1 Introduction
In recent years, plasma-based, spin-polarized particle sources have gained significant interest due to their applications, ranging from high energy[
Reference Glashausser
1
] to surface physics[
Reference Tusche, Chen and Schneider
2
]. Moreover, Kulsrud et al.
[
Reference Kulsrud, Furth, Valeo and Goldhaber
3
] showed that polarized reactants in nuclear fusion can increase the corresponding cross-section. In the case of the reaction
$d+t\to \alpha +n$
, the cross-section is approximately 1.5 times larger.
Accordingly, polarized fusion is being investigated by several groups as a possible pathway to higher fusion yields[ Reference Baylor, Deur, Eidietis, Heidbrink, Jackson, Liu, Lowry, Miller, Pace, Sandorfi, Smith, Tafti, Wei, Wei and Zheng 4 – Reference Heidbrink, Baylor, Büscher, Engels, Garcia, Ghiozzi, Miller, Sandorfi, Wei and Zheng 6 ].
From a purely accelerator-based perspective, magnetic vortex acceleration (MVA)[ Reference Jin, Wen, Zhang, Hützen, Thomas, Büscher and Shen 7 – Reference Zou, Guo, Wen, Liu, Yan, Liu and Jin 9 ] and collisionless shock acceleration (CSA)[ Reference Yan, Wu, Geng, Zhang, Shen and Ji 10 , Reference Reichwein, Shen, Büscher and Pukhov 11 ] have been investigated intensively as possible acceleration schemes for polarized protons and other ions. A review of the state-of-the-art for this field has been given by Reichwein et al. [ Reference Reichwein, Gong, Zheng, Ji, Pukhov and Büscher 12 ].
Using other schemes commonly utilized for ion acceleration, such as target normal sheath acceleration, is currently not feasible in the context of polarized beams, since the targets have to be pre-polarized using mechanisms such as metastability exchange optical pumping[ Reference Mrozik, Endner, Hauke, Heil, Karpuk, Klemmer and Otten 13 ].
Thus, available targets are currently limited to near-critical densities[
Reference Fedorets, Zheng, Engels, Engin, Feilbach, Giesen, Glückler, Kannis, Klehr, Lennartz, Pfeifer, Pfennings, Schneider, Schnitzler, Soltner, Swaczyna and Büscher
14
,
Reference Sofikitis, Reichwein, Stamatakis, Zois, Cohen, Büscher, Pukhov and Rakitzis
15
]. The first successful plasma-based acceleration of polarized helium-3 was shown by Zheng et al.
[
Reference Zheng, Fedorets, Engels, Engin, Glückler, Kannis, Schnitzler, Soltner, Chitgar, Gibbon, Reichwein, Pukhov, Zielbauer and Büscher
16
], where the dominant acceleration mechanism was identified as Coulomb explosion due to the specific target density and the interaction length. In particular, the ions were expelled at
$\pm 90{}^{\circ}$
with respect to the laser propagation direction, necessitating the placement of polarimeters in those directions and limiting the statistics compared to forward-directed beams.
In the MVA- and CSA-based studies it was observed that stronger laser fields lead to an increase in energy, but come at the cost of decreased beam polarization. A possible mitigation tactic is the ‘dual-pulse MVA’ scheme[
Reference Reichwein, Pukhov and Büscher
17
], where two laser pulses propagate side-by-side leading to a formation of a separate ion filament that is better shielded from depolarizing field components. A problem with this scheme, however, is the difficult realization of beam alignment in experiments since the two pulses would need to co-propagate with a carrier envelope phase difference of
$\pi /2$
.
Another approach to forming these central filaments is ion acceleration using Laguerre–Gaussian (LG) laser pulses, which carry orbital angular momentum (OAM) and are characterized by an azimuthal index
$\mathrm{\ell}$
and a radial index
$p$
[
Reference Allen, Beijersbergen, Spreeuw and Woerdman
18
].
Various theoretical studies have shown that – due to their inherently different field structure from Gaussian pulses – LG modes can be utilized to accelerate ion beams with a low divergence[ Reference Zhang, Shen, Zhang, Xu, Wang, Wang, Yi and Shi 19 – Reference Culfa, Sagir and Satilmis 22 ].
Similarly, so-called ‘light-spring pulses’ consisting of several LG modes have recently been proposed as an option for high-quality proton acceleration[ Reference Guo, Zhang, Shen and Tajima 23 ].
Currently, the experimentally achievable intensity and maximum order of LG modes are still limited. In 2020, Wang et al.
[
Reference Wang, Jiang, Dong, Lu, Li, Xu, Sun, Yu, Guo, Liang, Leng, Li and Xu
24
] presented results of a relativistic hollow laser with peak intensities of up to
$I\approx 6.3\times {10}^{19}$
W/cm
${}^2$
. With currently available and near-future laser facilities such as SULF and SEL[
Reference Wang, Liu, Lu, Chen, Long, Li, Chen, Chen, Bai, Li, Peng, Liu, Wu, Wang, Li, Xu, Liang, Leng and Li
25
], even higher-intensity LG modes could soon be realized.
In the context of polarized beams, Wu et al.
[
Reference Wu, Ji, Geng, Yu, Wang, Feng, Guo, Wang, Qin, Yan, Zhang, Thomas, Hützen, Büscher, Rakitzis, Pukhov, Shen and Li
26
] have already proposed the use of LG beams for electron acceleration. It was shown that due to the comparatively weaker azimuthal field, pre-polarized electrons maintained a higher polarization degree than with a Gaussian pulse. Further, they observed that the injection phase is the most crucial since polarization is only marginally affected once the particles reach a Lorentz factor of
$\gamma \gg 1$
.
In this paper, we propose to utilize LG laser pulses with
$\mathrm{\ell}=1,p=0$
to accelerate spin-polarized helium-3. Utilizing three-dimensional (3D) particle-in-cell (PIC) simulations, we show that the different geometry from conventional Gaussian pulses leads to a high degree of polarization and a low divergence, allowing for more forward-directed polarized ion beams. In Section 2 we will discuss the setup and the results of our 3D-PIC simulations. These results are further discussed in Section 3, where we derive a simplified analytical model to understand the magnetic field structure.
2 Particle-in-cell simulations
Three-dimensional PIC simulations were conducted with the fully electromagnetic code vlpl
[
Reference Pukhov
27
,
Reference Pukhov
28
]. The simulation domain has a size of
$x\times y\times z=120{\lambda}\times 60{\lambda}\times 60{\lambda}$
(
$x$
being the direction of laser propagation;
$\lambda =800$
nm). The grid resolution is
${h}_x=0.05\lambda, {h}_y={h}_z=0.125\lambda$
. As we use the rhombi-in-plane solver[
Reference Pukhov
29
], we choose the time step
$\Delta t={h}_x/c$
. Further, we make use of vlpl’s scaling feature, which increases the transverse grid size by a factor of
$1.05$
for
$\mid y\mid, \mid z\mid \geqslant 20\lambda$
for reasons of computational efficiency. For the laser pulse, we only consider an LG laser pulse with azimuthal index
$\mathrm{\ell}=1$
and radial index
$p=0$
, since realizing higher-order modes in experiment is still a significant challenge. The pulse has a focal spot size of
$6\lambda$
and a pulse duration of 20 fs. Its normalized laser vector potential
${a}_0={eE}_\mathrm{L}/\left({m}_\mathrm{e}c{\omega}_0\right)$
is varied in the range
${a}_0=20-50$
. Here,
$e$
denotes the elementary charge,
${m}_\mathrm{e}$
the electron rest mass,
$c$
the vacuum speed of light,
${\omega}_0$
the laser frequency and
${E}_\mathrm{L}$
the laser’s peak electric field.
The helium-3 target is modeled as an initially non-ionized, top-hat slab of
$60\lambda$
length and
$0.3{n}_{\mathrm{cr}}$
density (
${n}_{\mathrm{cr}}={m}_\mathrm{e}{\omega}_0^2/\left(4\pi {e}^2\right)$
being the critical density). We consider a fully pre-polarized target, that is, the initial spin direction for all helium ions is the
$+x$
-direction. It is generally based on the target used in the experimental campaign[
Reference Fedorets, Zheng, Engels, Engin, Feilbach, Giesen, Glückler, Kannis, Klehr, Lennartz, Pfeifer, Pfennings, Schneider, Schnitzler, Soltner, Swaczyna and Büscher
14
,
Reference Zheng, Fedorets, Engels, Engin, Glückler, Kannis, Schnitzler, Soltner, Chitgar, Gibbon, Reichwein, Pukhov, Zielbauer and Büscher
16
], although we consider higher densities and shorter targets throughout the various simulation runs. Field ionization in vlpl is described using the Ammosov–Deloine–Krainov (ADK) model[
Reference Ammosov, Delone and Krainov
30
].
The spin dynamics are incorporated into vlpl in form of the Thomas–Bargmann–Michel–Telegdi (T-BMT) equation[
Reference Thomas
31
,
Reference Bargmann, Michel and Telegdi
32
], which calculates the change of the semi-classical spin vector
$\mathbf{s}$
as follows:
$$\begin{align}\frac{\mathrm{d}\boldsymbol{s}}{\mathrm{d}t}=-\boldsymbol{\varOmega} \times \boldsymbol{s}.\end{align}$$
The precession frequency is given as follows:
$$\begin{align}\boldsymbol{\varOmega} =\frac{qe}{mc}\left[{\varOmega}_B\boldsymbol{B}-{\varOmega}_v\left(\frac{\boldsymbol{v}}{c}\cdot \boldsymbol{B}\right)\frac{\boldsymbol{v}}{c}-{\varOmega}_E\frac{\boldsymbol{v}}{c}\times \boldsymbol{E}\right],\end{align}$$
with
$qe$
denoting the ion charge,
$m$
its mass and
$c$
the vacuum speed of light. Here,
$\boldsymbol{E},\boldsymbol{B}$
correspond to the electromagnetic field the particle is subject to, while
$\boldsymbol{v}$
is its velocity. The prefactors further depend on the anomalous magnetic moment
$a$
and the Lorentz factor
$\gamma$
:
$$\begin{align}{\varOmega}_{B}=a+\frac{1}{\gamma },\kern1em {\varOmega}_{v}=\frac{a\gamma}{\gamma +1},\kern1em {\varOmega}_{E}=a+\frac{1}{\gamma +1}.\end{align}$$
The anomalous magnetic moment for an electron is
${a}_\mathrm{e}\approx {10}^{-3}$
. For the helium-3 considered here, its magnitude is significantly larger,
$a\approx -4.184$
.
As discussed by Thomas et al. [ Reference Thomas, Hützen, Lehrach, Pukhov, Ji, Wu, Geng and Büscher 33 ], other spin-related effects, such as the Stern–Gerlach force or the Sokolov–Ternov effect, can be neglected in our parameter regime due to the field strength and timescale we consider.
For dense targets (here
$0.3{n}_{\mathrm{cr}}$
), the dominant acceleration mechanism in our simulations is identified to be MVA[
Reference Nakamura, Bulanov, Esirkepov and Kando
34
].
In conventional MVA with a single Gaussian laser pulse[ Reference Park, Bulanov, Bin, Ji, Steinke, Vay, Geddes, Schroeder, Leemans, Schenkel and Esarey 35 ], the pulse generates a plasma channel due to its ponderomotive force. At the channel center, electrons are accelerated in the wake induced by the pulse, generating a strong forward current. Accordingly, a return current forms along the channel wall that, in turn, leads to the magnetic vortex structure. At the back edge of the target, the fields expand upon entering the vacuum region, leading to the formation of accelerating and focusing fields.
By comparison, the LG pulse utilized in our simulations creates a more complex field, which in the
$x$
–
$y$
-plane looks like two co-propagating structures (see Figure 1 for an exemplary comparison of the Gaussian- and LG-induced density and field structure). In fact, a similar field structure is seen in the dual-pulse MVA scheme[
Reference Reichwein, Pukhov and Büscher
17
], which essentially is nothing but a plane representation of the LG modes. These electromagnetic fields still lead to the formation of a well-defined filament along the optical axis
$y=0$
, which is subsequently accelerated.
Figure 1 Exemplary comparison of the filament formation (a), (c) and magnetic field (b), (d) for a Gaussian and an LG laser pulse. The electromagnetic fields are normalized to
${E}_0={B}_0={m}_\mathrm{e}c{\omega}_0/e.$
The prevalent structures in density and electromagnetic fields after approximately 470 fs are shown for the simulation with
${a}_0=50$
in Figure 2. The electron and ion density (Figures 2(a) and 2(b)) exhibit the typical central filament, which – in the case of the ions – is highly polarized (Figure 2(c)). The longitudinal sheath field visible in Figure 2(d) accelerates the ions to high energies (cf. the phase space in Figure 2(e)). The magnetic vortex structure is indicated by the component
${B}_z$
in Figure 2(f).
Figure 2 Exemplary PIC simulation result for a short target after 470 fs. Plots (a) and (b) show the electron and helium density, respectively. Nuclear spin polarization is shown in (c). The bottom row shows the accelerating field (d), the ions’ phase space (e) and the
$z$
-component of the magnetic field (f). The electromagnetic fields are normalized to
${E}_0={B}_0={m}_\mathrm{e}c{\omega}_0/e$
.
The data from the parameter scan are displayed in Table 1. As expected, the maximum ion energy rises with increased
${a}_0$
, for example, from 91.5 MeV at
${a}_0=20$
to approximately 365.8 MeV for
${a}_0=50$
. The corresponding energy spectra are shown in Figure 3 (using equal-width binning, like all subsequent spectra). No distinct mono-energetic features are observed for the laser and target parameters considered here.
Table 1 Results from 3D-PIC simulations using a short target (
${L}_{\mathrm{ch}}\equiv 60\lambda$
). Note that the minimum polarization
${P}_{\mathrm{min}}$
corresponds to the minimum polarization per energy bin (cf. Figure 4).
Figure 3 Energy spectra for various
${a}_0$
and the target with
$0.3{n}_{\mathrm{cr}}$
. No distinct mono-energetic features are observed.
The polarization per energy bin is calculated as
$P=\sqrt{P_x^2+{P}_y^2+{P}_z^2}$
, where
${P}_j={\sum}_i{s}_{i,j}/N$
is the average over the spin components of the
$N$
-particle ensemble in the spatial direction
$j\in \left\{x,y,z\right\}$
. The results are shown in Figure 4. As for previous studies, the degree of polarization decreases for higher intensities since the precession frequency of spin is
$\mid \boldsymbol{\varOmega} \mid \propto \max \left\{|\boldsymbol{E}|,|\boldsymbol{B}|\right\}$
. Throughout the intensity scan, polarization remains at a level of more than
$90\%$
. Moreover, the simulation results indicate that the initial polarization direction (
$x$
), not just the magnitude of the polarization vector, is generally well-preserved. Notably, the polarization for
${a}_0=40$
and
${a}_0=50$
is comparable, which can be attributed to the fact that the target (density) is not matched to the different intensities but rather is kept fixed throughout our scan. A direct comparison of the LG results to single-pulse[
Reference Jin, Wen, Zhang, Hützen, Thomas, Büscher and Shen
7
] and dual-pulse[
Reference Reichwein, Pukhov and Büscher
17
] MVA with Gaussian pulses is complicated, as the two different laser modes with the same
${a}_0$
will generally produce particle beams of different energy. Moreover, LG pulses have a different critical power ratio than Gaussian pulses, thus changing their interaction in underdense plasma dramatically (cf. Section 3).
Figure 4 Polarization spectra for the target with
$0.3{n}_{\mathrm{cr}}$
. Note that very high polarizations for large energies are partly of statistical nature, since the energy bins contain only a few macro-particles (
$<10$
for the highest-energy bins).
The angular spectra in Figure 5 show that for the case of
${a}_0=50$
fewer ions are forward-accelerated as compared to
${a}_0=20$
which, again, is due to the absence of any target parameter matching (see also the discussion in Section 3). Changing the laser and target parameters further away from ‘optimal MVA conditions’ would start to introduce stronger contributions of other acceleration mechanisms; for example, in the case of the experimental study on polarized helium-3 at PHELIX[
Reference Zheng, Fedorets, Engels, Engin, Glückler, Kannis, Schnitzler, Soltner, Chitgar, Gibbon, Reichwein, Pukhov, Zielbauer and Büscher
16
], the longer, low-density target as well as the longer, weaker laser pulse led to the dominance of Coulomb explosion in
$\pm 90{}^{\circ}$
rather than forward acceleration. Using a pre-ionized target instead (not shown here), energy and polarization spectra only exhibit marginal differences to the non-ionized case. However, significantly more particles are deflected in the
$\pm 90{}^{\circ}$
direction.
Figure 5 Angular spectra for
${a}_0=20$
and
${a}_0=50$
. The other curves are excluded for better visibility. Note that for higher intensity, fewer ions are accelerated forward.
The target parameters available in experiments are indeed what is currently limiting the acceleration of polarized ions via laser–plasma interaction. While high-density, short gas jets can generally be realized, experiments with polarized helium-3 require pre-polarized targets. These are – up to now – only available with a maximum density of approximately
${10}^{19}\ {\mathrm{cm}}^{-3}=0.006{n}_{\mathrm{cr}}$
. Moreover, the target used by Zheng et al.
[
Reference Zheng, Fedorets, Engels, Engin, Glückler, Kannis, Schnitzler, Soltner, Chitgar, Gibbon, Reichwein, Pukhov, Zielbauer and Büscher
16
] has an interaction length on the scale of 1 mm. Simulations by Gibbon et al.
[
Reference Gibbon, Zheng, Chitgar, Fedorets, Lehrach, Li and Büscher
36
] have shown that even a slightly shorter target could lead to a more forward-directed beam.
Therefore, we have also conducted additional simulations with reduced densities but the same interaction length of
$60\lambda$
to evaluate the effect on MVA via LG pulses. The density reduction leads to a strongly reduced maximum energy of 35.5 MeV at
$0.03{n}_{\mathrm{cr}}$
and only 4.2 MeV at
$0.006{n}_{\mathrm{cr}}$
. The minimum polarization in both cases exceeds the higher-density simulations at approximately 99%. The higher polarization can be attributed to the improved collimation process. Whereas the central filament for the higher-density target (see Figure 2(b)) has distinct kinks and imperfections, the filament at lower densities is much smoother and narrower. Thus, the particles in the filament will experience fewer depolarizing contributions. As mentioned before, laser and target parameters have not been matched for these simulations. We will discuss aspects of possible optimization in the following section.
3 Discussion
The PIC results show distinct improvements over conventional MVA with Gaussian laser pulses, and even the dual-pulse scheme[
Reference Reichwein, Pukhov and Büscher
17
]. The main reason behind these improvements is the inherently different field structure of the LG pulses: the potential for an LG pulse[
Reference Wilson, Sheng, McKenna and Hidding
37
] with arbitrary
$\mathrm{\ell}$
and
$p=0$
is
$$\begin{align}a\left(r,\theta, x\right)&={a}_0\exp \left[-{\left(\frac{t}{d_0}\right)}^2-{\left(\frac{r}{w_0}\right)}^2\right]{\left(\frac{r}{w_0}\right)}^{\mid \mathrm{\ell}\mid}\notag\\ &\quad{}\times \exp \left[i\left( kx-\omega t-\mathrm{\ell}\theta \right)\right].\end{align}$$
Here,
${d}_0$
and
${w}_0$
denote the pulse duration and beam waist, respectively. Thus, for
$\mathrm{\ell}=1,p=0$
, the potential will have a radial dependency
$a(r)\propto \exp \left(-{r}^2\right)r$
. We will ignore the
$\theta$
- and
$x$
-dependencies for now, since we are interested in the radial force exerted by the pulse. The ponderomotive force is calculated as
${F}_\mathrm{p}\propto -\left(1/\gamma \right)\nabla {a}^2(r)$
, where
$\gamma =\sqrt{1+{a}^2(r)}$
[
Reference Quesnel and Mora
38
]. Thus, in our case
$$\begin{align}{F}_{\mathrm{p},\perp }(r)\propto \frac{4\exp \left(-2{\tilde{r}}^2\right)\cdot {r}^3/{w}_0^4-2\exp \left(-2{\tilde{r}}^2\right)\cdot r/{w}_0^2}{\sqrt{1+\exp \left(-2{\tilde{r}}^2\right)\cdot {\tilde{r}}^2}},\end{align}$$
with
$\tilde{r}=r/{w}_0$
. This force expels ions for
$r>{w}_0$
, but focuses ions close to the central axis. Notably, the intensity of the LG mode is zero on the optical axis.
Thus, particles in the central accelerated filament are compressed by the ponderomotive force. Spin precession is mainly induced by the prevalent azimuthal magnetic field, as observed in other MVA studies[
Reference Jin, Wen, Zhang, Hützen, Thomas, Büscher and Shen
7
,
Reference Reichwein, Hützen, Büscher and Pukhov
8
,
Reference Reichwein, Pukhov and Büscher
17
]. In order to understand the high degree of polarization in the LG case better, we devise a strongly simplified model to reproduce the structure of the azimuthal magnetic field: using the ponderomotive force we can obtain the radial current
${j}_r$
and plug this expression into the continuity equation
${\partial}_t\rho +\nabla \cdot \boldsymbol{j}=0$
. For simplicity, we assume that the system is in steady-state, that is,
${\partial}_t\rho =0$
, and – averaging out any
$\theta$
-dependencies – we obtain the following:
$$\begin{align}\frac{1}{r}{\partial}_r\left({rj}_r\right)=-{\partial}_x{j}_x.\end{align}$$
Note that LG modes have a non-negligible
${E}_x$
component on-axis, which could modulate the axial currents further.
The longitudinal current profile obtained from this simplified model reproduces the regions of backward and forward currents (see the dashed line in Figure 6), but with strong differences in the relative magnitude of those currents compared to PIC simulations.
Figure 6 The heatmap shows the longitudinal current density
${j}_x$
in the
$x$
–
$y$
plane for an exemplary simulation. The black dashed line is the current density profile obtained from analytics. While the regions of forward and backward currents are reproduced, the relative strength of these regions deviates from PIC simulations due to the strongly simplified nature of the model.
Finally, the azimuthal magnetic field generated is calculated using
$\nabla \times \boldsymbol{B}={\mu}_0\boldsymbol{j}$
, and we find the following:
$$\begin{align}{B}_{\theta }(r)\propto \frac{2\exp \left(-2{\tilde{r}}^2\right){r}^3\left(-2{r}^2+{w}_0^2\right)}{\sqrt{1+\exp \left(-2{\tilde{r}}^2\right)\cdot {\tilde{r}}^2}{w}_0^4}.\end{align}$$
Again, due to the simplified nature of the model, the relative magnitude of the extrema does not coincide with PIC simulations, but the general behavior with respect to the radial coordinate
$r$
does. Most importantly, the analytics reproduce the fact that there only is a weak azimuthal field component around
$r=0$
. Therefore, particles close to the optical axis only experience small contributions to spin precession from the azimuthal magnetic field, which ensures the high degree of beam polarization. The mechanism here is similar to the dual-pulse MVA scheme[
Reference Reichwein, Pukhov and Büscher
17
], where two Gaussian pulses propagating side-by-side were used. The dual-pulse scheme presented an improvement over the single-pulse approach, generating similar field structures as in the LG case, but only in one plane. Naturally, field components other than
${B}_{\theta }$
can also induce spin precession. However, the PIC simulations indicate that the azimuthal magnetic field plays a dominant role. Moreover, while the strong laser fields can lead to strong precession in the high-intensity region of the pulse, the ponderomotive force pushes ions toward the central axis, where they are subject to comparatively weaker fields.
As we have seen in the different PIC simulations, the matching of laser and target parameters is crucial for efficient MVA. For conditional MVA, such a condition relating laser and target parameters was found by Park et al. [ Reference Park, Bulanov, Bin, Ji, Steinke, Vay, Geddes, Schroeder, Leemans, Schenkel and Esarey 35 ]:
$$\begin{align}\frac{n_\mathrm{e}}{n_{\mathrm{cr}}}=\sqrt{2}K{\left(\frac{P}{P_{\mathrm{cr}}}\right)}^{1/2}{\left(\frac{c\tau}{L_{\mathrm{ch}}}\right)}^{3/2}.\end{align}$$
Here,
${P}_{\mathrm{cr}}$
is the critical laser power for self-focusing,
${L}_{\mathrm{ch}}$
is the interaction length and
$K=1/13.5$
is a geometrical factor. This condition shows that increases in laser power need to be accommodated by increases in target density, if all other parameters remain fixed. Alternatively, longer targets can be employed.
In the context of pre-polarized sources, however, the choice of target parameters is rather restrictive, as not only are lower densities required[ Reference Fedorets, Zheng, Engels, Engin, Feilbach, Giesen, Glückler, Kannis, Klehr, Lennartz, Pfeifer, Pfennings, Schneider, Schnitzler, Soltner, Swaczyna and Büscher 14 , Reference Zheng, Fedorets, Engels, Engin, Glückler, Kannis, Schnitzler, Soltner, Chitgar, Gibbon, Reichwein, Pukhov, Zielbauer and Büscher 16 ], but also the interaction volume can be restricted: Sofikitis et al. [ Reference Sofikitis, Reichwein, Stamatakis, Zois, Cohen, Büscher, Pukhov and Rakitzis 15 ] proposed an experimentally feasible target based on hydrogen halides, where the degree of polarization strongly depends on the available volume.
For the specific case of LG laser pulses, the critical power ratio is modified compared to the Gaussian case[
Reference Willim, Vieira, Malka and Silva
39
]: for modes with
$\mathrm{\ell}\ne 0,\ p=0$
, it scales as
$P/{P}_{\mathrm{cr}}=\left(2|\mathrm{\ell}|\right)!/\left[{4}^{\mid \mathrm{\ell}\mid }|\mathrm{\ell}|!\left(|\mathrm{\ell}|+1\right)!\right]P/{P}_\mathrm{G}$
, where
${P}_\mathrm{G}$
denotes the critical power for a Gaussian laser. Thus, self-focusing of LG pulses for a given power can differ significantly and change the propagation of the laser pulse in the medium and the formation of related instabilities. This makes a direct comparison between Gaussian and LG pulses in underdense targets even more complicated.
Besides the effective interaction length for MVA, the density ramp at the back edge of the target is of importance. This effect has been neglected in our simulations and analytics so far, as we only model a top-hat slab. Nakamura et al.
[
Reference Nakamura, Bulanov, Esirkepov and Kando
34
] first calculated that the energy per nucleon essentially scales as
$\mathrm{\mathcal{E}}/A\propto {n}_1/{n}_2$
, where
${n}_1$
and
${n}_2$
correspond to the target density before and after the ramp, respectively. For polarized particle beams it was seen that ramps of significant length could influence the final polarization, as ions of different polarization states were piled up[
Reference Reichwein, Hützen, Büscher and Pukhov
8
]. In either case, shorter ramps were shown to be beneficial for the general collimation of the ion beam since the electromagnetic fields do not have enough time to expand in the direction transverse to laser propagation. From an experimental point of view, however, this aspect is limited by the available polarized ion sources as well. A more detailed analytic investigation of density ramps and their effects on polarized beams will be the subject of a separate study.
4 Conclusions
In this paper we have shown the acceleration of polarized helium-3 to several hundred MeV using LG laser pulses (
$\mathrm{\ell}=1,\ p=0$
) in the range of
${a}_0=$
20–50. The helical structure of these modes provides beneficial electromagnetic fields for preservation of polarization as well as low-divergence beams. The minimum polarization observed is at the level of 90% for all simulations. The conducted simulations clearly show that the low densities currently available from pre-polarized ion sources[
Reference Fedorets, Zheng, Engels, Engin, Feilbach, Giesen, Glückler, Kannis, Klehr, Lennartz, Pfeifer, Pfennings, Schneider, Schnitzler, Soltner, Swaczyna and Büscher
14
] inherently limit their efficient acceleration: while several hundred MeV can be obtained from targets in the region of
$0.3{n}_{\mathrm{cr}}$
, realistic densities of
$0.006{n}_{\mathrm{cr}}$
only yield a few MeV, but with approximately 99% polarization. Thus, future research on the optimization of target profiles is necessary to significantly advance the acceleration of polarized ions from laser–plasma interaction.
Acknowledgements
The authors gratefully acknowledge the Gauss Centre for Supercomputing e.V.[ 40 ] for funding this project (SPAF) by providing computing time through the John von Neumann Institute for Computing (NIC) on the GCS Supercomputer JUWELS at Jülich Supercomputing Centre (JSC). The work of M.B. has been carried out in the framework of the JuSPARC (Jülich Short-Pulse Particle and Radiation Center[ Reference Jülich 41 ]) and has been supported by the ATHENA (Accelerator Technology Helmholtz Infrastructure) consortium. The work of A.P. has been supported in parts by BMBF project No. 05P24PF1 (Germany). The work of T.-P.Y. has been supported by the National Natural Science Foundation of China (Grant No. 12375244) and the Natural Science Foundation of Hunan Province of China (Grant No. 2025JJ30002). L.R. would like to thank Oliver Mathiak for fruitful discussions.
Open access
