# Relativistic Propagation of Linearly/Circularly Polarized Laser Radiation in Plasmas

Authors: Sonu Sen; Meenu Asthana Varshney; Dinesh Varshney
Journal: ISRN Optics
 (2013)

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## Abstract

Paraxial theory of relativistic self-focusing of Gaussian laser beams in plasmas for arbitrary magnitude of intensity of the beam has been presented in this paper. The nonlinearity in the dielectric constant arises on account of relativistic variation of mass. An appropriate expression for the nonlinear dielectric constant has been used to study laser beam propagation for linearly/circularly polarized wave. The variation of beamwidth parameter with distance of propagation, self-trapping condition, and critical power has been evaluated. The saturating nature of nonlinearity yields two values of critical power of the beam (Pcr1 and Pcr2) for self-focusing. When P<Pcr1<Pcr2 the beam diverges. When Pcr1<P<Pcr2 the beam first converges then diverges and so on. When P>Pcr2 the beam first diverges and then converges and so on. Numerical estimates are made for linearly/circularly polarized wave applicable for typical values of relativistic laser-plasma interaction process in underdense and overdense plasmas. Since the relativistic mechanism is instantaneous, this theory is applicable to understanding of self-focusing of laser pulses.


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## Body

## 1. Introduction

The interaction of ultrahigh-power laser beams with plasmas is not only of technological importance but also rich in a variety of nonlinear phenomena. These phenomena become particularly interesting and involved when the laser power is sufficiently intense to cause the electron oscillation (quiver) velocity to become relativistic [1]. An important process that can affect the size of the focused spot of the radiation is self-focusing. In recent years the field of laser plasma interaction in the relativistic regime has been identified as an emerging area and is often referred to as high-field science. Several complex phenomena are included in the area of high-field science. These phenomena (on account of their nonlinear nature) are all significantly affected by the field distribution in the beam, and hence, self-focusing occupies a unique position in the field as it affects all other phenomena.Relativistic electron motion in a plasma due to an intense laser pulse modifies the refractive index and leads to two effects: relativistic induced transparency and relativistic self-focusing. In dense plasma withω<ωp, light cannot propagate and is reflected from the surface. However, for relativistic intensities generating large γ factors, the plasma becomes transparent. The dependence of the electron mass on intensity causes significant change of characteristic properties of the plasma and its nonlinear processes; the increase in effective electron mass decreases the electron plasma frequency and makes the penetration of electromagnetic waves into the overdense area of plasma, which is known as self-induced transparency or electromagnetically induced transparency, and is the cause of relativistic self-focusing. A combination of the relativistic self-focusing and relativistic induced transparency enables transmission of laser energy deep into plasmas which is useful for fast ignition of inertial fusion [2]. This so-called penetration sensitively depends on the focal position of the laser intensity due to the inhomogeneous density profile of the plasma and convergence of the laser pulse by final focusing optics.For ultrafast laser pulses lasting the order of a picosecond or less, the drift velocity of electrons in a plasma can be comparable to the velocity of light, causing a significant increase in the mass of the electron and consequently in the effective dielectric constant of the plasma. This leads to self-focusing of the laser beam, as pointed out [3]. The fact that the relativistic mechanism is the only mechanism of self-focusing that can manifest itself for subpicosecond pulses makes the understanding of this mechanism very important [4, 5]. The earlier analysis concerned with relativistic self-focusing of laser beams in plasmas ignored the effect of the saturating nature of the nonlinear dielectric constant and was essentially a perturbation treatment, based on the quadratic dependence of the dielectric constant on the electric field of the beam [6]. Hence, such an analysis has limited applicability to understand the self-focusing of beams with arbitrarily large electric field and consequently arbitrarily large nonlinear part of the dielectric constant.Relativistic focusing of radiation beams in plasma is applicable to pulse lengthτR in the range 1/ω<τR<rs/Cs, where Cs is the ion-acoustic speed [7], and can arise owing to the creation of a density depression in the plasma as well as to an increase in the electron mass due to relativistic effects. The time scale for self-focusing due to a density depression is longer than that for self-focusing due to relativistic mass increase. The latter time scale is τR≈ω-1, where ω is the radiation frequency and is assumed to be much greater than the electron plasma frequency. The analysis presented here will be concerned only with relativistic self-focusing on a time scale sufficiently short that the plasma density profile does not evolve significantly under the influence of the radiation beam. This implies that the pulse length τR of the radiation beam must be short compared with τs=rs/Cs (the time scale for the density depression to occur) and, of course, long compared with a radiation period τR. We make use of the steady-state paraxial-ray theory, as developed by Akhamanov et al. [8] and Sodha et al. [9].The organization of the paper is as follows. In Section2 the nonlinear dielectric constant due to relativistic variation of mass for a time-harmonic plane wave (i.e., a linearly/circularly polarized wave) is found. Section 3 is concerned with the relativistic self-focusing equation relating the variation of beamwidth parameter with distance of propagation. The self-trapping condition and the critical power are evaluated in Section 4. Results and discussion are made in Section 5.


## 2. Nonlinear Dielectric Constant of the Plasma

The relativistic equation of motion for a point charge is(1)ddt[mv(1-v2/c2)1/2]=e[E+(v×B)],
where m is the rest mass of a point charge, c is the velocity of light in vacuum, E is the electric field, and B is the wave magnetic field. For a homogeneous plane wave traveling in the direction of a unit vector n, the electric and magnetic vectors are perpendicular to n and are related by
(2)B=n×(Ec).
Substituting for B on the right-hand side of the equation of motion, (1) gives
(3)ddt[v(1-v2/c2)1/2]=em(1-n·vc)E+emc(E·v)n.
Considering the scalar product of (3) with n yields
(4)ddt[v(1-v2/c2)1/2]=emc(E·v).
Equation (4) together with the energy equation
(5)ddt[mc2(1-v2/c2)1/2]=eE·v
establishing that
(6)λ≡[1-n·v/c(1-v2/c2)1/2]
is constant. We now eliminate t in favour of the phase variable
(7)φ=ω(t-n·rc).
Here ω is the angular frequency of the wave, and r is the positive vector of the particle. Then
(8)v=drdt=ω(1-n·vc)r′,
where the prime denotes differentiation with respect to φ, and using (6)
(9)ddt[v(1-v2/c2)1/2]=λddt(v1-n·v/c)=ω2λ(1-n·vc)r′′.
Substitution of (8) and (9) into (3) enables the factor (1-n·v/c) to be cleared and leaves
(10)r′′=eλmω2[E+ωc(E·r′)n]
which is a second-order linear differential equation for r as a function of φ. The dielectric constant of the plasma is given by
(11)ε=1-(ωp2ω2)(mmr),
where  mr=γ·m is the relativistic mass, γ=(1-v2/c2)1/2 is the relativistic factor, and ωp=(4πn0e2/m)1/2 is the plasma frequency in the absence of the beam. For a circularly polarized wave, the components of (10) are
(12)x′′=eEcosφλmω2,y′′=-eEsinφλmω2,z′′=eEx′cosφ8m2λ2cω3,
where  φ=(ωt-kz) is the phase, and ω and k approximately satisfy the linear dispersion relation
(13)ω2=ωp2+c2k2.
Using (12), the average relativistic factor is
(14)〈γ〉=[1+e2E2m2ω2c2C1]1/2,
where
(15)C1=1+e2E216λ2m2ω2c2
for self-focusing considering the order of electric field up to second order and that the value of C1 is unity for circularly polarized wave [10] and half for linearly polarized wave. The dielectric constant can be written as [9]
(16)ε=ε0+ϕ(E0E0*),
where
(17)ε0=1-(ωp2ω2)
is the linear part of dielectric constant,
(18)ϕ(E0E0*)=ωp02ω2[1+(1-12αE0E0*C1)-1/2]
is the nonlinear relativistic term, and
(19)α=2e2m2ω2c2.
The effective dielectric constant for arbitrary large nonlinearity can be written as
(20)ε=ε0′-ε1(f)r2,
where f(z) is the dimensionless beamwidth parameter and ε0′ and ε1 represent, respectively, the linear and nonlinear dielectric constant for arbitrary nonlinearity.


## 3. Relativistic Self-Focusing Equation

Consider the propagation of Gaussian laser beam of frequencyω along z-direction; at z=0 the intensity distribution of the beam is given by
(21)EE*=E02exp(-r2r02),
and here, “r” is the radial coordinate of the cylindrical coordinate system, “r0” is the initial beamwidth,  and E0 is the axial amplitude. The wave equation governing the electric vector of beam in plasmas with the effective dielectric constant (20) is
(22)∇2E-∇(∇·E)+ω2c2εE=0.
To solve the prevoius equation, the Wentzel-Kramers-Brillouin (WKB) approximation has been used. In the WKB approximation, the second term ∇(∇·E) of (22) has been neglected, which is justified when (c2/ω2)|1/ε∇2lnε|≪1. The electric vector of the main beam can be expressed as
(23)∇2E+ω2c2εE=0.
In the presence of the modified background electron concentration due to relativistic nonlinearity, the intensity distribution of the beam inside the plasma can be obtained by using the WKB and paraxial ray approximations. Following Akhmanov et al. [8] and Sodha et al. [9] the solution for E can be written as
(24)E(r,z)=A(r,z)[k(0)k(f)]1/2exp(-i∫k(f)dz),
where
(25)k(f)=ωc[ε0′(f)]1/2,k(0)=ωc[ε0′(f=1)]1/2.
Substituting for E and ε from (24) and (20) in (23), one obtains
(26)-2ik(f)∂A∂z+∂2A∂r2+1r∂A∂r-ω2c2ε1(f)r2A=0.
Putting A=A0(r,z)exp[-ikS(r,Z)] in (26) and separating real and imaginary parts we get
(27)2(∂S∂z)+(∂S∂r)2+ω2c2ε1(f)k2(f)r2-1k2(f)A0(∂2A0∂r2+1r∂A0∂r)=0,(28)∂A02∂z2+∂S∂r∂A02∂r+A02(∂2S∂r2+1r∂S∂r)=0,
where S(r,z) is called the eikonal and related to the curvature of the wavefront. For a slightly converging/diverging beam the solution for a Gaussian laser beam (21) can be written as
(29)S=r22β(z)+φ(z),(30)A02=E02f2exp(-r2r02f2),
where
(31)β=1fdfdz.
It can be seen previously that β is the inverse of radius of curvature of the wavefront and r0f is the width of the beam. In the geometrical optics approximation, r=r0f(z) represents a ray in a plane containing the z-axis. On substituting for S into (27), using the paraxial ray approximation, such that (r/r0f)≪1, equating the coefficients of r2 on both sides of the resulting equations and substituting for β into (29), the dimensionless beamwidth parameter is given by
(32)k2(f)d2fdz2=1r04f3-ω2c2ε1(f)f.
Transforming the coordinate z and the initial beamwidth r0 to dimensionless forms
(33)ξ=(zcr02ω),ρ0=(r0ωc),
we get the characteristic beam propagation equation as
(34)d2fdξ2=1ε0′(f)f3-ρ02r02ε1(f)ε0′(f)f.
Physically, (34) governs the variation of beamwidth parameter f with distance of propagation. Substituting for E from (24) and S, A0, and β from (29)–(31) into (20) and using the paraxial ray approximation, ϕ can be written as
(35)ϕ(EE*)≈ϕ(k(0)k(f)E022f2)-r2{×(1+k(0)k(f)αE028λ22f2)]-3/2αωp02ω2k(0)k(f)E024r02f4×[1+k(0)k(f)αE022f2×(1+k(0)k(f)αE028λ22f2)]-3/2×[1+14λ2k(0)k(f)αE022f2][1+k(0)k(f)αE022f2(1+k(0)k(f)αE028λ22f2)]-3/2}
correct to terms in r2, where
(36)ϕ(k(0)k(f)E022f2)=ωp02ω2{0000000×(1+k(0)k(f)αE0216λ22f2)]-1/21-[1+k(0)k(f)αE022f2×(1+k(0)k(f)αE0216λ22f2)]-1/2}.
Equation (35) can put into the convenient form of (20), with [11]
(37)ε0′=ε0+ωp02ω2{1-[1+k(0)k(f)αE022f2(1+k(0)k(f)αE0216λ22f2)]-1/2×(1+k(0)k(f)αE0216λ22f2)]-1/2},ε1=αωp02ω2k(0)k(f)E024r02f4×{[1+k(0)k(f)αE022f2(1+k(0)k(f)αE028λ22f2)]-3/2×[1+14λ2k(0)k(f)αE022f2][1+k(0)k(f)αE022f2(1+k(0)k(f)αE028λ22f2)]-3/2}.
Consider second order of nonlinearity, for circularly polarized wave; we can rewrite the previous set of equations as
(38)ε0′(f)=1-ωp2ω2(1+k(0)k(f)αE022f2)-1/2,ε1(f)=ωp24ω2αE02r02f4(1+k(0)k(f)αE022f2)-3/2.
On substituting values of ε0′(f) and ε1(f) from (38) in (34), the equation governing the beamwidth parameter is
(39)d2fdξ2=1[1-ωp2ω2(1+k(0)k(f)αE022f2)-1/2]f3-ωp24ω2ρ02r02αE02r02f4(1+k(0)k(f)αE022f2)-3/2[1-ωp2ω2(1+k(0)k(f)αE022f2)-1/2]f.
In (39) the first term on right-hand side is responsible for diffraction divergence of the beam, and the second term corresponds to convergence, arising due to nonlinearity through the relativistic factor of linearly or circularly polarized beam, which contributes to focusing.


## 4. Self-Trapping Condition

When the two terms on the right-hand side of (39) balance each other the beam propagates without convergence or divergence, which is referred to as uniform waveguide propagation or self-trapping of the beam. For an initial plane wavefront of the beam the initial conditions on f are f(ξ=0)=1 and (df/dξ)ξ=0=0. As both the terms on right-hand side cancel each other hence at z=0, (d2f/dξ2)ξ=0=0; since (df/dξ) is also zero and f=1 at z=0, f=1 for all values of z; in other words beam can propagate without convergence or divergence. Therefore, the condition for self-trapping is(40a)ρ0Lin2=4ω2ωp2(1+αE02/2)3/2αE02/2
for linearly polarized beam and
(40b)ρ0Cir2=2ω2ωp2(1+αE02)3/2αE02for circularly polarized beam. The critical power of the beam is(41)P=c8π∫0∞ε1/2E0cr2exp(-r2r02)2πrdr,P=c8πr02E0cr2[ε0′(f=1)]1/2.


## 5. Results and Discussion

The differential equation (39) is to study the propagation of linearly and circularly polarized beams through plasma. We have chosen parameters accessible for interaction of such beams with moderately underdense plasma to slightly overdense plasma. The numerical values are chosen for laser intensity ranging between I = 1016 to 1018 W/cm2, electron density between 0.1 to 1.5 of critical density, laser frequency ω=1.7×1014 sec−1 and initial radius of the beam r0 laying between 1 to 3 μm. The dielectric function given by (20) and beam propagation equation (39) together with boundary conditions, are numerically solved. Further we consider the propagation of the beam in axially inhomogeneous plasma by including linear density variation in plasma.Figure1 shows the variation of relativistic factor γ versus intensity for linearly and circularly polarized laser beam. From the graph it is evident that the growth in relativistic factor for circularly polarized laser beam is more as compared to linearly polarized beam. Figure 2 shows plot of dielectric function versus axial intensity for linearly and circularly polarized beams in both underdense and overdense plasmas corresponding to different concentration of electron density. It is seen that initially there is an increase in dielectric function and after a certain value it attains a constant value. Because of very strong fields, the nonlinearity saturates. As a result the electromagnetic wave drives all of the plasma out of the regions of large field intensity and establishes equilibrium with radiation inside a vacuum channel surrounded by plasma. As we move from underdense region to overdense region the saturation effect slows down.Figure 1
Dependence of relativistic factor on axial intensity for linearly and circularly polarized laser beam.Figure 2
Variation of dielectric functionε as function of axial intensity for linearly (solid line) and circularly (dot line) polarized laser beam. Curves D0.7 and D1.2 correspond to (ωp/ω)2 = 0.7 and 1.2,  respectively.The critical curve (i.e., a plot of normalized radius of the beam “ρ0” against the axial intensity proportional to critical beam power) (40a) and (40b) is represented by Figure 3 for linearly and circularly polarized beams at Ωp2=(ωp/ω)2=0.7and1.2. Equations (40a) and (40b) have two critical powers Pcr1 and Pcr2, corresponding to two different values of electric field strength (or intensity of electric field), say Eocr1(orIocr1) and Eocr2(orIocr2) such that (Eocr1<Eocr2). The beam can be self-focused when its power P lies between the two critical values (Pcr1<P<Pcr2), and the range (Pcr2-Pcr1) increases rapidly with increasing normalized radius. The region above the critical curve (i.e.,Pcr1<P<Pcr2) is the self-focusing region, and region below the critical curve is known as the defocusing region. The effect of different concentration of electron density can be clearly seen from these critical curves. As concentration of electron density increases, that is, if we move from underdense region to overdense region the critical curve shifts downward.Figure 3
Critical curves, that is, the relation between dimensionless beam radiusρ0=(r0ω/c) and axial intensity for linearly (solid line) and circularly (dot line) polarized laser beam. Curves D0.7 and D1.2 correspond to (ωp/ω)2=0.7 and 1.2, respectively.Figures4(a) and 4(b) show the variations of dimensionless beamwidth parameter f with dimensionless distance of propagation ξ at relativistic intensity in plasma for different values of electron density in underdense and overdense plasmas. From the critical curves for Ωp2 = 0.7 (D0.7) and ρ0 = 4, the value (Pcr2/Pcr1)=113.22 for linearly/plane polarized beam, and (Pcr2/Pcr1)=113.21 for circularly polarized beam. At Ωp2=1.2 (D1.2) and ρ0=3, (Pcr2/Pcr1)=99.06 for linearly/plane polarized beam, and (Pcr2/Pcr1)=64.889 for circularly polarized beam. The beam shows focusing/defocusing for different values of P/Pcr1. This is because as we change the strength of the electric field, the maxima and minima get shifted. For a given value of ρ0 when (Pcr1<P<Pcr2), the second term on the RHS of (39) dominates the first term at z=0, and (d2f/dξ2) is negative; hence, f decreases with the distance of propagation.(a) Variation of beamwidth parameter(f) with dimensionless distance of propagation (ξ) for linearly (solid line) and circularly (dot line) polarized beams. Curves I, II, III, IV, V, VI, and VII correspond to (P/Pcr1) = 0.5, 5, 10, 20, 60, 100, and 200, respectively. Here (ωp/ω)2=0.7, ρ0=4,  and (Pcr2/Pcr1)=113.22 (for linearly polarized laser beam) and 113.21 (for circularly polarized laser beam). (b) Variation of beamwidth parameter (f) with dimensionless distance of propagation (ξ) for linearly (solid line) and circularly (dot line) polarized beams. Curves I, II, III, and IV correspond to (P/Pcr1) = 10, 60, 100, and 200, respectively. Here (ωp/ω)2=1.2, ρ0=3, and (Pcr2/Pcr1)=99.06 (for linearly polarized laser beam) and 64.89 (for circularly polarized laser beam).
(a)
(b)For certain value ofξ, the two terms on RHS of  (39) get cancelled resulting in (d2f/dξ2) = 0, and for larger values of ξ, RHS becomes positive. However, the beam still continues to converge on account of the curvature it has already gained, though (df/dξ) becomes less and less negative. At certain ξ, (d2f/dξ2)=0 and f=fmin. Beyond this point, the diffraction term dominates over the nonlinear term, and hence f exhibits the oscillatory behavior. From the figures it is evident that due to relativistic mass effect, increase in effective electron mass decreases the electron plasma frequency and makes the penetration of the beam into the overdense region of plasma, which is known as self-induced transparency. At higher concentration of electron density beam gets more focused as compared to low concentration of electron density. The variation of dimensionless axial intensity (αE02/f2)=(q0/f2) of the beam with distance of propagation ξ  corresponding to Figures 4(a) and 4(b) for self-focusing region is depicted in Figures 5(a) and 5(b). The intensity peaks for higher concentration of electron densities are higher with a reduced distance between two successive peaks.(a)  Variation of dimensionless axial intensity (q0/f2) with dimensionless distance of propagation (ξ) for linearly/plane (solid line) and circularly (dot line) polarized beams. Curves I, II, III, IV, and V correspond to (P/Pcr1) = 5, 10, 20, 60, and 100, respectively. Remaining parameters are as mentioned in Figure 4(a). (b) Variation of dimensionless axial intensity (q0/f2) with dimensionless distance of propagation (ξ) for linearly (solid line) and circularly (dot line) polarized beams. Curves I and II to (P/Pcr1)=10 and 60, respectively. Remaining parameters are as mentioned in Figure 4(b).
(a)
(b)Figure6(a) illustrates the variations of dimensionless beamwidth parameter f with distance of propagation ξ for different concentrations of electron densities in self-focusing region with linear increase in electron density. Careful observation of the results from figure indicates that for linearly increasing density plasma, minimum value of the normalized beamwidth parameter (fmin) for the second and higher orders decreases continuously in underdense and overdense plasmas. In underdense plasma it propagates long distance as compared to overdense plasma, but its focusing is less. The corresponding graph for variation of dimensionless axial intensity (q0/f2) of the beam versus distance of propagation ξ is shown in Figure 6(b). From the numerical analysis and graphs it is evident that both linearly polarized and circularly polarized beams can propagate through underdense plasma as well as they penetrate overdense plasma or say they exhibit self-induced transparency effect.(a) Variation of beamwidth parameter(f) with dimensionless distance of propagation (ξ) for linearly (solid line) and circularly (dot line) polarized beams. Curves (I, D0.7) correspond to (ωp/ω)2=0.7(1+2.5ξ), ρ0=4, and (Pcr2/Pcr1)=113.22 (for linearly polarized laser beam) and 113.21 (for circularly polarized laser beam), and curves (II, D1.2) correspond to (ωp/ω)2=1.2(1+2.5ξ), ρ0=3, and (Pcr2/Pcr1)=99.067 (for linearly polarized laser beam) and 64.89 (for circularly polarized laser beam). (b) Variation of dimensionless axial intensity (q0/f2) with dimensionless distance of propagation (ξ) for linearly (solid line) and circularly (dot line) polarized beams. Curves (I, D0.7) correspond to (ωp/ω)2=0.7(1+2.5ξ), ρ0=4, and (Pcr2/Pcr1)=113.22 (for linearly polarized laser beam) and 113.21 (for circularly polarized laser beam) and curves (II, D1.2) correspond to (ωp/ω)2=1.2(1+2.5ξ), ρ0=3, and (Pcr2/Pcr1)=99.067 (for linearly polarized laser beam) and 64.89 (for circularly polarized laser beam).
(a)
(b)In underdense plasma there is not much difference in propagation of linearly polarized and circularly polarized beams, while the propagation is affected in case of overdense plasma and focal point changes.A threshold exists for onset of self-focusing, as this effect must overcome the spreading of the beam due to diffraction. A light beam is focused to be self-trapped at any arbitrary diameter and will thus not spread. Further, self-trapping occurs at a critical power level, which is independent of the beam diameter. The theory presented here has a much wide range of application than the previous one, because it is not a perturbation treatment. Furthermore, it is applicable at all intensities—high and low.



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