Since the invention of chirped pulse amplification (CPA)^[1^], high-power laser technology has developed rapidly in the past several decades^[2^]. With ultra-high laser intensity ( $\ge {10}^{18}\ \mathrm{W}/{\mathrm{cm}}^2$ ), high-power lasers have become the cornerstone of the high-field sciences and have been applied in plasma-based charged particle accelerators^[3^–5^], laboratory astrophysics^[6^,7^], attosecond science^[8^] and high-energy-density physics^[9^,10^]. Meanwhile, the manipulation and detection of ultra-intense lasers have become increasingly challenging as the laser peak power has grown, primarily due to the limited damage thresholds of solid optical materials. To overcome this challenge, extensive research has been devoted to plasma optical components, which have rapidly developed owing to their orders-of-magnitude higher optical damage thresholds in comparison to solid-state optics^[11^–22^]. In the past decades, a variety of advanced plasma optical components have been demonstrated for their capacities to manipulate the temporal contrast^[11^], intensity^[12^,13^,18^], duration^[21^], phase^[15^,17^] and polarization^[14^,20^] of relativistic intensity laser pulses. Notably, plasma holograms have been proposed as advanced plasma optics and applied in various domains^[15^,17^,18^], particularly in the generation of relativistic intensity vortex lasers.

The relativistic vortex-laser–plasma interaction has received dramatic attention in the past year^[23^]. With ultra-intense intensity and helical electromagnetic fields, the relativistic vortex laser is regarded as a unique tool for accelerating and manipulating relativistic charged particles, as well as gaining insight into the transfer of angular momentum (AM) between particles and fields under high-field conditions^[24^–40^]. The relativistic intensity and precise phase of vortex lasers are foundational conditions that enable the realization of ingenious dynamic processes in these exciting theoretical and numerical studies. In order to advance the experimental research on relativistic vortex-laser–plasma interaction, various theoretical and numerical schemes have been proposed to generate relativistic intensity vortex lasers^[15^,17^,41^–46^], yet obstacles persist in several aspects, for example, further enhancing the intensity of vortex lasers and uncovering the exact phase information. In the laboratory, the maximum intensity of vortex lasers using reflected phase plates or off-axis spiral phase mirrors still remains around ${10}^{20}\ \mathrm{W}/{\mathrm{cm}}^2$ ^[32^,47^,48^]. Further enhancement of the output intensity beyond ${10}^{21}\ \mathrm{W}/{\mathrm{cm}}^2$ would necessitate a continuous increase in the diameters of the optics. In particular, uncovering the phase of relativistic vortex lasers is of high significance for not only demonstrating the generation of a relativistic vortex laser, but also achieving those exciting numerical and theoretical results in experiments. This has already reached consensus among researchers in the laser–plasma community^[23^,49^], yet an effective detection method is currently still unavailable.

In this paper, we demonstrate a novel method for the reconstruction of the vortex phase and generation of relativistic vortex lasers by surface plasma holograms (SPHs). Firstly, a moderate object laser (vortex laser) and a reference laser (Gaussian laser) are used to simultaneously irradiate the surface of a flat plasma target and interfere with each other. Under the modulation of the ponderomotive force of the interference laser and the generated charge separation fields, SPHs form on the surface plasma of the target. By using the quadrature phase-shift interference, we can reconstruct the phase profile of the incident vortex laser from the density distribution of the SPHs. After the SPH formation, an ultra-intense Gaussian laser as a read-out laser irradiates the hologram. The read-out laser is diffracted by the SPH and duplicates the phase of the object laser, which converts it into an ultra-intense vortex laser. Three-dimensional particle-in-cell (3D-PIC) simulations indicate that a Gaussian read-out laser pulse with intensity of $1.98\times {10}^{20}\ \mathrm{W}/{\mathrm{cm}}^2$ can be converted and amplified to be an ultra-intense vortex laser with intensity of $1.7\times {10}^{21}$ W/cm ${}^2$ at focus. The averaged orbital angular momentum (OAM) of the vortex-laser photon is up to $0.86\mathrm{\hslash}$ , with the energy conversion efficiency to the vortex laser as high as 13.6 $\%$ . As far as we know, this provides a practical way for the first time to reconstruct the vortex phase of relativistic vortex lasers, which is crucial for generating and applying vortex lasers in various domains, for example, attosecond charged particle generation and manipulation. This also demonstrates that plasma as an optical medium enables both manipulation and precise detection of high-power lasers, which will open a new avenue of plasma optics in the ultra-relativistic regime.

The fundamental characteristics of the hologram are the abilities of recording, storing and retrieving the phase of beams. Here, we take the vortex laser and Gaussian laser as examples to introduce the plasma hologram in our study. As shown in Figure 1(a), a linearly polarized (LP) Laguerre–Gaussian (LG) laser with an incident angle of $\theta$ with respect to the $x$ -axis serves as an object laser, while an LP Gaussian laser propagating along the $x$ -axis serves as the reference laser. The electric field amplitude of these two lasers can be expressed respectively as ${E}_{\mathrm{o}}\left(r,\varphi, x\right)={E}_{\mathrm{o}}\exp \left(i{\phi}_{\mathrm{o}}\right)$ and ${E}_{\mathrm{r}}\left(r,\varphi, x\right)={E}_{\mathrm{r}}\exp \left(i{\phi}_{\mathrm{r}}\right)$ , where $\left(r,\varphi, x\right)$ is the cylindrical coordinate and ${E}_{\mathrm{o}}={C}_{\mathrm{o}}\left[{w}_{\mathrm{o}}/{w}_{\mathrm{o}}(x)\right]{L}_{lp}\kern-1pt\left[2{r}^2/{w}_{\mathrm{o}}^2(x)\right]\kern-1pt{\left[\sqrt{2}r/{w}_{\mathrm{o}}(x)\right]}^{{l}}$ $\exp \left[-{r}^2/{w}_{\mathrm{o}}^2(x)\right]$ and ${E}_{\mathrm{r}}={C}_{\mathrm{r}}\left[{w}_{\mathrm{r}}/{w}_{\mathrm{r}}(x)\right]\exp \left[-{r}^2/{w}_{\mathrm{r}}^2(x)\right]$ are the amplitudes of the object laser and reference laser, respectively. Here, ${\phi}_{\mathrm{o}}= l\varphi +{\phi}_{{lp}}+{k}_\text{o}x\cos \theta +{k}_\text{o}y\sin \theta$ and ${\phi}_{\mathrm{r}}={k}_\mathrm{r}x+\left({k}_{\mathrm{r}}{r}^2x\right)/\left[2\left({f}_{\mathrm{r}}^2+{x}^2\right)\right]+\arctan \left(x/{f}_{\mathrm{r}}\right)$ are the phases of the object laser and reference laser, respectively, ${L}_{lp}$ is a generalized Laguerre polynomial with radial index $p$ and azimuthal index $l$ , ${\phi}_{lp}=\left({k}_{\mathrm{o}}{r}^2x\right)/\left[2\left({f}_{\mathrm{o}}^2+{x}^2\right)\right]+\left(l+2p+1\right)\arctan \left(x/{f}_{\mathrm{o}}\right)$ describes the space-dependent phase, ${f}_{\mathrm{o}}=\left(\pi {w}_{\mathrm{o}}^2\right)/{\lambda}_{\mathrm{o}}$ and ${f}_{\mathrm{r}}=\left(\pi {w}_{\mathrm{r}}^2\right)/{\lambda}_{\mathrm{r}}$ are the Rayleigh length of two lasers, respectively, and $k,$ $\lambda$ and $C$ are the wave number of the laser, the wavelength of the laser and a constant, respectively. The subscript ‘o’ denotes the object laser, and the subscript ‘r’ denotes the reference laser. For convenience, we set the parameter $p=0$ and ${k}_{\mathrm{o}}={k}_{\mathrm{r}}=k$ , and the intensity of the interference laser can be written as follows:

$$\begin{align}{I}_\mathrm{i}={\left|{E}_{\mathrm{o}}+{E}_{\mathrm{r}}\right|}^2={\left|{E}_{\mathrm{o}}\right|}^2+{\left|{E}_{\mathrm{r}}\right|}^2+2\mid {E}_{\mathrm{o}}\Vert {E}_{\mathrm{r}}\mid \cos \left({\phi}_{\mathrm{o}}-{\phi}_{\mathrm{r}}\right).\end{align}$$  (1)

We take the ${E}_{\mathrm{o}}$ and ${E}_{\mathrm{r}}$ as unit amplitudes. When the focus spot size of the object laser ${w}_{\mathrm{o}}$ , the reference laser ${w}_{\mathrm{r}}$ and the angle $\theta$ satisfy the following conditions, Equation $(1)$ can be simplified as follows:

$$\begin{align*}{I}_{\mathrm{i}}\simeq \left\{\begin{array}{l}2+2\cos \left[\frac{kr^2x}{2}\left(\frac{1}{f_{\mathrm{o}}^2+{x}^2}\right)+\left(l+1\right)\arctan \left(\frac{x}{f_{\mathrm{o}}}\right)+ l\varphi \right],\\ {}\theta ={0}^{\circ },\,{w}_{\mathrm{r}}\gg {w}_{\mathrm{o}}\sim {\lambda}_{\mathrm{o}},\hfill\left(2\mathrm{a}\right)\\ {}2+2\cos \left[ l\varphi + kx\left(1-\cos \theta \right)- ky\sin \theta \right],\\ {}\theta \ne {0}^{\circ },\,{w}_{\mathrm{o}}\sim {w}_{\mathrm{r}}\gg {\lambda}_{\mathrm{o}}.\hfill\left(2\mathrm{b}\right).\end{array}\right.\end{align*}$$  

Figures 1(b)–1(e) show holograms with parameters $\theta ={0}^{\circ }$ , $\theta ={20}^{\circ }$ and $l=1$ , $l=2$ , respectively. As shown in Figures 1(b) and 1(c), the holograms exhibit circular features as indicated by Equation (2a), and the number of vortex arms increases with $l$ . When the laser parameters satisfy the conditions of Equation (2b), the holograms exhibit fork features, and the number of forked stripes increases with $l$ . In particular, the parameter $l$ of the object laser can be retrieved through the pattern of the hologram in return. When a read-out Gaussian laser is diffracted by the holograms, it duplicates the phase of the object laser and converts it to a vortex laser.

In the following, we uncover the principle of phase reconstruction using quadrature phase-shift interference^[50^]. Taking Equation (2a) as an example, by introducing a phase shift of $\pi /2$ in the phase of the object laser, the intensity of the interference laser can be represented as follows^[51^]:

$$\begin{align}{I}_{\mathrm{i},\pi /2}&={\left|{E}_{\mathrm{o}}\exp \left( i\pi /2\right)+{E}_{\mathrm{r}}\right|}^2\nonumber\\ {}&={\left|{E}_{\mathrm{o}}\exp \left( i\pi /2\right)\right|}^2+{\left|{E}_{\mathrm{r}}\right|}^2+2\mid {E}_{\mathrm{o}}\Vert {E}_{\mathrm{r}}\mid \sin \left({\phi}_{\mathrm{o}}-{\phi}_{\mathrm{r}}\right).\end{align}$$  (3)

Combining Equations (1) and (3), the phase profile of the object laser can be expressed as follows:

$$\begin{align}{\phi}_{\mathrm{o}}={\phi}_{\mathrm{r}}+\arctan \left(\frac{-{I}_{\mathrm{i},\pi /2}+{I}_{\mathrm{o}}+{I}_{\mathrm{r}}}{I_\mathrm{i}-{I}_{\mathrm{o}}-{I}_{\mathrm{r}}}\right).\end{align}$$  (4)

Since ${w}_{\mathrm{o}}\gg {\lambda}_{\mathrm{o}}$ , the phase distribution of the reference laser can be approximated as a planar wavefront, for example, ${\phi}_{\mathrm{r}}=0$ for convenience. Thus, the phase distribution of the object laser can be retrieved by the four key parameters, that is, ${I}_\mathrm{i}$ , ${I}_{\mathrm{i},\pi /2}$ , ${I}_{\mathrm{o}}$ and ${I}_{\mathrm{r}}$ .

Figure 2 schematically illustrates the key features of the SPH and vortex-laser generation. To demonstrate the feasibility of the proposed method, we performed full 3D-PIC simulations with the open-source code EPOCH^[52^]. The grid size of the simulation box is $55{\lambda}_0\times 40{\lambda}_0\times 40{\lambda}_0$ , sampled by $1100\times 800\times 800$ cells with nine macro-particles per cell. The coordinate of the left-hand side of the simulation box is $x=-20{\lambda}_0$ . In this study, an LP LG laser with mode ( $l=1$ , $p=0$ ) is used as the object laser, while two LP Gaussian lasers serve as the reference laser and read-out laser, respectively. The object and reference lasers are incident simultaneously from the left-hand side of the simulation box. The dimensionless electric field amplitude of the three lasers can be expressed as ${\mathbf{a}}_{\mathrm{o}}={a}_{\mathrm{o}}\left[{w}_{\mathrm{o}}/{w}_{\mathrm{o}}(x)\right]\left[\sqrt{2}r/{w}_{\mathrm{o}}(x)\right]$ $\exp \left[-{r}^2/{w}_{\mathrm{o}}^2(x)\right]\cos \left(\varphi +{\phi}_{lp}\right){\mathbf{e}}_y$ , ${\mathbf{a}}_{\mathrm{r}}={a}_{\mathrm{r}}\left[{w}_{\mathrm{r}}/{w}_{\mathrm{r}}(x)\right]\exp \left(-{r}^2/{w}_{\mathrm{r}}^2\right){\mathbf{e}}_y$ and ${\mathbf{a}}_{\mathrm{r-o}}={a}_{\mathrm{r-o}}\cdot\left[{w}_{\mathrm{r-o}}/{w}_{\mathrm{r-o}}(x)\right]\exp \left(-{r}^2/{w}_{\mathrm{r-o}}^2\right){\mathbf{e}}_y$ , where ${a}_{\mathrm{o}}=4{a}_{\mathrm{r}}=1.2$ and ${a}_{\mathrm{r-o}}=12$ are the peak amplitude of the corresponding laser electric fields, respectively. The normalization factor of the electric field of the laser can be represented as $a=(\mathrm{e}E)/\left({m}_{\mathrm{e}}c{\omega}_0\right)$ . The space-dependent phase is ${\phi}_{10}=\left({kr}^2x\right)/\left[2\left({f}_{\mathrm{o}}^2+{x}^2\right)\right]+2\arctan \left(x/{f}_{\mathrm{o}}\right)$ . Here, ${w}_{\mathrm{o}}=1.5{\lambda}_0$ and ${w}_{\mathrm{r}}={w}_{\mathrm{r-o}}=12{\lambda}_0$ are the laser focus spot sizes, ${T}_0$ is the laser cycle, ${\omega}_0$ is the laser frequency, and $e$ , ${m}_{\mathrm{e}}$ and $c$ are the unit charge, the electron mass and the speed of light in vacuum, respectively. The focus of the lasers in vacuum is located at $x=0{\lambda}_0$ . All three lasers have Gaussian time profiles with duration of ${\tau}_{\mathrm{o}}={\tau}_{\mathrm{r}}=300{T}_0$ for the object and reference lasers, and ${\tau}_{\mathrm{r-o}}=7{T}_0$ for the read-out laser. The read-out laser is incident with a time delay of $320{T}_0$ . The flat target consists of fully ionized protons and electrons within the region of $25{\lambda}_0, $-18{\lambda}_0, $z<18{\lambda}_0$ . The density of the target has a longitudinal linear increase from $6{n}_{\mathrm{c}}$ to $30{n}_{\mathrm{c}}$ between $x=25{\lambda}_0$ and $x=27.5{\lambda}_0$ , and remains constant at $30{n}_{\mathrm{c}}$ between $x=27.5{\lambda}_0$ and $x=32{\lambda}_0$ , where ${n}_{\mathrm{c}}=\left({m}_{\mathrm{e}}{\varepsilon}_0{\omega}_0^2\right)/{e}^2$ is the critical density and ${\varepsilon}_0$ is the vacuum dielectric constant. Note that the vortex laser employed in the simulation can already be generated in the laboratory by using reflected phase plates or off-axis spiral phase mirrors^[32^,47^].

The object laser and the reference laser interfere on the target surface, resulting in the formation of a standing wave electromagnetic field with a specific distribution. Figure 3(a) shows the transverse distribution of the electric field ${E}_y$ of the interference laser at $x=25{\lambda}_0$ . The electric field ${E}_y$ of the interference laser has a helical distribution at the cross-section. The maximum amplitude of ${E}_y$ is ${a}_\mathrm{i}=0.3$ , corresponding to the intensity of ${10}^{17}\ \mathrm{W}/{\mathrm{cm}}^2$ . When the target surface is irradiated by the interference laser, the surface electrons are primarily driven by the laser ponderomotive force. We can calculate the transverse ponderomotive force of the interference laser by ${\boldsymbol{F}}_{\perp}=-{e}^2/\left(4{m}_{\mathrm{e}}{\omega}_0^2\right)\nabla {\left|{E}_\mathrm{i}\right|}^2\simeq \left({E}_{\mathrm{o}}{E}_{\mathrm{r}}{e}^2\right)/\left(2{m}_{\mathrm{e}}{\omega}_0^2\right)$ $\sin [\left({kr}^2x\right)/2\left({f}_{\mathrm{o}}^2+{x}^2\right)+2\arctan \left(x/{f}_{\mathrm{o}}\right)+\varphi ] \left[(krx)/\left({f}_{\mathrm{o}}^2+{x}^2\right){\widehat{e}}_{\mathrm{r}}+\left(1/r\right){\widehat{e}}_{\varphi}\right]$ , which depends on the azimuthal coordinate $\varphi$ . As shown in Figure 3(b), the intensity of the interference laser has a similar helical distribution, which agrees well with Figure 1(b). Furthermore, the transverse ponderomotive force exhibits a helical pattern, so that the surface electrons move sideways, forming a helical structure, as shown in Figure 3(c). However, due to the different charge-to-mass ratios of protons and electrons, the charge density distribution on the target surface, as shown in Figure 3(d), generates a strong charge separation electric field. This field strengthens with increasing differences in the charge density and drives the evolution of proton density towards electron density distribution. When the proton density distribution closely matches the electron density distribution, the electric field force exerted on the electrons is balanced by the ponderomotive force of the interference laser, resulting in the formation of SPHs. Figures 3(e) and 3(f) show the transverse distributions of electron and proton density at $t=300{T}_0$ . After the interaction between the interference laser and the plasma flat target, the electrons and protons on the target surface are pushed aside along the helical intensity distribution of the laser while their density profile exhibits a helical groove pattern.

Since the SPH is formed by the laser irradiation on the target, the depth of the SPHs is therefore positively correlated with the energy deposited by the interference laser, that is, ${d}_{\mathrm{SPH}}\left(y,z\right)\propto {I}_\mathrm{i}\left(y,z\right){\tau}_{\mathrm{o,r}}$ , where ${I}_{\mathrm{i}}\left(y,z\right)$ is the intensity of interference laser at the target surface. Thus, ${I}_\mathrm{i}\left(y,z\right)$ can be inferred from ${d}_{\mathrm{SPH}}\left(y,z\right)$ . To reconstruct the vortex phase of the object laser, we have performed three additional simulations, that is, adding $\pi /2$ to the phase of the object laser, having only the object laser and only the reference laser, respectively, while keeping other parameters unchanged. Here, we take ${n}_\mathrm{p}\simeq {n}_{\mathrm{c}}$ as an example to get the depth of the SPHs from the density distributions of the SPHs in the four simulations (see the Supplementary Material for more details). Comparative analysis reveals that altering the phase of the object laser does not change the pattern of the SPHs, but it does cause the pattern to rotate. We use the same laser duration in all four simulations, and the phase of the object laser can thus be expressed as follows:

$$\begin{align}{\phi}_{\mathrm{o}}\left(y,z\right)=\arctan \left[\frac{-{d}_{\mathrm{i},\pi /2}\left(y,z\right)+{d}_{\mathrm{o}}\left(y,z\right)+{d}_{\mathrm{r}}\left(y,z\right)}{d_\mathrm{i}\left(y,z\right)-{d}_{\mathrm{o}}\left(y,z\right)-{d}_{\mathrm{r}}\left(y,z\right)}\right].\end{align}$$  (5)

Figures 4(a)–4(d) respectively present the predicted and simulated phase profiles of the object laser, as well as the laser electric field derived from the phase. The helical phase distribution and the corresponding electric field pattern of the object laser are evident from the figures, demonstrating a strong agreement between the theoretical predictions and simulation results. By the use of data processing algorithms, one can further enhance the precision and accuracy of the phase reconstruction^[53^]. Accurate vortex phase information is crucial for understanding precise electron dynamics in the vortex-laser–plasma interaction. As far as we know, it is the first time that such a precise method for reconstructing the phase of relativistic vortex lasers has been given, which is of significance for generating high-quality relativistic vortex lasers in the laboratory and holds significant implications for relativistic vortex-laser–plasma interaction experiments. For example, spatiotemporal vortex lasers, which possess AM perpendicular to the optical axis, have attracted widespread interest due to their significant potential in generating and accelerating isolated ultrashort electron bunch^[54^]. This proposed method can be applied in detecting the phase distributions of relativistic structured lasers such as spatiotemporal vortex lasers, representing an indispensable aspect of experimental investigation into the interactions between relativistic structured lasers and plasmas^[54^].

We also considered the cases of a higher-order mode laser and oblique incidence of the object laser. When $l=2$ , the SPH exhibits two helical arms. When the object laser satisfies the condition given by Equation (2b), the SPH shows a fork pattern. In both cases, the patterns of the SPHs are consistent with those shown in Figures 1(b) and 1(c). In particular, we have also validated the applicability of Equation (5) in these two cases and depicted the phase reconstruction of the object lasers from theoretical calculations (see the Supplementary Material for more details). It should be noted that this phase reconstruction method is theoretically applicable to low-density plasma, and experimental techniques now allow for the detection of plasma density distribution using visible light, near-infrared light or X-rays^[49^,55^–58^]. For reference, an experimental setup has been proposed for generating and detecting SPHs (see the Supplementary Material for more details).

When the SPH is formed, the read-out laser is incident from the left-hand side of the simulation box at $t=320{T}_0$ . Due to the helical density distribution of the SPH, the reflected laser by the SPH reproduces the phase of the vortex laser. Ultimately, the output laser transforms into a vortex laser near the focal volume. Figure 5(a) shows the 3D isosurface distribution of the electric field ${E}_y$ at $t=388{T}_0$ . It is shown that ${E}_y$ of the output laser exhibits a typical helical feature. To evaluate the performance of the SPH, we approximate the isosurface (e.g., ${n}_\mathrm{p}\simeq 5{n}_{\mathrm{c}}$ ) of the target surface protons as an ideal mirror, and substitute its spatial distribution into Fresnel–Kirchhoff’s diffraction formula to calculate the diffracted electric field of the output laser:

$$\begin{align}E\left(y,z\right)=\frac{1}{i{\lambda}_0}\iint {u}_0\left({y}^{\prime },{z}^{\prime}\right)k\left(\theta \right)\frac{\exp \left( ik\rho \right)}{\rho}\mathrm{d}{y}^{\prime}\mathrm{d}{z}^{\prime },\end{align}$$  (6)

where $\rho =\sqrt{{\left[x-t\left({y}^{\prime },{z}^{\prime}\right)\right]}^2+{\left(y-{y}^{\prime}\right)}^2+{\left(z-{z}^{\prime}\right)}^2}$ , ${u}_0\left({y}^{\prime },{z}^{\prime}\right)=C\exp \left(-{r}^2/{\sigma}_0^2\right)$ is the incident Gaussian laser, $t\left({y}^{\prime },{z}^{\prime}\right)$ represents the spatial distribution of the SPH isosurface and $k\left(\theta \right)=\frac{\cos \left(n,r\right)-\cos \left(n,r_0\right)}{2}$ is the inclination factor. We select three positions within the region between $x=7.1{\lambda}_0$ and $8.1{\lambda}_0$ along the $x$ -axis to calculate the diffraction electric field ${E}_y$ of the output laser. Figures 5(b)–5(d) and 5(e)–5(g) show the simulation results and the theoretical calculations, respectively. One sees that both demonstrate transverse helical electric fields with an approximately $\pi$ phase distribution and a hollow electric field structure, which are in excellent agreement with the characteristic of a clear LG ${}_{10}$ mode laser. Note that part of the laser distributed in the outer ring will focus towards the central axis at an angle during the output vortex-laser focusing. This may lead to a slight increase in the duration of the output vortex laser.

Meanwhile, the output laser is focused near $x=6{\lambda}_0$ after replicating the phase of the object laser, with the focal spot size decreasing from $12{\lambda}_0$ to around $2{\lambda}_0$ , and its intensity increasing by an order of magnitude compared to the incident read-out laser. Figure 6(a) shows the intensity distribution of the output laser in the transverse section at $t=390{T}_0$ . One can see that the vortex laser is amplified as expected with the maximum intensity up to $1.7\times {10}^{21}$ W/cm ${}^2$ . These tightly focused relativistic vortex-laser pulses have diverse applications in high-energy-density physics^[23^,35^], novel optics, etc.

In order to investigate the weights of different modes in the output vortex laser, we select a cross-section of the electric field ${E}_y$ of the output laser at the position of $x=6{\lambda}_0$ at $t=390{T}_0$ and evaluate the corresponding weights of different LG modes from $l$ = 0 to $l$ = 4. Here, the weight of an LG mode can be expressed as follows:

$$\begin{align}{I}_{lp}=\frac{<{E}_{lp}\left(r,\phi, x\right)\mid {E}_y\left(r,\phi, x\right)>}{<{E}_y\left(r,\phi, x\right)\mid {E}_y\left(r,\phi, x\right)>},\end{align}$$  (7)

To investigate the effects of the laser parameters on the SPHs and the generation of output vortex lasers, we vary the parameters of the interference laser in the ( ${a}_{\mathrm{o,r}}$ , ${\tau}_{\mathrm{o,r}}$ ) plane. This involves varying the normalized amplitude and duration of the interference laser from ${a}_{\mathrm{o}}=4{a}_{\mathrm{r}}=0$ to $3$ , and ${\tau}_{\mathrm{o,r}}$ from 0 to 2.5 ps, respectively. Figures 7(a) and 7(b) show their effect on the average depth ( ${d}_0$ ) of the SPHs and the ratio of output vortex-laser intensity to incident read-out laser intensity ( $I$ / ${I}_0$ ). As mentioned previously, SPHs record and convey the vortex phase of the object lasers through the surface plasma density distribution. Therefore, we calculate the average depth, that is, ${d}_0=\left(\sum {d}_{\mathrm{grid}}/{N}_{\mathrm{grid}}\right)\left(r\le {w}_{\mathrm{o,r}}\right)$ , from the original target surface position to the formed SPH surfaces ( ${n}_\mathrm{p}\simeq 5{n}_{\mathrm{c}}$ ), where ${d}_{\mathrm{grid}}$ and ${N}_{\mathrm{grid}}$ are the depth of the simulation box grid and the number of grids, respectively. Since the motion of the surface ions is propelled by the charge separation electric fields, a sufficiently long laser duration is required to effectively modulate the surface ion density. In this sense, the intensity and duration of the drive lasers are two critical parameters for the formation of SPHs. When the pulse duration or intensity of the interference lasers cannot reach a certain value, the interference laser struggles to produce SPHs with sufficient depth, as shown in Figure 7(a). Under such circumstances, the ratio $I/{I}_0$ is also small, as shown in Figure 7(b). Once the duration and intensity of the interference lasers reach this value, the produced SPHs can amplify the intensity of the output vortex laser by an order of magnitude. However, with further increases in the duration and intensity of the interference laser, the amplification of the vortex-laser intensity decreases instead. This indicates that there exists an optimal parameter region for amplifying the intensity of the vortex laser.

We also considered the effects of target material and laser pre-pulses on the SPH formation. As the modulation of target surface plasma is driven by the ponderomotive force of the interference laser and the charge separation fields, the charge-to-mass ratio of ions significantly affects the time required for plasma density modulation. Ions with lower charge-to-mass ratios require a longer modulation time. Taking hydrocarbon targets, for example, a longer duration of laser pulses is required to achieve effective modulation of SPHs (see the Supplementary Material for more details). Since a long-duration interference laser is preferred for the formation of SPHs, the laser pre-pulses effect can thus be ignored, facilitating future experiments. Meanwhile, the expansion of the plasma due to thermal diffusion can be alleviated through multiple measurements during the experimental phase detection process. In addition, we also considered the lifetime of SPHs. After the interference laser leaves the target surface, the surface plasma undergoes an expansion process. Based on the average energy density of surface protons, we calculated the average thermal motion velocity to be approximately $0.001c$ ( $0.33\;\unicode{x3bc} \mathrm{m}/\mathrm{ps}$ ). Considering that the width of the helical arms of the SPH is approximately $3$ $\unicode{x3bc} \mathrm{m}$ , the theoretically predicted lifetime of the SPH is estimated to be around 10 ps. We increased the delay time of the read-out laser to $320{T}_0$ , and the electric field of the reflected vortex laser still exhibited prominent vortex-laser characteristics (see the Supplementary Material for more details).

Finally, we investigate the effects of the parameters of the read-out laser on the vortex-laser generation. Figure 7(c) shows the scaling of the output vortex-laser AM ( ${L}_x$ , black circles), the energy conversion efficiency to the vortex-laser pulse ( $\eta$ , red circles) and the ratio of output vortex-laser intensity to the incident read-out laser intensity ( $I/{I}_0$ , blue circles) with regard to the laser electric field amplitude ${a}_{\mathrm{r-o}}$ . With the increase in amplitude of the read-out laser, the AM of the output vortex laser exhibits an approximately linear growth, while the energy conversion efficiency to the vortex laser decreases approximately linearly. However, the ratio $I/{I}_0$ is insensitive to the laser normalized amplitude ${a}_{\mathrm{r-o}}$ . It slightly increases with the increase in ${a}_0$ before decreasing, reaching its maximum value of $8.57$ at ${a}_{\mathrm{r-o}}=12$ . In Figure 7(d) the laser spot size is varied from ${w}_{\mathrm{r-o}}=8{\lambda}_0$ to $16{\lambda}_0$ , while all other parameters remain unchanged. It is shown that the AM of the output vortex laser increases with the incident laser spot size ${w}_{\mathrm{r-o}}$ . However, the energy conversion efficiency to the vortex laser decreases significantly. This can be attributed to the decreased SPH depth from the $x$ -axis outward, which makes it inefficient to diffract the peripheral laser. Consequently, the energy conversion efficiency of generating the vortex laser decreases gradually. In addition, the ratio $I/{I}_0$ is insensitive to changes in the laser spot size, indicating robustness in oblique incidence laser cases.

In summary, we demonstrate the generation of SPHs by the interference of a vortex laser and a Gaussian laser on the plasma target surface, and confirm its capability of reconstructing the vortex phase and generating ultra-intense vortex lasers. 3D-PIC simulation results indicate that the generated ultra-intense vortex laser possesses ultra-high intensity ( $1.7\times {10}^{21}$ W/cm ${}^2$ ), small spot size ( $\sim 2{\lambda}_0$ ) and large AM ( $3.67\times {10}^{-16}\,\mathrm{kg}\cdot {\mathrm{m}}^2/\mathrm{s}$ ), with an energy conversion efficiency of up to 13.66 $\%$ . It is the first time that such a novel method to retrieve the vortex phase of relativistic vortex lasers has been proposed, which holds critical significance for experimental research on relativistic vortex-laser–plasma interaction. In particular, we demonstrate that plasma can serve not only as a medium for manipulating relativistic intensity laser pulses but also as a detector for precise measurements of the laser phase. This can facilitate future experimental research of vortex-laser–plasma interaction and shall open a new avenue of plasma optics in the ultra-relativistic regime.