Abstract
Twisted Laguerre–Gaussian lasers, with orbital angular momentum and characterized by doughnutshaped intensity profiles, provide a transformative set of tools and research directions in a growing range of fields and applications, from superresolution microcopy and ultrafast optical communications to quantum computing and astrophysics. The impact of twisted light is widening as recent numerical calculations provided solutions to longstanding challenges in plasmabased acceleration by allowing for highgradient positron acceleration. The production of ultrahighintensity twisted laser pulses could then also have a broad influence on relativistic laser–matter interactions. Here we show theoretically and with ab initio threedimensional particleincell simulations that stimulated Raman backscattering can generate and amplify twisted lasers to petawatt intensities in plasmas. This work may open new research directions in nonlinear optics and high–energydensity science, compact plasmabased accelerators and light sources.
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Introduction
The seminal work by Allen et al.^{1} on lasers with orbital angular momentum (OAM) has initiated a path of significant scientific developments that can potentially offer new technologies in a growing range of fields, including microscopy^{2} and imaging^{3}, atomic^{4} and nanoparticle manipulation^{5}, ultrafast optical communications^{6,7}, quantum computing^{8} and astrophysics^{9}. At intensities beyond material breakdown thresholds, it has been recently shown through theory and simulations that intense (with ≳10^{18} W cm^{−2} intensities) and short (with 10–100 fs durations) twisted laser beams could also excite strongly nonlinear plasma waves suitable for highgradient positron acceleration in plasma accelerators^{10}. As a result of their importance, many techniques have emerged to produce Laguerre–Gaussian lasers over a wide range of frequencies^{11}. Common schemes use spiral phase plates or computergenerated holograms to generate visible light with OAM, nonlinear optical media for highharmonic generation and emission of XUV OAM lasers^{12,13} or spiral electron beams in freeelectron lasers to produce OAM Xrays^{14,15}.
Optical elements such as spiral phase plates are designed for the production of laser beams with predefined OAM mode contents. Novel and more flexible mechanisms capable of producing and amplifying beams with arbitrary, welldefined OAM states, using a single optical component, would then be interesting from a fundamental point of view, while also benefiting experiments where OAM light is relevant. In addition, the possibility of extending these mechanisms to the production and amplification of laser pulses with relativistic intensities, well above the damage thresholds of optical devices, could also open exciting perspectives for highenergydensity science and applications. The use of a plasma as the optical medium is a potential route towards the production of OAM light with relativistic intensities. Although other routes may be used to produce highintensity OAM laser pulses, for instance, by placing spiral phase plates either at the start or at the end of a laser amplification chain^{16,17}, the use of plasmas can potentially lead to the amplification of OAM light to very high powers and intensities. Plasmas also allow for greater flexibility in the level of OAM in the output laser beam than other more conventional techniques.
Here we show that stimulated Raman scattering processes in nonlinear optical media with a Kerr nonlinearity can be used to generate and to amplify OAM light. Plasmas, optical fibres and nonlinear optical crystals are examples of nonlinear optical media with Kerr nonlinearity. Although optical parametric oscillators have also been used to transfer OAM from a pump to down converted beams^{18}, here we explore the creation of new OAM states absent from the initial configuration, according to simple selection rules. We also demonstrate that stimulated Raman scattering processes can generate and amplify OAM light even in scenarios where no net OAM is initially present. To this end, we use an analytical theory, valid for arbitrary transverse laser field envelope profiles, complemented by the first threedimensional (3D) ab initio particleincell (PIC) simulation of the process using the PIC code OSIRIS^{19}, considering that the optical medium is a plasma. Starting from recent experimental and theoretical advances^{20,21,22}, our simulations and theoretical developments show that stimulated Raman processes could pave the way to generate OAM light in nonlinear optical media and that the nonlinear optics of plasmas^{23,24} could provide a path to generate and amplify OAM light to relativistic intensities^{25,26,27,28}.
Results
Theoretical model
We illustrate our findings considering that the nonlinear optical medium is a plasma. Extension to other materials is straightforward. In a plasma, stimulated Raman backscattering is a threewave mode coupling mechanism in which a pump pulse (frequency ω_{0} and wavenumber k_{0}), decays into an electrostatic, or Langmuir, plasma wave (frequency ω_{p} and wavenumber 2k_{0}−ω_{p}/c) and into a counterpropagating seed laser (frequency ω_{1}=ω_{0}−ω_{p} and wavenumber k_{1}=ω_{p}/c−k_{0}). The presence of OAM in the pump and/or seed results in additional matching conditions that ensure the conservation of the angular momentum carried by the pump when the pump itself decays into a scattered electromagnetic wave and a Langmuir wave^{29}. These additional matching conditions, which are explored in more detail in Supplementary Notes 1–4 and Supplementary Figs 1–3), correspond to selection rules for the angular momentum carried by each laser and plasma wave. Here we illustrate key properties of OAM generation and amplification by exploring different seed and pump configurations.
In order to derive a model capable of predicting stimulated Raman scattering OAM selection rules, we start with the general equations describing stimulated Raman scattering, given by , and , where , D_{p}=2iω_{p}∂_{t}, and where the minus (−) sign is used to describe the seed pulse evolution. Moreover, A_{0,1} is the envelope of the pump/seed laser, with complex amplitude, given by , where t is the time and z the propagation distance. We note that A_{0,1} are arbitrary functions of the transverse coordinate r_{⊥}. The complex amplitude of the plasma density perturbations is , where k_{p}=ω_{p}/c is the plasma wavenumber, the plasma frequency, m_{e} the mass of the electron, the vacuum electric permittivity and e the elementary charge. Although these general equations can be used to retrieve the selection rules for the OAM that will be explored throughout this paper, it is possible to derive exact solutions in the long pulse limit, where and in the limit where the pump laser contains much more energy than the seed laser energy. In this case, since , and (pump has more energy than seed), then (this condition is strictly satisfied in our simulations when new modes are created and until their energy becomes comparable to the energy in the pump pulse). In this case, it is possible to show that stimulated Raman scattering of a seed beam A_{1} from a pump beam A_{0} creates a plasma wave density perturbation, given by:
where Γ is the growth rate at which the plasma amplitude grows as the interaction progresses and r_{⊥} is the transverse position. The amplification of the seed is given by:
where (ω_{1}, k_{1}) are the frequency and wavenumber of the seed laser pulse, respectively, and C is a constant of integration. The derivation of equations (1)–(3), , , presented in detail in Supplementary Note 1, assumes that the pump and the seed satisfy the frequency matching conditions stated above, being valid for arbitrary transverse laser envelope profiles as long as the paraxial equation is satisfied. Neglecting pump depletion does not change the selection rules for the OAM, as discussed in the remainder of this work. Unless explicitly stated, the generic expression for the pump vector potential (or electric field) is , where (e_{x}, e_{y}) are the unit vectors in the transverse x and y directions, and φ the azimutal angle. Similarly, the generic expression for the seed vector potential is . Selection rules can then be generally derived by inserting these expressions into the factor (A_{1}(t=0) ˙ A_{0}*)A_{0} in equation (3). Although we have assumed that the plasma is the optical medium, other nonlinear optical media with Kerr nonlinearity will also exhibit similar phenomena.
PIC simulations
We will now use equation (3) to explore OAM generation and amplification in three separate classes of initial setups, all identified in Fig. 1. We start by studying the case of the amplification of existing OAM modes. Figure 1a illustrates the process in a setup leading to the amplification of a seed in an arbitrary, single state of OAM in a plasma using a counterpropagating Gaussian pump laser without OAM. The mechanism is trivially generalized for a pump with arbitrary OAM . We can then assume a pump linearly polarized in the x direction with OAM , which decays into a Langmuir plasma wave with OAM and into a seed, also linearly polarized in the x direction with OAM . Making these substitutions into equation (3) confirms that the amplification of A_{1} retains the initial seed OAM. For the specific example in Fig. 1a, where , direct substitution of and in equation (1) shows that the plasma wave density perturbations have OAM , that is, the plasma wave absorbs the excess OAM that may exist between the pump and the seed (see Supplementary Note 2 and Supplementary Fig. 1 for several examples illustrating angular and linear momentum matching conditions, demonstrating that the plasma wave always absorbs the excess OAM between pump and seed.) The scheme is thus ideally suited to amplify an existing OAM seed using a long Gaussian pump without OAM. The amplification of circularly polarized OAM lasers, with both spin and OAM, obeys similar selection rules. For amplification to occur in this case, and similar to stimulated Raman backscattering of circularly polarized Gaussian lasers, both seed and pump need to be polarized with the same handedness either in e_{+}=e_{x}+i e_{y} or in e_{−}=e_{x}−i e_{y}.
Figure 2a illustrates 3D simulation results showing the amplification of an , linearly polarized seed from a linearly polarized Gaussian pump. Simulation parameters are stated in Table 1. Figure 2a shows that the growth rate for the amplification process is nearly indistinguishable from stimulated Raman amplification of Gaussian lasers. In agreement with equation (2), this result also indicates that, in general, the overall amplification process is OAMindependent.
Stimulated Raman scattering also provides a mechanism to create new OAM modes (that is, modes that are absent from the initial pump/seed lasers) and amplify them to very high intensities. Figure 1b illustrates the process schematically. The pump electric fields can have different OAM components in both transverse directions x and y. Each component is represented in blue and orange in Fig. 1b. The pump electric field component in x has OAM . The pump electric field component in y has OAM . The initial seed electric field contains an OAM component in the x direction. After interacting in the plasma, the pump becomes depleted and a new electric field component appears in the seed with OAM, given by .
The process can be physically understood by examining the couplings between the plasma and light waves in the example considered above. Initially, a plasma wave will be excited due to beating pump and seed components that have their electric fields pointing in the transverse x direction. According to equation (1), the plasma wave OAM is . This plasma wave ensures OAM conservation for the pump and seed electric field components in the x direction. The (same) plasma wave also couples the pump and seed modes with electric field components pointing in the y direction. Thus, must also hold in order to ensure conservation of angular momentum. This implies the generation of a new seed component with electric field polarized in y so that OAM is conserved at all times and in both components. The OAM of the new seed component is thus .
Alternatively, this selection rule can also be found by examining equation (3). Direct substitution of a pump profile with and of an initial seed profile with then leads to the generation of a new seed with . The same selection rules would also hold if the pump consists of combination of a right and lefthanded circularly polarized modes, each with different OAM, and the seed initially contains only a left or righthanded circularly polarized mode. In this case, a new seed component would appear with right or lefthanded circular polarization. The new mode is created to ensure conservation of OAM. The selection rules are identical as long as polarizations in e_{x}/e_{y} are replaced by polarizations in e_{+}/e_{−} (where e_{±}=e_{x}±i e_{y}). This setup provides a robust mechanism for the production and amplification of a new and welldefined OAM mode, absent from the initial set of lasers. The generation of a new OAM mode when a linearly polarized seed interacts with a pump with electric field components in the two orthogonal directions is also illustrated in Supplementary Note 3 and Supplementary Fig. 2.
Figure 3 shows a result of a 3D PIC simulation illustrating the production of a new seed mode with , which is initially absent from the simulation, from a pump with , and an initial seed with (simulation parameters given in Table 1). Figure 3 presents several distinct signatures of the new OAM mode with . The laser vector potential shows helical structures, which indicate that the new mode has OAM. The normalized vector potential forms a pattern that repeats each 3 turns, which turn in the clockwise direction from the front to the back of the pulse, a signature for . Field projections in the (x,y) plane also show a similar pattern further confirming that the new OAM mode has . The change in colour from blue–green in (a) to (green–red) in (b) is a clear signature for the intensity amplification of the new seed mode. Intensity was calculated using , where λ_{0}=0.8 μm is the central laser wavelength. Figure 3 also shows that the amplified laser envelope acquires a bowshaped profile^{21,22,30}, a key signature of Raman amplification identified in ref. 21. In agreement with theory (equations (2) and (3)), Fig. 2b shows that the new mode and the existing OAM mode amplify at nearly coincident growth rates. Still, since it grows from initially higher intensities, the existing mode reaches higher final intensities than the new OAM mode with . The generation of the new modes in Fig. 2b also illustrates the transition from the regime where the depletion of the pump is negligible (small signal and exponential growth) to the regime where the depletion of the pump is not negligible (strong signal and linear growth). Hence, Fig. 2b shows an exponential growth of the new mode up to z<0.6 mm. For z>0.6 mm, the energy in the new seed becomes comparable to the energy contained in the pump pulse. As a result, the growth slows down significantly, becoming linear with the propagation distance^{26}.
L. Allen et al.^{1} showed that particular superpositions of Hermite–Gaussian modes (also called transverse electromagnetic or TEM modes) are mathematically equivalent to Laguerre–Gaussian modes. Since the transverse amplitude distribution of highorder (transverse) laser modes is usually described by a product of Hermite–Gaussian polynomials, which is also usually associated with TEM modes, this result paved the way for experimental realization of vortex light beams with OAM from existing TEM laser modes. It is thus interesting and important to explore whether and how stimulated Raman backscattering can be used to generate and amplify light with OAM from Hermite–Gaussian laser beams, that is, from initial configurations with no net OAM. Figure 1c illustrates the process. From now on, we refer to each Hermite–Gaussian beam as a TEM_{m,n} laser, where (m, n) represents the Hermite–Gaussian mode. The TEM mode electric field is given by equation (5) (see Methods section). We consider first a Gaussian pump linearly polarized at 45°, that is, having similar electric field amplitudes in both transverse directions x and y. The Gaussian pump can then also be written as A_{0}∼TEM_{00}(e_{x}+e_{y}). In addition, we assume a seed with a TEM_{10} mode electric field component in x and with a TEM_{01} mode electric field component in y. The two seed modes are π/2 out of phase with respect to each other. The seed is given by A_{1}∼TEM_{10}e_{x}+iTEM_{01}e_{y}. This setup is represented in Fig. 1c, where blue and orange colours refer to the pump and seed components polarized in the x and y directions, respectively.
Although this setup has no initial OAM, since both pump and seed have no OAM, it results in the generation and amplification of an OAM mode with . In order to understand the OAM generation mechanism, we first consider equation (1). According to equation (1), the beating between the TEM_{10} seed with the Gaussian pump in the x direction will drive a TEM_{10} daughter plasma wave component. The beating between the iTEM_{01} seed and Gaussian pump in the y direction will drive a iTEM_{01} daughter plasma wave component. These two plasma wave components are π/2 out of phase with respect to each other. Hence, the resulting plasma wave will be a combination of TEM modes given by δn∼TEM_{10}−iTEM_{01}, where the i denotes the phase difference between modes. According to ref. 1, this mode combination is equivalent to a Laguerre–Gaussian mode with . In order to conserve angular momentum, a new seed component with will then have to be generated and amplified in the direction of polarization of the pump. This process is also illustrated in Supplementary Note 4 and Supplementary Fig. 3.
It is also possible to reach this conclusion by substituting in equation (3) the expressions for initial Gaussian pump transverse profile [A_{0}∼TEM_{00}(e_{x}+e_{y})] and initial TEM seed profile (A_{1}∼TEM_{10}e_{x}+iTEM_{01}e_{y}). This substitution yields a new seed transverse profile given by A_{1}∼(TEM_{10}+iTEM_{01})(e_{x}+e_{y}), corresponding to a Laguerre–Gaussian mode with (ref. 1). Similarly, a circularly polarized Gaussian pump and a A_{1}∼TEM_{10}e_{x}+TEM_{01}e_{y} seed (that is, without phase difference between the TEM_{10} and TEM_{01} modes) would also lead to a new seed component with . The plasma can then be viewed as a highintensity mode converter.
Figure 4 shows results from a 3D simulation that confirms these predictions (see Table 1 for simulation parameters). The simulation setup follows the example of Fig. 1c described earlier. Simulations show that stimulated Raman scattering leads to a new OAM mode with linearly polarized at 45°. Figure 2c shows that the amplification rates are comparable to the other typical scenarios shown in Fig. 2a,b. The change on the field topology of the seed normalized vector potential shown in Fig. 4, from plane isosurfaces to helical isosurfaces, indicates the generation of a laser with OAM from a configuration with no net OAM. Normalized vector potential isosurfaces, and projection in the yz direction, form a pattern that repeats each turn and that rotates clockwise from the front to the back of the pulse, thereby indicating an OAM with .
Discussion
We have so far assumed that the lasers are perfectly aligned. In experiments, however, the beams can only be aligned within a certain precision. In the presence of misalignments, our results will still hold as long as Raman sidescattering can be neglected, that is, when the angle between the two pulses is much smaller than 90°. The kmatching conditions are then still satisfied in the presence of small misalignments because the nonlinear medium, a plasma in the case of our simulations, absorbs any additional transverse wave vector component. Thus, momentum is still locally conserved, thereby allowing for Raman backscatter processes (interestingly, we note that when using OAM beams, the wave vectors of seed and pump are already locally misaligned). Despite lowering the total interaction time, and possibly the final amplification level, a small angle between the seed and pump will not change the OAM selection rules and the overall physics of stimulated Raman scattering.
We note that our seed laser pulse final intensity, on the order of 10^{17} W cm^{−2}, and seed laser spot size, on the order of 1 mm, indicate the production and amplification of Petawatt class twisted lasers with OAM. Additional simulations (not shown) revealed the generation and amplification of circularly polarized OAM modes using a scheme similar to that in Fig. 1b. Moreover, simulations showed that Raman amplification can also operate in the absence of exact frequency/wavenumber matching between seed and pump as long as the seed is short so that its Fourier components can still satisfy k and ωmatching conditions.
Finally, we note that our results could be extended to other nonlinear optical media with Kerr nonlinearities. In a plasma, the coupling between seed and pump is through an electron Langmuir wave, which also ensures frequency, wavenumber and OAM matching conditions will hold. In other nonlinear optical media, molecular vibrations, for instance, would play the role of the plasma Langmuir wave. We note that the possibility of OAM transfer has been explored in solids^{18}. Similar phenomenology as illustrated in this work could also be obtained in threewave mixing processes, where an idler wave could play the role of the plasma Langmuir wave. One advantage of testing these setups in nonlinear Kerr optical media such as a crystal is that lasers with much lower intensities could be used (see Supplementary Note 5 for a discussion in nonlinear optical media with Kerr nonlinearity admitting threewave interaction processes). The plasma, however, offers the possibility to amplify these lasers to very high intensities. This scheme could also be used in combination with optical pulse chirped pulse amplification to pregenerate and preamplify new OAM modes via stimulated Raman scattering before they enter the plasma to be further amplified. Similar configurations (for example, stimulated Brillouin backscattering^{31}) can also be envisaged to produce intense OAM light.
Methods
Setup of numerical simulations and simulation parameters
Simulations have been performed using the massively parallel, fully relativistic, electromagnetic PIC code OSIRIS^{19}. In the PIC algorithm, spatial dimensions are discretized by a numerical grid. Electric and magnetic fields are defined in each grid cell and advanced through a finite difference solver for the full set of Maxwell’s equations. Each cell contains macroparticles representing an ensemble of real charged particles. Macroparticles are advanced according to the Lorentz force. Since background plasma ion motion is negligible for our conditions, ions have been treated as a positively charged immobile background. The plasma was initialized at the front of the simulation box that moves at the speed of light c. Note that although the simulation are performed in a frame that moves at c, the moving window corresponds to a Galilean transformation of coordinates where all computations are still performed in the laboratory frame. The simulation box dimensions were 50 × 2,870 × 2,870 μm, it has been divided into 650 × 2,400 × 2,400 cells and each cell contains 1 × 1 × 1 particles (3.7 × 10^{9} simulation particles in total). Additional simulations with 1 × 2 × 2 particles per cell showed no influence on our conclusions and simulation results. The pump laser was injected backwards from the leading edge of the moving window^{32,33}. In order to conserve canonical momentum, the momentum of each plasma electron macroparticle has been set to match the normalized laser vector potential. The particles are initialized with no thermal spread.
The initial OAM seed and pump laser electric field is given by:
where c.c. denotes complex conjugate, E_{0}=(E_{0x}, E_{0y}) is the laser electric field at the focus, with (E_{0x}, E_{0y}) being the electric field amplitudes in the transverse x and y directions, respectively. For a linearly polarized laser, there is no phase difference between E_{0x} and E_{0y}. For circularly polarized light, both components are π/2 out of phase, that is, E_{0x}=±iE_{0y}. In addition is the waist of the beam as a function of the propagation distance z in vacuum, w_{0} the waist at the focal plane, the Rayleigh length, and λ=2πc/ω=2π/k the central wavelength of the laser, ω and k are its central frequency and wavenumber, respectively. In addition, is a generalized Laguerre polynomial with order , with being the index that gives rise to the OAM, the radial distance to the axis, θ_{0} an initial phase and z_{0} the centre of the laser. We note that all simulations involving Laguerre–Gaussian modes have p=0. The initial electric field of an Hermite–Gaussian (TEM) laser is given by:
where H_{m} is an Hermite polynomial of order m. Moreover, the wavenumber of the pump laser (which travels in the plasma) in all simulations presented in Figs 2, 3, 4 is set according to the linear plasma dispersion relation , where is the plasma frequency associated with a background plasma density n_{0}, and where e and m_{e} are, respectively, the elementary charge and electron mass. The seed frequency and wavenumber are set according to the matching conditions for Raman amplification (Table 1).
Additional information
How to cite this article: Vieira, J. et al. Amplification and generation of ultraintense twisted laser pulses via stimulated Raman scattering. Nat. Commun. 7:10371 doi: 10.1038/ncomms10371 (2016).
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Acknowledgements
This work was supported by the European Research Council through the Accelerates European Research Council project (contract ERC2010AdG267841), Fundação para a Ciência e para a Tecnologia, Portugal (contract EXPL/FIZ PLA/0834/1012) and the European Union (EUPRAXIA grant agreement 653782). We acknowledge PRACE for access to resources on SuperMUC (Leibniz Research Center).
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Vieira, J., Trines, R., Alves, E. et al. Amplification and generation of ultraintense twisted laser pulses via stimulated Raman scattering. Nat Commun 7, 10371 (2016). https://doi.org/10.1038/ncomms10371
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DOI: https://doi.org/10.1038/ncomms10371
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