Direct Laser-Driven Electron Acceleration and Energy Gain in Helical Beams
A detailed study of direct laser-driven electron acceleration in paraxial Laguerre–Gaussian modes corresponding to helical beams with azimuthal modes is presented. Due to the difference between the ponderomotive force of the fundamental Gaussian beam and helical beams , we found that the optimal beam waist leading to the most energetic electrons at full width at half maximum is more than twice smaller for the latter and corresponds to a few wavelengths for laser powers of PW. We also found that, for azimuthal modes , the optimal waist should be smaller than . Using these optimal values, we have observed that the average kinetic energy gain of electrons is about an order of magnitude larger in helical beams compared to the fundamental Gaussian beam. This average energy gain increases with the azimuthal index leading to collimated electrons of a few 100 MeV energy in the direction of the laser propagation.
The well-known Laguerre–Gaussian () modes of paraxial light with integer radial and azimuthal, and , indices have a phase distribution of , where is the azimuthal angle. Here, corresponds to the azimuthal or rotational order of the mode with a well-defined orbital angular momentum (OAM) of per photon . Such higher-order modes lead to twisted light by forming an optical vortex in the direction of propagation associated with the optical phase singularity. The spiral shape of the wavefront is formed by interconnected helices; hence, beams are called helical beams.
These distinctive properties of higher-order Laguerre–Gaussian modes set forth to an ever-increasing amount of applications in different areas of optical communications, imaging techniques, quantum information technologies, and other topics; see [2–6] and references therein.
In recent years with the development of ultraintense multi-PW laser technology, Laguerre–Gaussian laser modes have other potential applications in the fields of plasma accelerators and inertial confinement fusion and in the generation of X-rays and -rays with OAM [7–14]. In particular, it has been shown that, in laser wakefields driven by helical pulses, the wakefield shows a donut-like structure with a ring-shaped hollow electron beam . Furthermore, for a lower-density plasma or a smaller laser spot size, besides the donut-like wakefield, a central bell-like wakefield forms in the center of the donut-like wake. On the contrary, further reducing the plasma density or laser spot size leads to an on-axis electron beam acceleration only.
It was also demonstrated that Laguerre–Gaussian beams transfer a part of their OAM to electrons through the dephasing process similar to the direct electron acceleration (DLA) in Gaussian beams . Furthermore, the propagation of optical beams with OAM leads to plasma waves that may also carry OAM which couple to the plasma electrons and involve Landau damping and particle acceleration accompanied with the generation of quasi-static axial and azimuthal magnetic fields . When Laguerre–Gaussian plasma waves are subjected to Landau damping, a higher azimuthal mode number leads to a larger OAM transfer to particles traveling close to the phase velocity of the plasma wave . Vacuum-based charge acceleration with Laguerre–Gaussian beams has also been studied very recently [18, 19] showing that it is possible to generate GeV high-quality electron bunch with low spread in energy and radial deflection.
Motivated by these interesting results, in this paper, we will study direct electron acceleration in vacuum in various helical Laguerre–Gaussian laser pulses corresponding to helical modes . Laser beams with and define the fundamental Gaussian mode, while beams with and have a hollow ring-like transverse intensity profile with zero intensity at the center. The central hollowness corresponds to a potential well which confines/accelerates the electric charges through the transverse/longitudinal ponderomotive forces.
This type of ponderomotive trap is also realized using higher-order transverse electromagnetic modes (TEMs), i.e., the Hermite–Gaussian modes, such as or the combination of with . This ponderomotive potential is similarly axisymmetric and has a minimum on the axis [20–24]. This is certainly expected since orthogonal Hermite–Gaussian modes may be decomposed into Hermite–Gaussian modes with a phase difference, and vice versa; see [1, 25] for the general formulas.
Here, we specifically focus our study on the energy gain in femtosecond lasers of low to very high intensity, thereby gaining valuable estimates about relevant parameters for lasers operating at ELI-NP . Our results are based on the 3-dimensional numerical solution of the relativistic equations of motion for free electrons in paraxial laser fields. Henceforth, similarly as in very low-density plasmas, in DLA, we also observe collimated and intertwining electron beams in the direction of the laser propagation, while in addition, we also show that the average energy gain increases with the azimuthal mode index .
Furthermore, we found that the optimal beam waist leading to the most energetic electrons is more than twice smaller in case of higher-order Laguerre–Gaussian beams than in case of the fundamental Gaussian beam that was presented in . For lasers of PW power, the optimal beam waists are and correspond to peak intensities, while taking into account the intensity profiles of the beams, these values are reduced by for . Using these optimal values, we have observed that, for the same laser power, the average kinetic energy gain of electrons is about an order of magnitude larger in helical beams compared to the fundamental Gaussian beam.
This paper is organized as follows. In Section 2, we present some of the characteristic properties of helical beams, the equations of motion for electrons, and the initial conditions corresponding to our study. In Section 3.1, we have estimated the optimal values of beam waist leading to the most energetic electrons for given laser power. Applying these optimal values, we present and discuss the electron dynamics and energy gains in linearly polarized (LP) and circularly polarized (CP) helical beams in Section 3.2. The conclusions are summarized in Section 4.
2. Direct Laser-Driven Electron Acceleration in Helical Beams
2.1. Laguerre–Gaussian Beams
A well-known solution [28, 29] to the paraxial wave equation is obtained in cylindrical coordinates , with the help of generalized Laguerre polynomials. This solution is cylindrically symmetric around the axis of propagation , with radius and azimuth , expressed in Cartesian coordinates. These are the Laguerre–Gaussian () beams [1, 10, 12], with radial index and azimuthal index . The general expression for the electric field distribution of a monochromatic pulse iswhere is the wavenumber, is the speed of light in vacuum, is the angular frequency, is the amplitude of the electric field, and is the initial phase. Furthermore, is the Rayleigh range, is the radius of curvature, and is the Gouy phase. The beam waist is defined aswhere the beam waist radius at focus is .
The Laguerre polynomials are denoted by , and the normalization constant, , follows from the orthonormality of the Laguerre polynomials . The fundamental Gaussian beam is obtained for , where .
The components of the electric and magnetic fields arewhere and such that or in case of linear polarization along the -axis or -axis, respectively, and for circular polarization, while elliptic polarization, otherwise.
The longitudinal components of the electric and magnetic fields are calculated from Maxwell’s equations, ; thus, in the paraxial approximation,
Therefore, the electromagnetic field of Laguerre–Gaussian pulses is given bywhere the Gaussian temporal envelope with duration and peak intensity position at reads 
Note that there are more appropriate choices for the temporal profile such as the hyperbolic secant ; see [32–34] for more details. Using this profile, we found that the energy gain may be reduced by as much as compared to Gaussian.
2.2. Helical Beams
The Laguerre–Gaussian beams, , with nonzero azimuthal modes contain a phase change given by . Note, however, that, for all modes, the generalized Laguerre polynomials have a contribution equal to one, i.e., . These type of Laguerre–Gaussian beams, , are the helical beams associated with the nonzero OAM of light [1, 35].
In Figure 1, the normalized intensity profiles of linearly polarized fundamental Gaussian and different helical beams are shown as a function of radial distance, in units of beam waist radius . These plots represent using equation (1), for and , while the intensity is .
The intensity of -modes is largest for corresponding to the fundamental Gaussian beam, and it is decreasing with an increasing number of azimuthal modes. Due to the factor, all modes with have zero intensity at the center, , that is known as an optical vortex or phase singularity on the axis.
The intensity profiles of Gaussian beams are concave functions on the whole interval. The intensity of helical beams is independent of and has a convex part with maxima at after which the functions change from convex to concave. The width of the convex part widens with increasing azimuthal index , while using the positions of maxima, the intensity peaks of -modes relative to fundamental Gaussian lead, , as shown in Figure 1.
2.3. Electron Acceleration in the Electromagnetic Field
The motion of electrically charged particles in an external electromagnetic field is governed by the Lorentz force, , and leads to the following set of nonlinear differential equations :
Here, is the electron’s charge, the Cartesian coordinates and normalized velocity are denoted by and , while the Lorentz factor is .
The four-momentum of the electron is , where is its invariant rest mass. The relativistic energy and momentum of electrons are expressed as
Laser-driven electron acceleration in vacuum is the consequence of the direct interaction of the laser pulse with electrons [37–46]. At any given time, equations (8) and (9) are input for the electromagnetic field of the laser pulse, i.e., equations (5) and (6); hence, the trajectory of the propagating electric charge dynamically maps the laser pulse.
The 3-dimensional solutions to the electron trajectories and velocities are obtained by solving these coupled differential equations numerically by an adaptive time-step Runge–Kutta method with an accuracy and numerical precision up to 12 digits.
2.4. Initial Conditions
Unless stated otherwise, initially, all electrons are at rest, i.e., and . These electrons at coordinates are uniformly distributed in the orthogonal plane, , on a disk with a radius that is three times the beam waist radius, i.e., . Thus, initially, over 99% of the laser’s energy is contained within this disk. The initial position of the peak of the laser pulse is located on the longitudinal axis at behind the electrons, i.e., full pulse interaction, while all electrons are independent from each other and only interact with the laser pulse .
For current purposes, we have fixed the laser wavelength to nm. The laser pulse duration at full width at half maximum (FWHM), fs, corresponds to . Similarly, the beam waist at FWHM leads to waist radius.
The peak intensity and peak power for a monochromatic LP Gaussian laser are and , where the normalized electric field amplitude is . For PW power and beam waists of , these values are listed in Table 1. For helical beams, the field intensities at the local maxima are since the total power of the beam is constant, .
3.1. Optimal Beam Waist
First of all, we are interested in the values of the beam waist for different laser powers that lead to maximal energy gains, in case of the Gaussian beam and the helical beams , , , and .
The energy gain of electrons interacting with an laser pulse is a function of the initial location of electrons, the laser spot size, and azimuthal mode . To estimate the value of the beam waist that correspondingly leads to maximum energy gains for a given laser power, we have varied the initial position of electrons uniformly at and calculated the respective energy gain of a single electron for each position:where . Furthermore, for all discrete values of beam waist , we have also calculated the average of these energy gains, , where corresponds to the number of the initial positions of electrons in the transverse plane.
These weighted averages for different laser powers are shown in Figure 2 for both LP and CP pulses. Here, the average energy gains corresponding to laser powers of PW are plotted with red, blue, and black, as a function of initial spot size. The full and dashed lines correspond to CP and LP lasers, respectively.
First, we discuss these results qualitatively. For a given laser power, the amplitude of the electron oscillations along the polarization direction increases with intensity. Increasing the beam waist decreases the intensity, and the scattering of electrons decreases; hence, they remain confined in the pulse being able to gain more energy from the laser, until the oscillations become larger than the waist and the electron scatters out from the pulse.
On the contrary, increasing the waist of the beam also decreases the longitudinal components of the electric field and the Lorentz force, i.e., and , and therefore reduces the net kinetic energy gain of electrons. The electrons are accelerated to larger and larger velocities in the front part of the pulse, and thus, the electron trajectories are elongated in the direction of the laser propagation, while the deceleration in the back part of the pulse becomes less efficient.
This means that the beam waist corresponding to the highest average energy gain, i.e., the highest peaks of the averages in Figure 2, represents the optimal waist for the given laser power and polarization. For larger power lasers, a wider initial beam waist is more optimal to ensure that the electrons remain confined inside the pulse to gain more energy.
Therefore, using Figure 2, we can approximate the beam waists corresponding to the peaks in net energy gain. In case of the fundamental Gaussian beam, the optimal beam waist at FWHM corresponds to few tens of wavelengths, , for laser powers of PW, such that the net energy gain increases about for every order of magnitude increase in laser power. Even with those optimal values, the average energy gain of only a few MeV was observed in beams; see  for more details. Note also that, in case of the Gaussian pulse, the outcome is independent on the polarization, and the averaged results overlap. This behavior is similar for the helical beam, but for higher modes, the distinction between CP and LP pulses becomes more apparent.
Now, averaging the energy gains of the helical beams and for a circularly polarized laser from Figure 2, we have approximated the optimal beam waists at FWHM. These optimal beam waists are corresponding to increasing laser power of PW. These approximated values represent the chosen optimal values for direct electron acceleration in all helical beams of interest, . Note, however, that the optimal beam waist also reduces slightly as the mode number increases (see Figure 2). Therefore, the previously chosen beam waists are suboptimal for and modes where even a smaller beam waist would be more favorable for larger energy gains.
The most important observation in case of CP beams is that the optimal spot sizes of helical beams are more than twice smaller than for the fundamental Gaussian beam. In case of LP beams, this difference further increases with the mode index . Furthermore, for these relatively tight initial waists, of a few wavelengths, the helical beams might lead to almost an order of magnitude larger net energy gains compared to the fundamental Gaussian beam at high laser power.
A straightforward explanation can be formulated in terms of the ponderomotive force, , where the ponderomotive potential, the cycle-averaged oscillation energy, is directly proportional to the intensity, , shown in Figure 1. The ponderomotive force causes the charges oscillating in an inhomogeneous electric field to drift from where the electric field is larger to where it is smaller. Therefore, the immediate consequence of the transverse ponderomotive force is the scattering of charges from “regions” of higher to lower electric field intensity. Due to the fact that the intensity of the helical beams has a wide convex region, the charges found in this region are naturally driven to the beam center with zero intensity.
In other words, the transverse ponderomotive force in Gaussian beams is always positive; hence, the electrons are scattered outwards from the pulse. In helical beams, the transverse ponderomotive force of the convex region is negative, and hence, the electrons are effectively trapped inside the “hollow” pulse (see Figure 1). This leads to less spread, better focusing, and collimated electron trajectories confined near the axis of propagation. These captured electrons are accelerated further by the longitudinal ponderomotive force while continue to gain more energy through the phase synchronization process leading to larger energy gains; see  for more details.
3.2. Energy Gain for Optimal Beam Waists
Using the previously given initial conditions together with the optimal values listed in Table 1 for both CP and LP lasers of PW power and initial beam waist of , we have numerically calculated the direct laser-driven electron acceleration corresponding to the fundamental Gaussian and helical beams with azimuthal modes .
In Figure 3, we have plotted all Cartesian components of the electric field as a function of time in units of the normalized field intensity as mapped by accelerated electrons with lower index . In beams, the electrons are accelerated at the front part of the pulse, but without reaching the available peak intensity of the pulse, the electrons are scattered out by the transverse ponderomotive force. In helical beams, e.g., and , the available “peak” intensities are about 2.5 and 5.5 times smaller than in . However, these intensity maxima are located further away from the midpoint, i.e., , the location of maximum intensity of the Gaussian beam and zero intensity for the helical beams (see Figure 1). Therefore, the electrons found in the convex part of the pulse are captured and accelerated for a much longer time, being clearly visible in Figure 3, where the time axes of the electric field components are an order of magnitude longer for the helical beams. This also means that the trajectories of some electrons captured by helical beams are up to an order of magnitude longer in the direction of the laser propagation. Furthermore, as apparent in Figure 3, the electrons also have a twisted circular motion with intertwining trajectories, similar as presented in .
To further elucidate these issues, in Figure 4, we have plotted the net energy gain of electrons as a function of the initial radial distance, , at the origin , for varying laser power. Here, all figures correspond to an initial beam waist of , while CP and LP pulses are plotted with “o” and “x,” respectively. Similar to the previously presented figures, red, blue, and black correspond to PW laser power. Figures 4(a0) and 4(b0) correspond to Gaussian beams, while Figures 4(a1) and 4(b1) are for helical beams . Similarly, the helical beams, , and , , with different polarizations are shown.
Here, we observe that the net energy gain as a function of the initial radial distance also reflects the initial intensity profiles shown in Figure 1. The intensity of the Gaussian beam falls off exponentially as a function of the radius; hence, the electric charges found further away from the center gain less and less energy. In the case of the helical beams, the largest acceleration occurs within the convex part of the intensity curves. Furthermore, as the distance between the center and the intensity peak widens with the azimuthal index, the peaks in intensity of the helical beams are also decreasing (see Figure 1). This explains why there is less and less net energy gained around the middle of the helical beams with increasing mode index (see Figure 4).
In Figure 5, the histograms of the energy and the polar angle of electrons are shown after the interaction with the pulse. Here, the 3-dimensional polar angle is , where is the radial distance from the origin. All histograms correspond to a CP laser of PW power and spot. In Figure 5, (a0), (b0) and (a1, b1) show the histograms of energy and polar angle corresponding to and beams. Similarly, Figures (a2), (b2), (a3), (b3) and (a4), (b4), (a5), (b5) show the outcome from the helical beams , and , .
These histograms once again reflect the difference in the ponderomotive force and its influence on the energy gain as well as the angular distribution of electrons. Due to the interaction with the pulse, the electrons have scattered out with polar angle. In case of the fundamental Gaussian beam, this polar angle is predominantly in the direction orthogonal to the direction of laser propagation, i.e., degrees. For helical beams with increasing azimuthal mode, we observe an increasing number of electrons that are scattered parallel to the longitudinal axis, at polar angles of degree, and, at the same time, fewer electrons in the orthogonal directions. This obviously means that helical beams lead to a larger number of collimated electrons than fundamental Gaussian beams, while their number is also increasing with increasing mode index.
Furthermore, the distribution of energy gain is also different in helical beams. The electrons are distributed following a multimodal distribution, leading to at least a second peak at finite energy at about 150 MeV energy for the helical beams, , , and . Although, here, we have only shown the results for the PW laser, a very similar behavior is observed for the PW laser, with a peak at about 50 MeV energy. For a PW laser, the intensities of the helical beams are so weak such that these striking differences disappear.
In Figures 6–8 corresponding to initial beam waists of , , and , we have plotted the average net energy and the largest energy gained, , both from circularly and linearly polarized pulses. Here, the average energy is calculated from , where is the number of electrons. These averages are shown with full lines for circularly polarized and with dotted lines for linearly polarized lasers. Similar as before, red, blue, and black, respectively, represent the power of the laser PW. In Figures 6–8, (a0) and (b0) show the average energy gained within the fundamental Gaussian beams, while Figures (a1) and (b1) show the same for the helical beams with given waist. Figures (a2) and (b2) correspond to , while Figures (a3) and (b3) correspond to . Similarly, Figures (a4), (b4) and (a5), (b5) present the outcome for and helical beams.
We observe that the mean energy gain of electrons for any given laser power is largest for an optimal waist, and this optimal waist is increasing with increasing laser power. Therefore, for a PW laser, the optimal waist size is , compare the mean energies, i.e., the red lines, in Figures 6–8. Similarly, by comparing the blue lines, for a PW laser, the waist size that leads to the largest energy gains is , while for a PW laser, the optimal waist size is , in accordance with the results of Section 3.1.
On the contrary, we also recognize that the average energy gain in helical beams is increasing with increasing azimuthal index . This is evident by comparing the blue and black lines in Figures 6–8. For a larger initial waist, there is larger energy gain for higher laser power. However, in Figure 8, we also observe that, for the largest waist and largest laser power, the average energy is increasing up to , while it is decreasing for higher modes. This was somewhat expected based on Figure 2, meaning that, for the highest power lasers with modes, the optimal waist should be smaller than .
The effect of laser polarization on energy gain is a delicate matter as already suggested by Figure 2. The average net energy gain in fundamental Gaussian beams is largely independent on the polarization. However, for helical beams, the outcome is different in each case depending on the beam waist and mode index, and therefore, the difference is from a few percent to up to . We have also observed that a larger average energy gain slightly favors the circularly polarized helical beams with mode indices for any beam waist and laser power. For linearly polarized helical beams, the optimal waist size should be slightly smaller than in the circularly polarized case to obtain similar energy gains, as can be concluded from the results.
The average net energy gain in Gaussian pulses, for the highest laser power and largest waist, is less than 2 MeV, while the highest energy electrons are MeV (see Figure 8). As previously discussed, the energy gains in fundamental Gaussian pulses may be a little higher for optimal beam waists , but even so, these values are easily surpassed in helical beams leading to an average of about a few and up to 45 MeV, and, in some cases, with highest energy electrons of MeV or more. Such energy gains are still below than the so-called ponderomotive limit [21, 47], where the intensity maxima of higher-order helical beams can be more than 5 times lower than those of Gaussian beams.
In this paper, we have studied and compared the direct laser-driven electron acceleration in Laguerre–Gaussian beams with azimuthal mode indices, corresponding to the fundamental Gaussian beam, and helical beams , , , , and .
We have found that the acceleration of electrons from rest is vastly different in helical beams compared to the fundamental Gaussian beam, mainly due to the difference in ponderomotive forces. Most importantly, for relatively tight initial waists, the helical beams lead to at least an order of magnitude larger energy gain compared to the fundamental Gaussian beam, and this energy gain also increases with the azimuthal mode .
For laser powers of PW, the optimal waist of helical beams leading to the most energetic electrons is more than twice smaller, , than in the case of the fundamental Gaussian beam . This also means that the beam waist that is optimal for helical beams is suboptimal for the Gaussian beam, and vice versa.
Finally, compared to Gaussian beams, the electron trajectories in helical beams are confined in the direction of the laser propagation leading to collimated electrons with trajectories that are at least an order of magnitude longer in the direction of the laser propagation. These conclusions hold for both linearly and circularly polarized lasers.
The data used to support the findings of this study are included within the article.
Conflicts of Interest
The authors declare that they have no conflicts of interest.
The authors are thankful to S. Ataman, D. Doria, J. F. Ong, K. Tanaka, and S. Tzenov for corrections and suggestions. E. Molnár thanks H. S. Ghotra for the comparison of early results and valuable discussions. D. Stutman acknowledges the support by a grant of the Ministry of Education and Research, CNCS-UEFISCDI (project no. PN-IIIP4-ID-PCCF-2016–0164), within PNCDI III. The authors are thankful for the financial support from the Nuclei Project (PN 19060105).
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