López, Ehret, Malko, Salvadori, Pisarczyk, Chodukowski, Rusiniak, Krupka, Guillon, Lendrin, Pérez-Callejo, Vlachos, Hannachi, Tarisien, Consoli, Verona, Prestopino, Dostal, Dudzak, Henares, Apiñaniz, De Luis, Debayle, Caron, Ceccotti, Hernández-Martín, Hernández-Toro, Huault, Martín-López, Méndez, Nguyen-Bui, Perez-Hernández, Vaisseau, Varela, Volpe, Gremillet and Santos^26, Reference Puyuelo-Valdes, Henares, Hannachi, Ceccotti, Domange, Ehret, d’Humieres, Lancia, Marquès, Ribeyre, Santos, Tikhonchuk and Tarisien^34]: (i) thermal ions that expand as part of the laser plasma and (ii) a less numerous population of fast ions accelerated in the charge separation field produced by the escaped hot electrons^[ Reference Debayle, Mollica, Vauzour, Wan, Flacco, Malka, Davoine and Gremillet^28, Reference Sentoku, Liseikina, Esirkepov, Califano, Naumova, Ueshima, Vshivkov, Kato, Mima, Nishihara, Pegoraro and Bulanov^35]. We restrict ourselves to modelling the thermal ions, since they carry most of the energy.

Following a short phase of gas ionization, electron heating and plasma charging, the plasma expands and cools down. After the end of the laser pulse, there is no more energy supply and the plasma expands adiabatically under the electron thermal pressure. The plasma pressure is much higher than the ambient gas pressure, so the plasma expands freely with electrons transferring their energy to ions. The plasma charge is conserved during the expansion phase and the potential decreases logarithmically as the plasma radius increases (see Equation (5)). The plasma expansion can be described in some special cases by a self-similar rarefaction wave model^[ Reference Mora^36, Reference Murakami and Basko^37]. More detailed analysis is performed for a spherical plasma expansion in Ref. [Reference Popov, Bychenkov, Rozmus and Ramunno38]. In practice, the ion energy distribution depends on the density profile and on the ratio of the plasma radius to the Debye length. For our purposes, it is sufficient to estimate the average ion kinetic energy ${\varepsilon}_{\mathrm{i}}$ by equating the ion and electron energy densities, ${n}_{\mathrm{i}}{\varepsilon}_{\mathrm{i}}\simeq {n}_{\mathrm{e}}{\varepsilon}_{\mathrm{e}}\approx \frac{3}{2}{n}_{\mathrm{e}}{T}_{\mathrm{e}}$ , where ${n}_{\mathrm{i}}$ is the ion density in the plasma channel and ${\varepsilon}_{\mathrm{e}}$ is the average electron kinetic energy. The total number of ions in the plasma is ${N}_{\mathrm{i}}={n}_{\mathrm{i}}{V}_{\mathrm{p}}$ .

2.3 Model estimates for Vulcan-TAP conditions

The plasma charging model described in the previous section takes several laser and gas parameters as inputs that must either be experimentally determined or estimated by other means. Input parameters relevant to the experiments considered in this paper are given in Tables 1 and 2, along with the outputs from our model given in Table 3. We use the Vulcan-TAP parameters in Sections 3 and 5 to explore likely mechanisms of gas ionization and nozzle damage. The VEGA-3 parameters are used to benchmark our model against the experiments described in Section 6.

Table 1

Representative input laser parameters – measured or inferred – as described in the text and Refs. [Reference Hicks, Ettlinger, Borghesi, Carroll, Clarke, Ditter, Frazer, Gray, McIlvenny, McKenna, Palmer, Willingale and Najmudin23,Reference Ospina-Bohórquez, Salgado-López, Ehret, Malko, Salvadori, Pisarczyk, Chodukowski, Rusiniak, Krupka, Guillon, Lendrin, Pérez-Callejo, Vlachos, Hannachi, Tarisien, Consoli, Verona, Prestopino, Dostal, Dudzak, Henares, Apiñaniz, De Luis, Debayle, Caron, Ceccotti, Hernández-Martín, Hernández-Toro, Huault, Martín-López, Méndez, Nguyen-Bui, Perez-Hernández, Vaisseau, Varela, Volpe, Gremillet and Santos26].

Table 2

Representative gas and plasma parameters (measured and assumed). The plasma radius ${r}_{\mathrm{p}}$ and the laser energy fraction converted to hot electrons are estimated from dedicated PIC simulations^[ Reference Hicks, Ettlinger, Borghesi, Carroll, Clarke, Ditter, Frazer, Gray, McIlvenny, McKenna, Palmer, Willingale and Najmudin^23, Reference Ospina-Bohórquez, Salgado-López, Ehret, Malko, Salvadori, Pisarczyk, Chodukowski, Rusiniak, Krupka, Guillon, Lendrin, Pérez-Callejo, Vlachos, Hannachi, Tarisien, Consoli, Verona, Prestopino, Dostal, Dudzak, Henares, Apiñaniz, De Luis, Debayle, Caron, Ceccotti, Hernández-Martín, Hernández-Toro, Huault, Martín-López, Méndez, Nguyen-Bui, Perez-Hernández, Vaisseau, Varela, Volpe, Gremillet and Santos^26].

Table 3

Plasma properties estimated using the model presented in Section 2.1.

We assume the laser energy is separated as follows: the total laser energy is multiplied by some fraction to reflect the amount of energy contained within the laser focus, which is called ${E}_{\mathrm{L}}$ ; the energy in the focus is then multiplied by a fraction ${\eta}_{\mathrm{L}}$ , which reflects its absorption in the gas and a further fraction ${\eta}_{\mathrm{las}\to \mathrm{h}}$ , which is the fraction of energy converted to hot electrons. The laser energy not converted into hot electrons goes into the thermal electrons and is eventually converted into the kinetic energy of the plasma ions as the plasma expands.

Four of the input parameters for our model are ‘assumed’, which means they have been estimated based on simulations or previous experimental data. The laser absorption ${\eta}_{\mathrm{L}}$ in the gas is inferred from dedicated particle-in-cell (PIC) simulations^[ Reference Hicks, Ettlinger, Borghesi, Carroll, Clarke, Ditter, Frazer, Gray, McIlvenny, McKenna, Palmer, Willingale and Najmudin^23, Reference Ospina-Bohórquez, Salgado-López, Ehret, Malko, Salvadori, Pisarczyk, Chodukowski, Rusiniak, Krupka, Guillon, Lendrin, Pérez-Callejo, Vlachos, Hannachi, Tarisien, Consoli, Verona, Prestopino, Dostal, Dudzak, Henares, Apiñaniz, De Luis, Debayle, Caron, Ceccotti, Hernández-Martín, Hernández-Toro, Huault, Martín-López, Méndez, Nguyen-Bui, Perez-Hernández, Vaisseau, Varela, Volpe, Gremillet and Santos^26], which indicate that the laser is entirely depleted after it has passed through the dense gas. The conversion efficiency of laser energy to hot electrons, ${\eta}_{\mathrm{las}\to \mathrm{h}}$ , is a function of many variables, including the gas density and laser intensity. It is not measured in any of the experiments described here and must therefore be estimated to the nearest order of magnitude. For near-critical density plasmas the available data is relatively scarce, although there is evidence that the hot electron conversion efficiency ranges from a few percent to more than 10% under certain conditions^[ Reference Brunetti, Campbell, Lovell and Jaroszynski^39, Reference Feng, Li, Tan, Wang, Li, Zhang, Meng, Ge, Liu, Yan, Fu, Chen and Zhang^40]. Here, we take an upper estimate of ${{\eta}_{\mathrm{las}\to \mathrm{h}}=0.4}$ to illustrate the scenario of strong charging and EMP. The plasma channel radius and length are estimated from PIC simulations^[ Reference Hicks, Ettlinger, Borghesi, Carroll, Clarke, Ditter, Frazer, Gray, McIlvenny, McKenna, Palmer, Willingale and Najmudin^23, Reference Ospina-Bohórquez, Salgado-López, Ehret, Malko, Salvadori, Pisarczyk, Chodukowski, Rusiniak, Krupka, Guillon, Lendrin, Pérez-Callejo, Vlachos, Hannachi, Tarisien, Consoli, Verona, Prestopino, Dostal, Dudzak, Henares, Apiñaniz, De Luis, Debayle, Caron, Ceccotti, Hernández-Martín, Hernández-Toro, Huault, Martín-López, Méndez, Nguyen-Bui, Perez-Hernández, Vaisseau, Varela, Volpe, Gremillet and Santos^26, Reference Willingale, Mangles, Nilson, Clarke, Dangor, Kaluza, Karsch, Lancaster, Mori, Najmudin, Schreiber, Thomas, Wei and Krushelnick^31, Reference Bonvalet, Loiseau, Marquès, Atukpor, d’Humières, Domange, Forestier-Colleoni, Hannachi, Lancia, Raffestin, Tarisien, Tikhonchuk and Nicolaï^41] and experimental interferograms^[ Reference Ospina-Bohórquez, Salgado-López, Ehret, Malko, Salvadori, Pisarczyk, Chodukowski, Rusiniak, Krupka, Guillon, Lendrin, Pérez-Callejo, Vlachos, Hannachi, Tarisien, Consoli, Verona, Prestopino, Dostal, Dudzak, Henares, Apiñaniz, De Luis, Debayle, Caron, Ceccotti, Hernández-Martín, Hernández-Toro, Huault, Martín-López, Méndez, Nguyen-Bui, Perez-Hernández, Vaisseau, Varela, Volpe, Gremillet and Santos^26, Reference Maitrallain, Marquès, Bontemps, Bonvalet, Atukpor, Bagnoud, Carrière, Hannachi, Henares, Hornung, Huber, d'Humières, Lancia, Loiseau, Nicolaï, Santos, Tikhonchuk, Zielbauer and Tarisien^42], which suggest that channels several hundred micrometres in length and tens of micrometres in radius can be formed on the Vulcan-TAP and VEGA-3 laser systems a few ps after the arrival of the laser pulse.

Consider conditions on the Vulcan Petawatt laser, with pulse energy ${E}_{\mathrm{L},\mathrm{tot}}=200$ J, duration ${\tau}_{\mathrm{L}}=600$ fs and wavelength ${\lambda}_{\mathrm{L}}=1.053\kern0.22em \mu \mathrm{m}$ ^[ Reference Hicks, Ettlinger, Borghesi, Carroll, Clarke, Ditter, Frazer, Gray, McIlvenny, McKenna, Palmer, Willingale and Najmudin^23]. The laser beam is focused using ${f}_{\#}=3$ optics to a spot with full width at half maximum (FWHM) ${w}_{\mathrm{L}}=3.9\kern0.22em \mu \mathrm{m}$ . Only 40% of the total laser energy is contained within the FWHM, for a maximum on-target intensity of ${I}_{\mathrm{L}}\simeq 2.9\times {10}^{20}$ W cm⁻². The spatial extent of the laser channel in the gas depends on the wavelength of the laser and the gas density. For typical gas pressures ${p}_{\mathrm{gas}}$ ranging from 0.03 to 30 bar, the atomic/molecular densities in the laser focal region are in the range ${{n}_{\mathrm{gas}}\sim {10}^{18}-{10}^{21}}$  cm⁻³. The maximum electron density in a fully ionized plasma is smaller than the critical density, so the laser can propagate through the gas.

The Rayleigh length of a diffraction-limited Gaussian beam in our example is ${Z}_{\mathrm{R}}=\pi {w}_{\mathrm{L}}^2/{\lambda}_{\mathrm{L}}\simeq 44\kern0.22em \mu \mathrm{m}$ . Since the gas jet width is usually larger than ${Z}_{\mathrm{R}}$ and the beam is susceptible to relativistic self-guiding, the laser produces a channel significantly longer^[ Reference Maitrallain, Marquès, Bontemps, Bonvalet, Atukpor, Bagnoud, Carrière, Hannachi, Henares, Hornung, Huber, d'Humières, Lancia, Loiseau, Nicolaï, Santos, Tikhonchuk, Zielbauer and Tarisien^42, Reference Sylla, Flacco, Kahaly, Veltcheva, Lifschitz, Malka, d’Humières, Andriyash and Tikhonchuk^43] than ${Z}_{\mathrm{R}}$ . It can be viewed as an ${l}_{\mathrm{p}}\simeq 0.5$ mm-long plasma cylinder created at a typical height of $h\simeq 0.5$ mm above the nozzle. We take the initial radius of the plasma channel to be a factor of a few times larger than the laser focal radius, ${r}_{\mathrm{p}}=20\kern0.22em \mu \mathrm{m}$ , to reflect the average size of the channel as the laser deposits energy over the full length of its path through the gas. We assume that laser absorption in the gas jet is ${\eta}_{\mathrm{L}}\sim 100$ %, with 40% transferred to hot electrons.

For the parameters of the Vulcan experiment given in Tables 1–3, a plasma channel of radius ${r}_{\mathrm{p}}=20\kern0.22em \mu \mathrm{m}$ and length ${l}_{\mathrm{p}}=0.5$ mm has volume ${V}_{\mathrm{p}}=\pi {r}_{\mathrm{p}}^2{l}_{\mathrm{p}}\simeq 6\times {10}^{-7}$ cm³. A hydrogen gas pressure of 15 bar corresponds to an atomic gas density ${n}_{\mathrm{at}}\simeq 8.1\times {10}^{20}$ cm ${}^{-3}$ at a distance $h\simeq 0.5$ mm above the nozzle, so we have ${N}_{\mathrm{e}}\simeq 5\times {10}^{14}$ electrons. Equation (2) yields an effective electron temperature ${T}_{\mathrm{e}}=250$  keV for the total bulk energy of 43 J.

A hot electron temperature of ${T}_{\mathrm{h}}=5.0$ MeV is prescribed following the ponderomotive scaling^[ Reference Wilks, Kruer, Tabak and Langdon^44], $\left(\sqrt{1+{a}_0^2}-1\right){m}_{\mathrm{e}}{c}^2$ . If we further assume that ${\eta}_{\mathrm{las}\to \mathrm{h}}=0.4$ on the Vulcan laser, then Equation (4) gives a hot electron fraction ${n}_{\mathrm{h}}/{n}_{\mathrm{e}}\simeq 2.5$ % with total energy of 29 J. The hot electron density follows from the hot electron temperature and the heat capacity of a relativistic electron gas, as shown in the previous section.

The solution of Equation (5) for typical parameters ${h/{r}_{\mathrm{p}}=25}$ and ${r}_{\mathrm{p}}{\omega}_{\mathrm{ph}}/c=18$ gives ${\Phi}_{\mathrm{p}}=24.8$ MV. Knowing the plasma potential and the plasma capacitance $C\simeq 0.0086$ pF, we find the charge ejected from the plasma column, ${Q=C{\Phi}_{\mathrm{p}}\simeq 234}$  nC. This corresponds to a fraction of escaped electrons $\delta {n}_{\mathrm{h}}/{n}_{\mathrm{e}}\approx 2.8\times {10}^{-3}$ and is consistent with the experiment^[ Reference Simpson, Scott, Mariscal, Rusby, King, Grace, Aghedo, Pagano, Sinclair, Armstrong, Manuel, Haid, Flippo, Winslow, Gatu-Johnson, Frenje, Neely, Kerr, Williams, Andrews, Cauble, Charron, Costa, Fischer, Maricle, Stuart, Albert, Lemos, Mackinnon, MacPhee, Pak and Ma^45].

Since the time required for a hot electron to cross the channel is relatively short at approximately $2{r}_{\mathrm{p}}/c=0.13$ ps, the time of plasma charging is determined by the propagation time of the laser pulse through the gas, approximately 3 ps.

Following Equation (6), the total energy of escaped electrons ${\mathrm{\mathcal{E}}}_{\mathrm{esc}}$ is divided between the electrostatic energy of the charged plasma ${\mathrm{\mathcal{E}}}_{\mathrm{es}}={Q}^2/2C\simeq 3.2$ J and the kinetic energy of the escaped electrons asymptotically equal to $4.2$ J.

As discussed in the previous section, the average ion kinetic energy, ${\varepsilon}_{\mathrm{i}}\simeq 0.4$ MeV, is 1.5 times the bulk electron temperature for a hydrogen plasma. This corresponds to an ion velocity of ${v}_{\mathrm{i}}\simeq 9\kern0.22em \mu \mathrm{m}/\mathrm{ps}$ , and an ion expansion time to the nozzle ${t}_{\mathrm{exp}}\simeq 60$ ps. The total energy carried by these ions is of the order of the energy carried by the expanding thermal electrons – that is, about $\left(1-{\eta}_{\mathrm{las}\to \mathrm{h}}\right){\eta}_{\mathrm{L}}{E}_{\mathrm{L}}\sim 40$ J for the Vulcan experiment.

The model estimate of $5\times {10}^{14}$ ions with a combined kinetic energy of several tens of joules can be compared with measured ion spectra and simulations. Figure 3(a) shows an ion spectrum from Ref. [Reference Hicks, Ettlinger, Borghesi, Carroll, Clarke, Ditter, Frazer, Gray, McIlvenny, McKenna, Palmer, Willingale and Najmudin23] measured at 90° to the laser axis. The peak ion yield of approximately ${10}^{11}$ MeV ${}^{-1}$ sr⁻¹ occurs at approximately 2 MeV. The proton signal drops off at lower energies because the configuration of B-/E-fields inside the spectrometer limits its dynamic range to about two decades. Other ion spectral measurements^[ Reference Wei, Mangles, Najmudin, Walton, Gopal, Tatarakis, Dangor, Clark, Evans, Fritzler, Clarke, Hernandez-Gomez, Neely, Mori, Tzoufras and Krushelnick^16, Reference Hicks, Ettlinger, Borghesi, Carroll, Clarke, Ditter, Frazer, Gray, McIlvenny, McKenna, Palmer, Willingale and Najmudin^23, Reference Puyuelo-Valdes, Henares, Hannachi, Ceccotti, Domange, Ehret, d’Humieres, Lancia, Marquès, Ribeyre, Santos, Tikhonchuk and Tarisien^34, Reference Marquès, Loiseau, Bonvalet, Tarisien, d’Humières, Domange, Hannachi, Lancia, Larroche, Nicolaï, Puyuelo-Valdes, Romagnani, Santos and Tikhonchuk^46, Reference Marquès, Lancia, Loiseau, Forestier-Colleoni, Tarisien, Atukpor, Bagnoud, Brabetz, Consoli, Domange, Hannachi, Nicolaï, Salvadori and Zielbauer^47] and simulations^[ Reference Hicks, Ettlinger, Borghesi, Carroll, Clarke, Ditter, Frazer, Gray, McIlvenny, McKenna, Palmer, Willingale and Najmudin^23, Reference Bonvalet, Loiseau, Marquès, Atukpor, d’Humières, Domange, Forestier-Colleoni, Hannachi, Lancia, Raffestin, Tarisien, Tikhonchuk and Nicolaï^41] suggest that the sub-MeV thermal ion population should be orders of magnitude more numerous than the multi-MeV plasma-accelerated ions. Ion spectra measured at the PHELIX laser using spectrometers specifically designed to measure sub-MeV ions^[ Reference Marquès, Loiseau, Bonvalet, Tarisien, d’Humières, Domange, Hannachi, Lancia, Larroche, Nicolaï, Puyuelo-Valdes, Romagnani, Santos and Tikhonchuk^46] show sub-MeV ion yields of approximately ${10}^{14}$ particles.

Figure 3

Ion spectra collected in gas jet experiments. (a) Proton spectrum from an experiment on the Vulcan-TAP laser, measured at $90{}^{\circ}$ to the laser axis using a Thomson parabola spectrometer with BAS-TR image plate^[ Reference Hicks, Ettlinger, Borghesi, Carroll, Clarke, Ditter, Frazer, Gray, McIlvenny, McKenna, Palmer, Willingale and Najmudin^23]. The shaded region is the $3\sigma$ detection limit. (b) $\alpha$ -particle spectra from an experiment at VEGA-3^[ Reference Ospina-Bohórquez, Salgado-López, Ehret, Malko, Salvadori, Pisarczyk, Chodukowski, Rusiniak, Krupka, Guillon, Lendrin, Pérez-Callejo, Vlachos, Hannachi, Tarisien, Consoli, Verona, Prestopino, Dostal, Dudzak, Henares, Apiñaniz, De Luis, Debayle, Caron, Ceccotti, Hernández-Martín, Hernández-Toro, Huault, Martín-López, Méndez, Nguyen-Bui, Perez-Hernández, Vaisseau, Varela, Volpe, Gremillet and Santos^26], measured at $\pm 17{}^{\circ}$ from the laser axis using diamond time-of-flight detectors. The two spectra were recorded on different shots. See also Figure 5(a). (c) Proton spectrum from a separate experiment at VEGA-3^[ Reference Henares, Puyuelo-Valdes, Salgado-López, Apiñaniz, Bradford, Consoli, de Luis, Ehret, Hannachi, Hernández-Martín, Huber, Lancia, Mackeviciute, Maitrallain, Marquès, Pérez-Hernández, Santos, Santos, Stankevic, Tarisien, Tomkus, Volpe and Gatti^24], measured using a Thomson parabola spectrometer at $90{}^{\circ}$ to the laser axis. The spectrometer dynamic range limits reliable measurements to energies more than approximately 1.3 MeV. The blue dashed line represents the background noise level. See also Figure 5(b).

In addition to ions accelerated by bulk electron pressure in the expanding plasma, some ions are accelerated to energies of a few MeV in the electrostatic field created by the escaped electrons. Hicks et al. ^[ Reference Hicks, Ettlinger, Borghesi, Carroll, Clarke, Ditter, Frazer, Gray, McIlvenny, McKenna, Palmer, Willingale and Najmudin^23] report on the number of such fast protons accelerated in the radial direction as 30 nC/sr. Assuming an emission solid angle of $1-2$ sr, the total charge of ejected protons is about 60 nC and their overall energy is about 0.2 J. These values are consistent with 230 nC charge of ejected electrons and a corresponding energy of approximately 4 J, as estimated above.

3.1 X-ray photoionization of the gas

The bremsstrahlung emission of electrons in the laser-created plasma covers a broad range of photon energies up to the electron kinetic energy. Assuming the electron energy distribution is characterized by an effective temperature ${T}_{\mathrm{e}}$ , the power per unit volume of bremsstrahlung emission from a hydrogen plasma can be written as follows^[ Reference Richardson^48]:

$$\begin{align*}{P}_{\mathrm{Brem}}=1.69\times {10}^{-32}{n}_{\mathrm{e}}^2{T}_{\mathrm{e}}^{1/2}\ \mathrm{W}\;{\mathrm{cm}}^{-3},\end{align*}$$

where the electron density is in cm⁻³ and the electron temperature is in eV. The radiative contribution of bulk electrons dominates that of hot electrons because ${{n}_{\mathrm{e}}{T}_{\mathrm{e}}\gtrsim {n}_{\mathrm{h}}{T}_{\mathrm{h}}}$ under the present conditions. For an electron density of ${n}_{\mathrm{e}}=8\times {10}^{20}$ cm⁻³ in fully ionized plasma and a temperature ${{T}_{\mathrm{e}}\simeq 250}$  keV, we have ${P}_{\mathrm{Brem}}=6\times {10}^{12}$ W cm⁻³. Accounting for the plasma volume of ${V}_{\mathrm{p}}\sim 6\times {10}^{-7}$ cm³ and lifetime ${{t}_{\mathrm{exp}}\sim 60}$  ps (see Section 3.3), the total radiated energy is about ${\mathrm{\mathcal{E}}}_{\mathrm{Brem}}={P}_{\mathrm{Brem}}{V}_{\mathrm{p}}{t}_{\mathrm{exp}}\simeq 0.2$ mJ. The spectrum of emission is flat for photons with energy ${\varepsilon}_x\lesssim {T}_{\mathrm{e}}$ and decreases exponentially with a temperature ${T}_{\mathrm{rad}}\simeq {T}_{\mathrm{e}}$ for higher energies.

The mean free path of photons with energies above 3 keV in hydrogen is approximately constant at ${\lambda}_x{\rho}_{\mathrm{gas}}\sim 3$ g cm^−2[ Reference Yao^49]. For a gas jet density of ${\rho}_{\mathrm{gas}}\sim 1.3$ mg cm⁻³, the absorption length is 20 m and the probability of gas ionization over a millimetre distance is negligible. The mean free path of lower energy photons strongly decreases as the energy decreases^[ Reference Yao^49]. It can be approximated as ${\lambda}_x{\rho}_{\mathrm{gas}}\sim {10}^{-10}{\varepsilon}_x^3$ g cm⁻² for hydrogen, where ${\varepsilon}_x$ is the photon energy in eV. The mean free path of photons with the energy of 15–20 eV – comparable to the hydrogen ionization potential ${U}_{\mathrm{ion}}=13.6$ eV – is therefore just a few micrometres.

The photons with energy of about ${\varepsilon}_{\mathrm{h}}\sim $ 100–200 eV produce the most efficient photoionization because their mean free path is comparable to the plasma-nozzle distance. The fraction of bremsstrahlung energy carried by these photons is ${\varepsilon}_{\mathrm{h}}/{T}_{\mathrm{e}}\sim {10}^{-3}$ – that is, about $0.2\kern0.22em \mu \mathrm{J}$ . Knowing the energy required to ionize a hydrogen atom and the volume of gas between the plasma and the nozzle, ${{V}_{\mathrm{gas}}\sim 4\times {10}^{-4}}$  cm³, the gas ionization level can be estimated as ${\mathrm{\mathcal{E}}}_{\mathrm{Brem}}{\varepsilon}_{\mathrm{h}}/{T}_{\mathrm{e}}{U}_{\mathrm{ion}}{V}_{\mathrm{gas}}\sim 1.7\times {10}^{14}$ cm⁻³. This corresponds to an ionized fraction of approximately $3\times {10}^{-7}$ . The photoionization time of approximately 60 ps is defined by the time of bremsstrahlung emission, which is the lifetime of the hot plasma channel.

3.2 Ionization by hot electrons

Hot electrons also contribute to the ionization process. These electrons are those escaping the plasma potential barrier and their characteristics are estimated in Section 2. The stopping power of electrons in hydrogen gas for this range of energies of a few MeV is approximately 4 MeV cm²/g^{[ 50]}, so a hot electron loses approximately 260 eV over the distance ${h\simeq 0.5}$ mm. The energy of secondary electrons is comparable to the ionization potential of the gas^[ Reference Chepel and Araújo^51], which means that one primary electron creates approximately 20 secondary electrons in the gas volume. Using the number of escaped electrons estimated in Section 2.1, ${N}_{\mathrm{esc}}\simeq 1.4\times {10}^{12}$ , the density of secondary electrons produced by collisional ionization is approximately $7.5\times {10}^{16}$ cm⁻³. This corresponds to an ionized fraction of approximately ${10}^{-4}$ , which is produced in a short time of hot electron emission of a few ps.

Alternatively, hot electrons can produce field ionization of the gas if the electron beam density is sufficiently high. For a beam of 3 MeV electrons passing through a neutral gas, field ionization dominates over collisional ionization for beam densities exceeding approximately ${10}^{17}$ cm^−3[ Reference Tikhonchuk^52]. Considering ${10}^{12}$ hot electrons contained within the initial plasma volume, the maximum beam density is approximately ${2.5\times {10}^{17}}$  cm⁻³. So, field ionization has approximately the same impact as collisional ionization.

3.3 Ionization by plasma ions

The stopping power of a representative 0.4 MeV proton in hydrogen is 1200 MeV cm²/g^{[ 53]}. The energy needed for the creation of one secondary electron by a fast ion is of the order of the ionization potential, ${U}_{\mathrm{ion}}$ , and it varies weakly with the ion energy^[ Reference Giesen and Beck^54, Reference Baek and Grosswendt^55]. A 0.4 MeV proton passing through hydrogen gas, therefore, creates approximately 6000 secondary electrons over the 0.5 mm distance between the plasma and the nozzle, losing about 0.1 MeV of its kinetic energy. In a gas volume of approximately $4\times {10}^{-4}$ cm⁻³, this corresponds to complete ionization of the ambient gas. This is, however, a relatively long process that takes approximately 60 ps.

The contribution of fast ions to gas ionization is smaller by more than three orders of magnitude, but their velocity is about three times higher. An ionization level of approximately $3\times {10}^{-3}$ is therefore produced prior to plasma expansion, during the time of flight of the fast ions, which is about 20 ps.

3.4 Gas ionization by electrical breakdown

When hot electrons are ejected from the laser plasma, it becomes positively charged with respect to the nozzle. The electric field between the plasma and nozzle may then break down the gas and propagate a discharge. The discharge regime is determined by the product of the gas pressure and electrode separation ${p}_{\mathrm{gas}}h$ . Under Vulcan-TAP conditions, with ${p}_{\mathrm{gas}}h\gtrsim 1$ bar cm, avalanche ionization will occur if the potential is above the breakdown value of ${20\,{-}\,30}$  kV^[ Reference Raizer^56]. This is much smaller than the plasma potential of approximately 25 MV estimated in Section 2.

In the avalanche process, the electron density increases exponentially in time from the seed level ${n}_{\mathrm{e}0}/{n}_{\mathrm{at}}\sim {10}^{-4}- {10}^{-3}$ created by fast electrons or ions, ${n}_{\mathrm{e}}(t)={n}_{\mathrm{e}0}\kern0.1em \exp \left({\nu}_{\mathrm{ion}}t\right)$ , where ${\nu}_{\mathrm{ion}}$ is the characteristic ionization rate. According to Refs. [Reference Raizer56,Reference Solovyev, Terekhin, Tikhonchuk and Altgilbers57], the ionization rate is ${\nu}_{\mathrm{ion}}\sim {10}^{12}$ s⁻¹ for Vulcan conditions and the gas can be fully ionized in a few picoseconds. However, the plasma potential decreases with time for two reasons: firstly, it decreases logarithmically with time because of plasma expansion according to Equation (5) and, secondly, because the energy deposited during the ionization process is extracted from the electrostatic energy. The decrease in electrostatic energy is related to the ionization loss, $\Delta \mathrm{\mathcal{E}}\simeq {U}_{\mathrm{ion}}{n}_{\mathrm{e}}{V}_{\mathrm{gas}}$ , and the discharge stops when all the available electrostatic energy ${\mathrm{\mathcal{E}}}_{\mathrm{es}}$ has been exhausted. This relation defines the maximum ionization that can be achieved by avalanche breakdown, ${{n}_{\mathrm{e},\max}\sim 4\times {10}^{21}}$  cm⁻³, which is larger than the atomic gas density.

3.5 Conclusions on ionization processes and plasma resistance

In conclusion, photoionization of the gas jet is low and can be neglected. Instead, ionization by charged particles is produced in three steps: firstly, at the level of ${10}^{-4}$ by fast electrons in a few ps, then at the level of ${10}^{-3}$ by fast ions within 20 ps, and finally by the expanding plasma on a timescale of 60 ps. Free electrons produced during the first two steps provide the seed for a discharge by electrical breakdown. Avalanche breakdown is initiated from the seed level of ionization produced by fast electrons or fast ions on a $10-20$ ps timescale. It can fully ionize the gas under the conditions of the Vulcan experiment before the expanding plasma reaches the nozzle.

The degree of gas ionization determines the plasma resistance and the discharge current that can be supported. We estimate the plasma resistance as $R=\eta h/A$ , where $\eta$ is the plasma resistivity and $A\approx 2{r}_{\mathrm{p}}{l}_{\mathrm{p}}$ is the cross-sectional area of the ionized gas between the nozzle and the laser channel. The plasma resistivity in a fully ionized plasma is dominated by electron–ion collisions and can be estimated from the Drude formula:

(7) $$\begin{align}\eta ={m}_{\mathrm{e}}{\nu}_{\mathrm{ei}}/{e}^2{n}_{\mathrm{e}},\end{align}$$

where ${\nu}_{\mathrm{ei}}$ is the electron–ion collision frequency. Assuming the electron temperature to be of the order of the ionization potential, we find ${\nu}_{\mathrm{ei}}\sim {10}^{14}$ s⁻¹ and the plasma resistivity is $\eta \simeq 5\times {10}^{-6}\ \Omega$ m. This corresponds to a very small resistance of the order of $0.1\kern0.22em \Omega$ . A path to the ground is established when the gas is fully ionized; the potential drop across the nozzle is of comparable magnitude to the plasma potential and a discharge current is produced. The accumulated plasma charge and discharge time puts a limit on the maximum discharge current of the order of approximately 10 kA, as discussed in the next section.

5.1 Energy released through ohmic heating

The energy released by ohmic heating is ${J}^2{Rt}_{\mathrm{p}}$ , where ${J=Q/{t}_{\mathrm{p}}}$ is the discharge current. The resistance $R$ is calculated from the metal resistivity ${\eta}_{\mathrm{d}}$ , the current-carrying surface ${A}_{\mathrm{d}}$ and nozzle length ${h}_{\mathrm{d}}$ . Since the discharge is short, the current is confined within skin depth, $\delta =\sqrt{\eta_{\mathrm{d}}/\left({\nu}_{\mathrm{emp}}{\mu}_0\right)}$ . For Cu resistivity ${\eta}_{\mathrm{d}}=1.7\times {10}^{-7}\kern0.1em \Omega$ m and frequency ${\nu}_{\mathrm{emp}}\approx 2.5$ GHz, the skin depth is $\delta \sim 10\ \mu \mathrm{m}$ . Assuming the current flows along the ${h}_{\mathrm{d}}=3$ cm nozzle with a radius of ${r}_{\mathrm{d}}=5$ mm, the current-carrying cross-sectional area is ${A}_{\mathrm{d}}\sim 3\times {10}^{-3}$ cm ${}^2$ and the resistance is $R={\eta}_{\mathrm{d}}{h}_{\mathrm{d}}/{A}_{\mathrm{d}}\approx 0.01\kern0.22em \Omega$ . The energy released by ohmic heating with a kA-level current over ${{t}_{\mathrm{p}}\sim 2h/c\approx 3}$ ps is therefore less than approximately $0.1\kern0.22em \mu \mathrm{J}$ .

Will the conducting layer melt if it is supplied with $0.1\kern0.22em \mu \mathrm{J}$ of heat energy? The volume of heated material is ${{h}_{\mathrm{d}}{A}_{\mathrm{d}}\sim {10}^{-2}}$  cm³, which gives a heated mass of approximately 80 mg. The available electrostatic energy is not sufficient to heat such a large mass, so it is unlikely that the melting of gas nozzles is caused by ohmic heating from a discharge current.

5.2 Heating caused by plasma deposition

Plasma ions are the primary source of nozzle heating. Assuming that ${N}_{\mathrm{i}}$ ions in the plasma are expanding isotropically, the angular ion flux is ${N}_{\mathrm{i}}/4\pi$ . The solid angle subtended by the nozzle is given by $2\pi \left(1-\cos \alpha \right)$ , where $\tan \alpha ={r}_{\mathrm{d}}/h$ . For $h=0.5$ mm and ${r}_{\mathrm{d}}=5$ mm, the solid angle is approximately $2\pi$ and the number of ions incident on the nozzle is around half the ion population.

The stopping power of 0.4 MeV protons in Cu is 166 MeV cm²/g^{[ 53]} and the rate of energy deposition is approximately 1500 MeV/cm. The ions therefore deposit all their energy over a distance of less than approximately 10 μm. The maximum heated volume is $8\times {10}^{-6}$ cm³ and the mass of heated material is approximately 0.02 mg.

Based on the estimates of plasma density and volume from Section 2.3, there are ${N}_{\mathrm{i}}\sim 5\times {10}^{14}$ ions at energy approximately 0.4 MeV for a combined energy of 40 J. Half of these ions strike the nozzle and deposit an energy of 250 kJ/g. This is more than 100 times higher than the energy required to melt Cu, so plasma heating melts the nozzle easily.

The same conclusion applies to a ceramic nozzle, even with the greater heat resistance. Consider SiC with a melting temperature of 3100 K, 370 J/g latent heat of melting and a specific heat capacity of $0.67{-}1.4$ J/(g K) for temperatures between 300 and 4000 K^{[ 61]}. Using these values, we find that approximately 4 kJ/g is required to melt SiC. According to the National Institute of Standards and Technology (NIST) proton stopping catalogue, the stopping power of a 0.5 MeV proton in SiO₂ is 290 MeV cm²/g^{[ 53]}. For a density of 3.2 g cm⁻³, the rate of energy deposition is 1000 MeV/cm and the deposition depth is approximately 5 μm, for a heated volume of approximately $2\times {10}^{-5}$ cm³ and a heated mass of $0.06-0.1$ mg. This is consistent with SRIM Monte Carlo simulations^[ Reference Ziegler and Biersack^62] of 0.4 MeV protons incident on SiC, which give a 4 μm range. The 20 J of incident ion energy deposited in a few micrometres corresponds to heating of approximately 200 kJ/g – more than sufficient to melt the ceramic.

This conclusion is supported by a gas jet experiment on the VEGA-3 laser^[ Reference Henares, Puyuelo-Valdes, Salgado-López, Apiñaniz, Bradford, Consoli, de Luis, Ehret, Hannachi, Hernández-Martín, Huber, Lancia, Mackeviciute, Maitrallain, Marquès, Pérez-Hernández, Santos, Santos, Stankevic, Tarisien, Tomkus, Volpe and Gatti^24]. The laser was focused to an intensity of $2.2\times {10}^{19}$ W cm⁻² in a He (97%) and H₂ (3%) gas mix with peak atomic densities of the order of approximately ${10}^{21}$ cm⁻³ (see Section 6.2 for more details of the experiment). Tungsten nozzles suffered progressive damage over tens of shots when the laser was focused at a distance of approximately 900 μm, whereas a UV fused silica nozzle was destroyed when the laser was focused at a distance of approximately 400 μm from the nozzle surface.

We apply this model of nozzle damage to a Vulcan-TAP experiment. The amount of energy deposited by the ions is sensitive to the number of ions and their average energy. Taking a vertical gas density profile from measurements by Hicks et al. ^[ Reference Hicks, Ettlinger, Borghesi, Carroll, Clarke, Ditter, Frazer, Gray, McIlvenny, McKenna, Palmer, Willingale and Najmudin^23], we estimate the number of ions generated in the laser channel when the laser is focused at different heights above the gas jet. We assume a value of ${N}_{\mathrm{i}}$ at a fixed height of 160 μm, where the density is maximal, and scale it by the normalized vertical density profile as the laser focus is shifted to different heights above the nozzle. Following the method outlined earlier, we then calculate the ion flux on the nozzle surface and the amount of energy deposited when the laser is focused at different distances from the nozzle. In the experiment, metallic nozzles were instantly destroyed at a nozzle-focus distance of $400\kern0.22em \mu$ m and virtually undamaged when they were separated by 2 mm. Since the melt threshold for Cu is 1.4 kJ/g, this suggests that the ion energy deposition must reach approximately 2 kJ/g when the laser is focused somewhere between these two distances. These observations give bounds on the total number of 0.5 MeV plasma ions produced by the laser at a height of $160\kern0.22em \mu \mathrm{m}$ , which satisfies $4\times {10}^{12}<{N}_{\mathrm{i}}<2\times {10}^{14}$ . The product of the initial plasma volume and peak gas density gives a maximum electron number of approximately $5\times {10}^{14}$ , which may be considered an upper limit on the number of accelerated ions.

The situation is illustrated graphically in Figure 4. Figure 4(a) shows the ion energy deposited in the nozzle as a function of distance, assuming $4\times {10}^{12}$ plasma ions at 0.5 MeV when the laser is focused at a height of $160\kern0.22em \mu \mathrm{m}$ . Figure 4(b) shows the energy deposition for $2\times {10}^{14}$ plasma ions at a height of $160\kern0.22em \mu \mathrm{m}$ above the nozzle. The amount of nozzle heating increases as the laser approaches the peak gas density at approximately 160 μm and then drops steeply as the laser is focused further away from the nozzle. This is caused partially by the reduced solid angle subtended by the nozzle and also the changing gas density profile. Accounting for ion collisions in the gas before they reach the nozzle means that less overall energy is deposited in the nozzle, but the energy per unit mass of heated material increases due to a higher ion stopping power at lower energies.

Figure 4

Ion energy deposited per mass of nozzle material as a function of laser-nozzle separation for the number of ions ${N}_{\mathrm{i}}=4\times {10}^{12}$ (a) and $2\times {10}^{14}$ (b) normalized to the plasma height of $160\kern0.22em \mu \mathrm{m}$ . The red dot represents the theoretical melt threshold for a Cu nozzle. Red and green vertical dashed lines represent observed distances where a steel nozzle was destroyed and survived, respectively. The ion energy is 0.5 MeV.

Figure 5

Schematic diagrams of two experiments conducted on the VEGA-3 laser system. (a) Setup described in Section 6.1. A Thomson parabola spectrometer (TP), two electron spectrometers (E-Spec) and four diamond time-of-flight detectors (Diamond ToF) are represented by coloured boxes. (b) Setup described in Section 6.2. Three Thomson parabola spectrometers are placed at 0°, 60° and 90° to the laser axis. The B-dot probe was positioned at variable distances ( $\sim 2{-}3$ m) from the gas target, with its measurement axis horizontal and orthogonal to the line-of-sight axis. A camera was used to take images of the gas at twice the laser fundamental frequency. Further details of these experiments can be found in Refs. [Reference Henares, Puyuelo-Valdes, Salgado-López, Apiñaniz, Bradford, Consoli, de Luis, Ehret, Hannachi, Hernández-Martín, Huber, Lancia, Mackeviciute, Maitrallain, Marquès, Pérez-Hernández, Santos, Santos, Stankevic, Tarisien, Tomkus, Volpe and Gatti24,Reference Ospina-Bohórquez, Salgado-López, Ehret, Malko, Salvadori, Pisarczyk, Chodukowski, Rusiniak, Krupka, Guillon, Lendrin, Pérez-Callejo, Vlachos, Hannachi, Tarisien, Consoli, Verona, Prestopino, Dostal, Dudzak, Henares, Apiñaniz, De Luis, Debayle, Caron, Ceccotti, Hernández-Martín, Hernández-Toro, Huault, Martín-López, Méndez, Nguyen-Bui, Perez-Hernández, Vaisseau, Varela, Volpe, Gremillet and Santos26] .

The estimates presented in this section suggest that nozzle damage is caused primarily by ion energy deposition rather than a resistive current, so nozzle material has little impact on nozzle survival. On the other hand, just as for EMPs emitted from solid targets, the discharge current and EMP amplitude and spectrum change when one moves from conducting to dielectric nozzles.

6.1 Ion acceleration experiment on VEGA-3

An experiment was conducted on the VEGA-3 laser system with the aim of using petawatt laser pulses to trigger laser channelling in inert gases (He, N ${}_2$ , He-N ${}_2$ ) and thereby learn more about ion acceleration mechanisms^[ Reference Ospina-Bohórquez^25, Reference Ospina-Bohórquez, Salgado-López, Ehret, Malko, Salvadori, Pisarczyk, Chodukowski, Rusiniak, Krupka, Guillon, Lendrin, Pérez-Callejo, Vlachos, Hannachi, Tarisien, Consoli, Verona, Prestopino, Dostal, Dudzak, Henares, Apiñaniz, De Luis, Debayle, Caron, Ceccotti, Hernández-Martín, Hernández-Toro, Huault, Martín-López, Méndez, Nguyen-Bui, Perez-Hernández, Vaisseau, Varela, Volpe, Gremillet and Santos^26]. Refer to Figure 5(a) for the vacuum chamber geometry and location of major diagnostics.

A two-lens imaging system was used to monitor the focal spot diameter during the experiment, which was fixed at approximately 12 μm FWHM. A laser pulse duration of ${\tau}_{\mathrm{L}}=72\pm 24$ fs was measured using an autocorrelator. The laser energy varied in the $18.4\pm 2.3\ \mathrm{J}$ range (uncertainties correspond to the standard deviation over $\sim 100$ shots), although only approximately 47% of the pulse energy is contained within the focal spot^[ Reference Ospina-Bohórquez^25]. Two types of shock nozzles were used: Sourcelab J2021 nozzles (peak atomic density ${n}_{\mathrm{at},\max}\approx 5\times {10}^{20}$ cm⁻³ at a height of $\sim 500\ \mu \mathrm{m}$ above the nozzle) and S900 nozzles^[ Reference Henares, Puyuelo-Valdes, Hannachi, Ceccotti, Ehret, Gobet, Lancia, Marquès, Santos, Versteegen and Tarisien^63] (peak atomic density ${{n}_{\mathrm{at},\max}\approx {10}^{20}}$ cm⁻³ up to $\sim 900$ μm above the nozzle). The S900 nozzles were designed to produce a convergent shock further from the nozzle surface than the J2021 design in order to reduce nozzle damage and degradation of the gas density profile. Interferometric measurements showed that the J2021 had a narrower, denser gas profile along the laser axis than the S900 nozzle. They also revealed that He gas produced denser wings and broader density peaks than N ${}_2$ or the He-N ${}_2$ mix. J2021 and S900 nozzles will hereafter be referred to as ‘short-focus’ and ‘long-focus’ nozzles, respectively.

To measure the electron density in the plasma channel, a folding-wave interferometer was used to take optical interferograms of the ionized gas at different temporal delays relative to the drive laser^[ Reference Pisarczyk, Santos, Dudzak, Zaras-Szydłowska, Ehret, Rusiniak, Dostal, Chodukowski, Renner, Gus’kov, Korneev, Burian, Vlachos, Kochetkov, Makaruk, Rosinski, Kalal, Krupka, Pfeifer, Klir, Cikhardt, Krasa, Singh, Borodziuk, Krus, Juha, Hrebicek, Golasowski and Skala^64]. Figure 6(b) shows a He density distribution from the experiment taken at approximately equal to 150 ps after the arrival of the laser, revealing a laser channel with average radius of approximately equal to 70 μm. Interferograms could not be recovered at earlier probing times because the channel boundaries were obscured by plasma self-emission. Modelling the expansion as a Sedov–Taylor cylindrical blast wave^[ Reference Hutchens^65, Reference Zeldovich and Raizer^66], ${R(t)={\xi}_0{\left({\mathrm{\mathcal{E}}}_{\mathrm{b}}{t}^2/{\rho}_{\mathrm{gas}}{l}_{\mathrm{p}}\right)}^{1/4}}$ , gives an energy of ${\mathrm{\mathcal{E}}}_{\mathrm{b}}\simeq 1.3$ J (taking ${\xi}_0=0.9$ ^[ Reference Zeldovich and Raizer^66]) deposited in the channel over its length of ${{l}_{\mathrm{p}}\simeq 0.5}$  mm, which is less than 20% the deposited laser energy of 7.3 J. Such a significant difference is explained by the fact that the expanding plasma is essentially collisionless. Plasma ions propagate through the ambient gas and ionize atoms without creating a density compression – only a small portion of the slow ion population contributes to shock wave formation.

Figure 6

Images corresponding to optical probe arrival approximately 150 ps after the drive laser in a He gas with a long-focus shock nozzle. (a) Raw interferogram. (b) Density map showing a plasma channel straddling the peak density region at $x=250$ μm. The laser focus position in the vacuum was set at $x=0$ μm.

Two-dimensional (2D) PIC simulations in CALDER^[ Reference Ospina-Bohórquez, Salgado-López, Ehret, Malko, Salvadori, Pisarczyk, Chodukowski, Rusiniak, Krupka, Guillon, Lendrin, Pérez-Callejo, Vlachos, Hannachi, Tarisien, Consoli, Verona, Prestopino, Dostal, Dudzak, Henares, Apiñaniz, De Luis, Debayle, Caron, Ceccotti, Hernández-Martín, Hernández-Toro, Huault, Martín-López, Méndez, Nguyen-Bui, Perez-Hernández, Vaisseau, Varela, Volpe, Gremillet and Santos^26, Reference Debayle, Mollica, Vauzour, Wan, Flacco, Malka, Davoine and Gremillet^28] and experimental interferograms of the gas at the point of laser arrival suggest that, by the time the laser has travelled through the low-density wings of the gas density profile and arrived at the central high-density region, the laser has become significantly defocused. For a gas density of 4.5 bar and a plasma channel radius of $20\ \mu \mathrm{m}$ , the plasma volume is approximately $6\times {10}^{-7}$ cm³, the laser energy deposited in the gas is 7.3 J, the bulk electron temperature is ${T}_{\mathrm{e}}\simeq 140$  keV and the pressure is approximately 50 Mbar (see Table 3).

The stopping power of 140 keV electrons in He is approximately 3 MeV cm²/g^{[ 50]}, which corresponds to a mean free path of more than 50 cm for our gas density. The Debye radius, however, is of the order of $0.1\ \mu \mathrm{m}$ , so bulk electrons remain in the plasma due to the Coulomb attraction and the plasma expansion is quasi-neutral. Bremsstrahlung losses are negligible on this timescale, so the plasma expands adiabatically.

Assuming that all bulk electron energy is transferred to ions, the average energy of helium ions is about 0.43 MeV, their velocity is approximately 5 μm/ps and the expansion time is 100 ps. In this experiment, about 10% of the absorbed laser energy is transferred to hot electrons with an effective temperature of approximately 1.1 MeV given by the ponderomotive scaling. Then using the plasma charging model described in Section 2, we estimate a plasma capacitance of 0.0086 pF, a plasma potential of 4.4 MV and 42 nC charge of escaped electrons. The plasma electrostatic energy is about 0.1 J and the escaped electrons have carried away approximately 0.15 J.

Applying the analysis of gas ionization described in Section 2, we find that the photoionization probability is very low – about $1.6\times {10}^{-7}$ , the level of ionization by fast electrons is two orders of magnitude larger at approximately $3.3\times {10}^{-5}$ and the dominant ionization processes are electrical breakdown and ions in the expanding plasma. The plasma ionization time is, therefore, within a few tens of ps. The plasma discharge results in EMP emission with energy of approximately 0.17 mJ, which corresponds to an electric field of approximately 6.3 kV/m and a magnetic field of $21\kern0.22em \mu \mathrm{T}$ at 1 m from the source. Nozzle damage is due to the energy deposition of a few joules by the plasma ions.

Progress of gas ionization between the laser and nozzle was measured with a pick-off beam converted in the second harmonic and directed transversely to the laser channel for interferometric imaging. Figure 7 shows interferograms taken at two different times after the arrival of the laser pulse. Figure 7(a) corresponds to the earliest probing time measured after the laser pulse arrival. The shadow of the gas is visible in both images, suggesting that the entire gas volume can be ionized within 40 ps. The speed of the ionization front, therefore, exceeds approximately 20 μm/ps, which is consistent with gas ionization by electrical breakdown.

Figure 7

Interferograms of the VEGA-3 laser interacting with N₂ gas ejected from a short-focus shock nozzle. Probe times relative to the arrival of the pump beam are 40 ps (a) and 90 ps (b). The laser intensity is ${10}^{20}$ W/cm² and the gas density is ${10}^{20}$ cm⁻³.

To monitor ion emission during the experiment, five diamond time-of-flight detectors^[ Reference Salvadori, Consoli, Verona, Cipriani, Anania, Andreoli, Antici, Bisesto, Costa, Cristofari, de Angelis, Di Giorgio, Ferrario, Galletti, Giulietti, Migliorati, Pompili and Zigler^67] were placed in multiple different locations around the vacuum chamber (0°, $\pm 17{}^{\circ}$ , $4.85{}^{\circ}$ , $5.5{}^{\circ}$ with respect to the laser axis, always inclined at 9° to the horizontal plane of the laser) and a Thomson parabola spectrometer was placed along the laser axis in the same horizontal plane as the laser. When the diamond detectors were placed at $\pm 17{}^{\circ}$ , nitrogen ions with energy up to approximately 80 MeV were measured. For shots on He gas, $\alpha$ -particles were accelerated to 0.7 MeV/u with ${10}^9$ particles per steradian, while shots on N₂ gas produced ions up to 5.7 MeV/u with ${10}^7$ particles per steradian. These ions were measured in the laser forward direction within a $\pm 17{}^{\circ}$ cone^[ Reference Ospina-Bohórquez, Salgado-López, Ehret, Malko, Salvadori, Pisarczyk, Chodukowski, Rusiniak, Krupka, Guillon, Lendrin, Pérez-Callejo, Vlachos, Hannachi, Tarisien, Consoli, Verona, Prestopino, Dostal, Dudzak, Henares, Apiñaniz, De Luis, Debayle, Caron, Ceccotti, Hernández-Martín, Hernández-Toro, Huault, Martín-López, Méndez, Nguyen-Bui, Perez-Hernández, Vaisseau, Varela, Volpe, Gremillet and Santos^26]. Sample He spectra from the time-of-flight diagnostics can be found in Figure 3(b). We expect higher yields perpendicular to the laser axis.

6.2 EMP experiment on VEGA-3

A second experiment was conducted on VEGA-3 with a view to characterize the EMP and ions produced in laser–gas interactions (see Figure 5(b)). The laser energy before the compressor was approximately 30 J and the pulse duration was 30 fs. Based on images of the focal spot taken at low energy, 21% of the energy on-target was contained within the first Airy disk^[ Reference Henares, Puyuelo-Valdes, Salgado-López, Apiñaniz, Bradford, Consoli, de Luis, Ehret, Hannachi, Hernández-Martín, Huber, Lancia, Mackeviciute, Maitrallain, Marquès, Pérez-Hernández, Santos, Santos, Stankevic, Tarisien, Tomkus, Volpe and Gatti^24] for an on-target intensity of the order of approximately ${10}^{20}$  W cm⁻² at best compression, similar to the intensity reported for the experiment in the previous section. The laser contrast was ${10}^{-12}$ at $0.1$ ns, with no significant pre-pulses^[ Reference Henares, Puyuelo-Valdes, Salgado-López, Apiñaniz, Bradford, Consoli, de Luis, Ehret, Hannachi, Hernández-Martín, Huber, Lancia, Mackeviciute, Maitrallain, Marquès, Pérez-Hernández, Santos, Santos, Stankevic, Tarisien, Tomkus, Volpe and Gatti^24]. A Prodyn RB-230(R) radiation-hardened B-dot probe was used to measure the amplitude of the magnetic field at different distances from the gas jet, while two diamond time-of-flight detectors and three Thomson parabolas were used to monitor charged particle emission. Signal degradation due to EMP pick-up in the unshielded oscilloscope prevented the easy identification of a photo-peak in the time-of-flight data, so quantitative analysis of the ion spectrum is not possible. A proton spectrum from the Thomson parabola positioned at 90° to the laser axis is shown in Figure 3(c). The data is integrated over five shots, with a lower proton sensitivity limit of approximately 1.3 MeV. The proton yield increases towards lower energies, with a maximum of approximately $3\times {10}^{11}$ MeV⁻¹ sr⁻¹ at the low-energy limit. B-dot signals were recorded on a Rohde&Schwarz RTO64 digital oscilloscope with 2 GHz bandwidth and 10 GS/s sampling rate. The B-dot probe was oriented so that its axis was parallel to the ground and sensitive to an azimuthal magnetic field relative to the nozzle axis.

B-dot voltage signals were bandpass-filtered between 0.4 and 2 GHz, with the lower limit determined by the probe frequency response^[ Reference Rączka, Dubois, Hulin, Tikhonchuk, Rosiński, Zaraś-Szydłowska and Badziak^68, Reference Dubois, Rączka, Hulin, Rosiński, Ryć, Parys, Zaraś-Szydłowska, Makaruk, Tchórz, Badziak, Wołowski, Ribolzi and Tikhonchuk^69] and the upper limit by the oscilloscope bandwidth. The waveforms were then cropped, the zero-point offset removed and cable attenuation corrected in the Fourier domain. The cable attenuation functions were measured using a Rohde&Schwarz ZNA4 vector network analyser from 5 MHz to 4 GHz, but the correction was only applied between 0.4 and 2 GHz to avoid amplifying noise beyond the sensitivity range of the diagnostic. Finally, the voltages were integrated in time and multiplied by the probe effective area of 0.2 cm² (supplied by the manufacturer) to yield the magnetic field.

Both solid and gaseous targets were studied during the experiment. The gas was a 3:97 H₂-He mix at approximately 1000 bar backing pressure, forced vertically downwards through the nozzle aperture to the laser focus. The electron density in the laser focal region was close to ${10}^{21}$ cm⁻³. On shots with solid targets, the nozzle and solenoid valve assembly (Figure 8) was replaced by a bracket and multi-foil array. The foils were made from 6-μm-thick aluminium. Figure 9 shows typical EMP waveforms for solid and gaseous targets, demonstrating a reduction by a factor of two to three in the peak magnetic field for the same laser parameters when solid targets were switched to gas. This is consistent with the results of Kugland et al. ^[ Reference Kugland, Aurand, Brown, Constantin, Everson, Glenzer, Schaeffer, Tauschwitz and Niemann^8] on the PHELIX laser with an Ar gas jet and tallies with our theoretical estimates. The ChoCoLaT2 code^[ Reference Poyé, Hulin, Ribolzi, Bailly-Grandvaux, Lubrano-Lavaderci, Bardon, Raffestin, Santos and Tikhonchuk^70] evaluates the charge produced by the VEGA-3 laser interacting with 6-μm-thick Al foils to be of the order of 100 nC, which is two times higher than the 42 nC estimated for a gas in Section 6.1.

Figure 8

Three-dimensional graphic of the gas jet nozzle and solenoid valve assembly at VEGA-3. Arrows indicate dimensions relevant to electromagnetic emission.

Figure 9

Comparison of EMP waveforms for solid and gaseous targets on VEGA-3. The signals were measured using a Prodyn RB-230(R) probe positioned at 60° to the laser forward direction at a horizontal distance of $2.66$ m from the nozzle and vertically in-line with the laser focal spot. The maximum amplitude of the magnetic field was a factor two to three times lower for the gas targets compared to 6-μm-thick solid Al foils.

Figure 10 shows measurements of the decay of the magnetic field with distance from the gas jet. The data points come from experimental measurements and represent the average of the maximum and minimum magnetic field values in the waveform. Error bars represent one standard deviation from the mean. The green points represent data taken when the B-dot was positioned at ${60}^{\circ }$ to the laser axis, outside the vacuum chamber and behind a glass window. A Thomson parabola spectrometer inside the chamber blocked the probe’s direct line of sight to the target.

Figure 10

Variation of EMP maximum magnetic field with distance from the gas jet. Data was collected with the B-dot probe positioned at $\phi =60{}^{\circ}$ to the laser axis, with the line of sight to the target occluded. The fitted curve is for a 3-cm-tall antenna with the angle between the antenna axis and the probe assumed constant at $\theta =90{}^{\circ}$ for the different distances.

The magnitude of the magnetic field is of the order of $5{-}10\kern0.22em \mu \mathrm{T}$ at a distance of approximately 2 m from the jet. Significant shot-to-shot variations are due to adjustments in the laser focal position inside the gas to optimize the laser coupling to the target. There are insufficient data points to identify an unambiguous scaling with distance, but they can allow us to estimate the charge accumulated in the gas by the laser ejection of hot electrons if we assume a dipolar radiation field. The solid line represents a least squares fit to the data points with Equation (1) from Ref. [Reference Minenna, Poyé, Bradford, Woolsey and Tikhonchuk27], assuming an antenna height of ${h}_{\mathrm{d}}=3$ cm (consistent with the vertical height of the jet nozzle in Figure 8) and leaving the target charge $Q$ as a free parameter. The best-fit charge is approximately 20 nC in this case. This is in agreement with the model presented in Section 2, which predicts a charge of approximately 40 nC for the VEGA-3 experimental conditions.

Peaks in the EMP Fourier spectrum constrain the EMP emission mechanism. The average of the EMP Fourier spectra for shots with the gas jet targets reveals multiple prominent resonances between ${\nu}_{\mathrm{emp}}\sim 1.2$ and 1.9 GHz (not shown here). Assuming antenna emission from a monopole of height $c/4{\nu}_{\mathrm{emp}}$ , the strongest resonances correspond to heights of approximately 4–5 cm, similar to the dimensions of the nozzle. Note that our measurements were only sensitive to emissions from 0.4 to 2 GHz and there were other large metallic objects in the chamber that might contribute to the EMP.