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Front. Phys., 22 March 2019
Sec. Optics and Photonics
Volume 7 - 2019 |

Minimum Spectral Bandwidth in Echo Seeded Free Electron Lasers

  • SLAC National Accelerator Laboratory, Menlo Park, CA, United States

This paper examines the impact of non-linear longitudinal phase distortions on the spectral bandwidth in echo seeded free electron lasers (FELs). It extends the existing theory developed in Hemsing [1] for echo-enabled harmonic generation (EEHG) to include finite laser pulse durations. An analytic expression for the shape of the optimized longitudinal bunching envelope is derived, and is used to determine the laser and electron beam pulse durations that minimize the seeded bandwidth in the presence of arbitrary phase distortions. The time-bandwidth product (TBP) is also derived, and is shown that the TBP and the bandwidth increase by no more than 2 from their transform-limited values when the bandwidth is minimized.


Externally seeded FELs use lasers to produce coherent high harmonic density modulations (bunching) in relativistic electron beams that are then used for the emission of coherent radiation at short wavelengths. Seeding is useful for overcoming the otherwise noisy output of SASE (self-amplified spontaneous emission) from these beams to generate narrowband FEL radiation. Besides improved longitudinal coherence, external seeding also enables control over the character of the FEL output pulses [2, 3], allowing adjustable coherent bandwidths [4] or the ability to produce multiple, phase locked pulses [5, 6], or multiple colors [7, 8].

Several different external seeding schemes have been proposed, and a few demonstrated (see e.g., [9] and references therein). Relevant specifically to this work, echo-enabled harmonic generation (EEHG) is a scheme that uses two external laser pulses (generally UV wavelengths) to efficiently generate bunching in the electron beam down to soft x-rays [10, 11]. In EEHG, the first laser produces a sinusoidal energy modulation in the electron beam that is typically only a few times the intrinsic slice energy spread. The beam then goes through a strong longitudinally dispersive section that folds over the sinusoids and creates a filamentary phase space structure in the particle distribution. The second laser then modulates the filamented phase space distribution, and a final dispersive section creates high harmonic bunching at short wavelengths in the current distribution. The beam then enters the FEL where coherent light is emitted and exponentially amplified.

A primary goal of seeding schemes is to minimize the FEL bandwidth and produce transform-limited pulses. In principle, the narrowest obtainable bandwidth is given by the inverse electron beam bunch length. In practice however, electron beams in modern FELs have distortions in the longitudinal phase space that mix additional frequencies into the harmonic up-conversion that spoil the purity of the final output spectrum [1220]. In Hemsing [1] a general method was developed to calculate the impact of beam energy distortions through the broadening they introduce in the bunching spectrum (i.e., the Fourier transform of the current distribution). The broadening width was then used to set limits on the amplitude of common distortions to maintain near transform-limited seeding.

The magnitude, shape, and location of these distortions, within both the electron beam and the laser pulse, is an important factor in the optimization of external seeding schemes. The analysis in Hemsing [1] assumed infinitely long lasers that completely covered the electron beam (e-beam). In this limit, the bunching spectrum is predicted to be highly sensitive to e-beam energy variations because the whole beam contributes to the final spectrum and can have strong nonlinear portions in the head and tail. However, in practice, the seed lasers can be comparable in length to the electron beam or shorter, and positioned longitudinally within the e-beam to avoid seeding in the strong nonlinear portions. Shorter pulses naturally have broader bandwidths, so in order to achieve the narrowest harmonic bunching spectrum, a balance must be found between the transform limited bandwidth of the short laser and the broadening from the nonlinear phase contributions.

Here, using an extension of the formalism in Hemsing [1], we examine this more practically relevant case where the seed laser pulse can vary in duration, and also carry nonlinear temporal phase structures. This allows analysis of the bunching spectrum in the presence of nonlinearity in the electron beam and laser phase. From a general expression for the bandwidth, we show that laser pulses optimized in duration can produce much narrower bunching spectra once the e-beam energy distortions reach a threshold value. We also define the requirements that allow the laser phase to precisely compensate the e-beam distortions to obtain transform limited pulses.

The paper is arranged as follows. We first present an extension to the theory in Hemsing [1] that includes a finite seed laser pulse that produces a modulation with a longitudinal profile given by the function g(z). Under reasonable approximations, the bunching bandwidth can be calculated straightforwardly from g(z), the e-beam distribution f(z), and the combined phase distortions φ(z). Since the spectral-temporal properties in EEHG are inherited primarily from the second laser, we assume the first laser is infinite. Assuming that the EEHG bunching amplitude is optimized, we then derive an analytic expression for g(z) with a Gaussian seed laser. From this we retrieve the well-known m−1/3 harmonic compression effect, and are able to calculate the transform-limited bandwidth. Arbitrary phase distortions are then included as a Taylor series, and their impacts to each order on the total bandwidth and time-bandwidth product (TBP) are then calculated analytically. We then derive the conditions on the laser pulse length and e-beam length to minimize the bandwidth, and study a few examples.

Mathematical Description

Notation closely follows that of Xiang [11]. Consider an EEHG electron beam transformation of the form,

p1=p+A1sin(k1z)+Δp1(z),z1=z+B1p1/k1,p2=p1+A2(z1)sin[k2z1+ψ2(z1)]+Δp2(z1),z2=z1+B2p2/k1.    (1)

where the normalized laser modulations are A1, 2 = ΔE1, 2E, normalized dispersions are B1,2=k1R56(1,2)σE/E, the slice energy spread is σE, and E is the electron beam energy. Here, distinct from the analysis in Hemsing [1], we allow the second laser to have a finite pulse length, A2(z1), as well as a longitudinally dependent phase ψ2(z1). The first laser, A1, is assumed to be ideal and infinite in length. Additional energy distortions in the electron beam, Δp1 and Δp2, are again modeled as occurring alongside the laser modulations.

The bunching spectrum near the harmonic peak kE = aEk1 = (n + mK)k1 is given by

bn,m(k)=e-ξE2/2Jn(-ξEA1)e-iz(k-kE)+iφ(z)×f(z)Jm(-aEA2(z)B2)dz,    (2)

where ξE = nB1 + aEB2 is the EEHG scaling parameter, and f (z) is the longitudinal electron beam distribution function. The beam is assumed to have an uncorrelated Gaussian initial energy distribution. Similar to Hemsing [1], here we utilize the weakly-folding approximation which assumes that the energy structures satisfy B1dΔp1/dzk1 and are small enough so that they do not lead to large changes in the phase space distribution after the first chicane. We also assume that the longitudinal variations in Δp2, A2, and ψ2 are sufficiently slowly-varying that the full integral can be simplified by replacing z for z1 in the function arguments. It is also assumed that the system is far from the minimum pulse duration limit [21].

With these approximations, the phase φ(z) captures the combined impact of energy distortions in the electron beam, Δp1, 2, and the phase variation ψ2 in the second laser,

φ(z)=-ξEΔp1(z)-aEB2Δp2(z)+mψ2(z).    (3)

The z-dependence of the second laser envelope A2(z) is still within the argument of the Jm Bessel function, which complicates simple analytic solutions. We therefore search for an ansatz of the form,

Jm(-aEA2(z)B2)=g(z)Jm(-aEA2B2),    (4)

where the imprint of the slowly-varying laser envelope is captured by the function g(z), determined shortly by approximate expansion. Note that in the limit of an infinitely long laser, g → 1. In anticipation of a Gaussian laser profile, A2 = A2(0) is the peak of the modulation.

With bn,m(k)=b~n,m(z)e-ikzdz, the longitudinal bunching factor can then be expressed as

b~n,m(z)b̄n,mf(z)g(z)eikEz+iφ(z),    (5)

where f(z)g(z) together form the z-dependent envelope, and b̄n,m=e-ξE2/2Jn(-ξEA1)Jm(-aEA2B2) the optimized bunching amplitude [20]. Now the instantaneous spatial bunching frequency is just the z-derivative of the full longitudinal phase,

kz(z)=kE+φ(z).    (6)

The average frequency is then

kz=-kz(z)[f(z)g(z)]2dz-[f(z)g(z)]2dz=kE+φ(z),    (7)

and the spectral bandwidth of the harmonic bunching spike is

σk2=σkE2+(φ)2-φ2,      =σkE2+σφ2,    (8)

where the transform-limited bunching bandwidth is [22]

σkE2=[(fg)]2dz(fg)2dz.    (9)

This gives the bandwidth due to the combination of the laser modulation g(z) with the electron beam distribution function f(z). It is dominated by the shorter of the two if they coincide longitudinally. The bandwidth due to the nonlinear phase structures is given by σφ.

Optimized Modulation

We consider the effect of a Gaussian laser pulse in the second echo modulator on the longitudinal profile of the bunching. This will enable us to calculate an approximate form for g(z), and thus the harmonic compression factor and scaling of the bunching bandwidth in the presence of the phase φ(z). Slippage in the modulator is ignored.

The optimum amplitude of the second laser from time-independent echo theory is A2=jm,1/aEB2, given by the requirement that Jm(aEA2B2) is peaked, with jm,1=m+0.8087m1/3 the first zero of the Bessel function Jm. Small relative changes in the bunching due to variations from the optimum modulation are given by [20]

Δb̄n,mb̄n,m=-(ΔA2A2)2(jm,1)2-m22,    (10)

where m ≫ 1 is the harmonic of the second laser. Let us assume that the laser modulation envelope has an rms intensity duration σL/c,

A2(z)=A2e-z2/4σL2    (11)

To lowest order near the z = 0 peak, small changes in the laser amplitude vary according to ΔA2/A2=-z2/4σL2. This suggests that the bunching envelope function g(z) can be written as g(z)1-(z24σL2)2(jm,1)2-m22. Mathematically, this looks like a lowest order expansion about z = 0 for small values of the second term. We posit then, that the functional dependance of g(z) may be modeled as a super-Gaussian distribution that has the same series expansion to lowest order:

g(z)exp[-(z24σL2)2(jm,1)2-m22]        =exp[-q22(zσg)4]    (12)

where q = Γ(3/4)/Γ(1/4) ≈ 1/3. This form for the z-dependent bunching envelope induced by the laser closely matches exact solutions, as shown in Figure 1. The rms width of |g(z)|2 is, to a good approximation,

σgσLm1/3.    (13)

Figure 1. (Top) Bunching envelope and harmonic compression effect for m=50. The approximate super-Gaussian g(z) is slightly narrower than the exact solution. (Bottom) Corresponding frequency spectra.

Thus we recover the m−1/3 scaling of the harmonic compression effect of the initial laser pulse length [13, 14], where for large harmonics (jm,1)2-m21.62m4/3. The FWHM has the same scaling but with a different proportionality, Δg1.4m1/3ΔL, where ΔL=σL8ln2 is the FWHM of the seed laser intensity. These scalings are plotted against exact values in Figure 2.


Figure 2. Normalized RMS and FWHM lengths of the bunching envelope from exact numerical calculations (solid lines) and from the super-Gaussian approximation (dashed lines).

Harmonic compression is the result of the high harmonics being increasingly more sensitive to the optimal modulation amplitude to produce bunching, so the longitudinal region of the Gaussian modulation that matches this condition becomes narrowed. The flattened, super-Gaussian form of g(z) is thus characteristic of the optimized bunching envelope for a Gaussian second seed laser. We note that it slightly underestimates the exact longitudinal width of the bunching envelope, as shown in Figures 1, 2. The rms value in (13) is low by about 10%, so the predicted spectral bandwidths can also differ slightly, but the scaling with m still holds.

With an analytic form for g(z) in hand, the transform-limited bandwidth in Equation (9) can be calculated for a specified electron beam distribution f(z). For the sake of simplified calculations, we assume that f(z) has the same, super-Gaussian form as g(z), but with a different rms, σz, and properly normalized,

f(z)=2qσzΓ(1/4)exp[-q2(zσz)4].    (14)

The rms transform-limited bandwidth of the bunching spectrum then has simple analytic solution that is approximately (see Supplementary Material),

σkE212(1σz4+12σg4)1/2=12(1σz4+m4/32σL4)1/2.    (15)

Similarly, the rms length of the bunching envelope |b~n,m(z)|2 is simply (see Equation 51),

σb13σkE.    (16)

Figure 3 shows how σkE varies with σL for different harmonics. Two limiting regimes can be identified. If the laser is much longer than the beam σLm1/3σz, then σkE is independent of m and is at its narrowest value. This is the regime studied in Hemsing [1]. In the opposite limit, with g(z) much shorter than the electron beam, the bandwidth grows like m1/3 because of the harmonic compression effect. Note that the relative bandwidth decreases in this limit like m2/3,

σνE=σkEkE~σνLm2/3,    (17)

assuming kE = aEk1mk2, and σνL = 1/2σLk2 is the relative bandwidth of the laser.


Figure 3. Transform-limited bandwidth σkE as a function of laser pulse length σL from Equation (15). Because of harmonic compression, the laser pulse length needs to increase slightly with increasing harmonic number to maintain a fixed bandwidth.

In general, the transform-limited bunching bandwidth σkE is set by the length of the laser on the electron beam. However, nonlinear phase structures φ(z) introduce additional bandwidth through the term σφ in Equation (8). Depending on the origin of the nonlinear phase structures, it may be possible to limit their impact on the total bandwidth by adjusting σkE, either with the laser pulse length σL or the electron beam length σz. In other words, what combination of σL or σz gives the smallest total bandwidth of the bunching spike σk? Consider the example of an electron beam with a quadratic chirp, as shown in Figure 4. On one hand, a narrowband laser with a longer pulse length could work, but it may extend over or add more of the undesirable nonlinearities that add bandwidth during the harmonic up-conversion. Conversely, a short laser pulse is intrinsically broadband, but may be less impacted by the presence of nonlinearities. As we will see, the optimization is straightforward once the phase is known, and the answer depends on the amplitude and source of the non-linearity.


Figure 4. Example electron beam phase space distribution (from FERMI [Allaria, personal communication]) with dominant quadratic structure and higher order structure near the head and tail. The optimized laser pulse length to produce a minimum bandwidth depends on the amplitude of the non-linearities in the beam.

Simple Nonlinear Structure

Without regard to the origin of the nonlinear phase structure (i.e., laser phase ψ2 or electron beam energy structures Δp1, 2), let us first calculate the impact of generalized phase structures on the bunching bandwidth σk. We will then use the results to derive conditions for obtaining the minimum bandwidth.

Arbitrary continuous phase distortions can be expanded in a Taylor series about z = 0. Similar to the temporal phase in laser physics, we can expand the bunching phase φ(z) as,

φ(z)=N=1ϕNN!zN,    (18)

where each ϕN=Nφ(z)/zN|z=0 is real. The absolute phase of the pulse ϕ0 is ignored, as it does not affect the frequency or bandwidth. With Equation (6), the instantaneous frequency is kz(z)=kE+ϕ1+ϕ2z+ϕ32z2+ Combined with (7) and (8), the bandwidth σφ2 associated with the energy distortions can be calculated analytically up to arbitrary order in N (see Supplementary Material).

Single Phase Term

The analysis is simplified by isolating a single term in the phase expansion,

φ(z)=ϕNN!zN.    (19)

The total bunching bandwidth is then written in terms of the nonlinear coefficient ϕN, as

σk2=σkE2(1+GNϕN2σkE2N).    (20)

The second term is the excess bandwidth from the phase nonlinearity. The analytic expression for the numerical coefficient GN is given in the Supplementary Material, and the lowest order numerical values are given in Table 1.


Table 1. Numerical values of GN.

The time-bandwidth product (TBP) of the bunching spectrum is the dimensionless product of the rms envelope length (16) and the rms bandwidth (20),

TBP=σbσk131+GNϕN2σkE2N.    (21)

Figure 5 plots shows how the TBP is impacted by the different order nonlinear phases. Here we see that larger order longitudinal phase structures have a larger effect on the TBP. This is in contrast to different order spectral phases in which only the even orders broaden the bunching bandwidth [14].


Figure 5. Time-bandwidth product as a function of the phase change over the rms bunching envelope φ(σb)=ϕNσbN/N!. Results are predicted from Equation (21).

Minimum Bandwidth

With the expression for the bunching bandwidth in (20), it is straightforward to find the values of the laser pulse length or the electron beam length that minimize σk in the presence of a phase nonlinearity. In either case this amounts to finding the optimal value of σkE for a given ϕN. Assuming that ϕN is fixed with respect to the parameter being changed, the minimum bandwidth occurs when σkE can be adjusted to satisfy,

σkE2N=ϕN2GN(N-1).    (22)

The minimum total bandwidth then scales directly with optimal σkE,

(σk)min=σkENN-1.    (23)

An example of how the minimum bandwidth varies in general for different amplitude phase distortions is shown in Figure 6.


Figure 6. Total bandwidth vs. σkE for different N = 2 phase distortions. The minimum total bandwidth follows the dashed curve if ϕN is large enough (i.e., if Equation 22 is satisfied). Otherwise the minimum is set by the minimum possible value of σkEkE = 1, in this example for ϕN = 0 and 1).

The full expressions for the optimal electron beam length and laser pulse length are given in (60) and (62) the Supplementary Material. Consider the case where the transform-limited laser pulse length can be varied over a fixed length electron beam. If the phase distortion is large enough that ϕN2GN(N-1)1/(2σz2)N, then the laser that minimizes the bandwidth is given by

(σL2)min=m2/322[ϕN2GN(N-1)]1/N.    (24)

Figure 7 illustrates this scenario. Identical values of the dimensionless phase distortion ϕNσzN=20 for different orders N show that, as N is increased, shorter and shorter laser pulses are needed to minimize the bandwidth, as given by Equation (24).


Figure 7. Scaled bunching bandwidth vs. relative laser duration for phase distortions of ϕNσzN=20 caused by different orders. Harmonic m = 50 is modeled.

Alternatively, if the laser is held fixed and ϕN2GN(N-1)(m2/3/8σL2)N, the optimal electron bunch length is

(σz2)min=12[ϕN2GN(N-1)]1/N.    (25)

Note that this is independent of the harmonic, in contrast to the optimal laser pulse length.

The TBP at the minimum bandwidth is,

TBP=13NN-1.    (26)

It has the same dependence on the order of the phase distortion as σk; both approach their transform-limited values as N becomes large. Clearly the lowest order phase distortions have the greatest impact on both. These results shows that, if the phase distortions are described by a single polynomial term, then by proper optimization the TBP and the bandwidth will be no more than 2 times the transform-limit.

Inspection of the full expression for the TBP shows that it cannot be minimized simultaneously with the total bandwidth by adjustment of σkE alone, though it is possible if ϕN is not held fixed.

Quadratic Electron Beam Chirp

In modern FELs, it is common that the electron beam has some residual energy-time correlation in the phase space. These correlations can be the result of wakefields or other collective effects during compression and transport. They may be difficult to remove completely, and may be present at the entrance to the EEHG seeding system, or can develop within the EEHG beam line from collective effects [1]. In either case, their impact on the final bunching bandwidth can be calculated within the present framework and stated constraints.

Consider a purely quadratic energy chirp on the electron beam of the form,

Δp(z)=h2k22z2.    (27)

The chirp amplitude is characterized by the dimensionless factor h2. Assuming the second seed laser is transform-limited (ψ2 = 0), the bunching phase can be written generically as [1],

φ(z)=-ηΔp(z),    (28)

where η = ξE or aEB2 depending on where the energy distortion occurs, as expressed in Equation (3). The nonlinear coefficient in (19) for N = 2 is then

ϕ2=-2ηh2k22.    (29)

Plugging this into Equation (22) and optimizing the laser pulse length, one can show that if the amplitude of the quadratic beam chirp strongly satisfies

h2>34η(k2σz)2,    (30)

then the laser pulse length that minimizes the bandwidth is, from Equation (24),

(σL)min5m1/39k2ηh2.    (31)

The corresponding relative bandwidth from Equation (23) is then

(σν)min=(σk)minkE3ηh22m.    (32)

Consider the realistic case of electron beams at the FERMI FEL [23] (for example in Figure 4), which can have a quadratic chirp of 30 MeV/ps2 upstream of the 260 nm seeding sections. This corresponds to h2=2×10-6 for a slice energy spread of σE = 0.15 MeV. In this case Equation (30) is satisfied for beams longer than σz = 30 μm (100 fs), which is easily the case for the ps-scale beams at FERMI (assuming η = 1/2). The minimum bandwidth setting from (31) requires a laser pulse duration of 250 fs at the 36th harmonic and produces (σν)min=4.2×10-5. At the 64th harmonic, a 300 fs laser is optimum to generate (σν)min=2.3×10-5.

Linear Laser Frequency Chirp

Similar to quadratic structure on the electron beam, a linear laser chirp in the second seed laser introduces frequency-time correlations that mix into the harmonic up-conversion process and impact the final bunching bandwidth. If the electron beam phase space is flat, the bunching phase φ(z) in Equation (3) is only the laser phase times the harmonic,

φ(z)=mψ2(z).    (33)

It is useful to separate laser chirps according to whether they are defined in terms of a fixed pulse length as in Siegman [24] or in terms of a fixed bandwidth (e.g., [25]).

Fixed Laser Pulse Length

A linear frequency chirp corresponds to a quadratic phase of the form [24],

ψ2(z)=αz2.    (34)

Assuming the pulse length is fixed, α only affects the laser bandwidth. The quadratic coefficient of the bunching phase is then ϕ2 = 2, and the analysis is the same as with a quadratic e-beam chirp with the replacement -ηh2k22=mα. If both the e-beam and the laser phase have quadratic structure, then their effect on the bunching cancels if ηh2k22=mα.

Fixed Laser Bandwidth

On the other hand, for a fixed-bandwidth laser pulse with rms intensity σkL, a linear frequency chirp that changes only the pulse length σL corresponds to a phase,

ψ2(z)=CσkL2z2,    (35)

where the chirp is

C=±x2-1x2,    (36)


x=σLσL0=2σLσkL1,    (37)

is the pulse stretch factor. The laser bandwidth corresponds to transform-limited pulse length, σL0 = 1/2σkL.

Note that the chirp grows from zero to a maximum of |C| = 1/2 when the pulse length is stretched by x=2, and then decreases to zero as the pulse is stretched further. This is shown in Figure 8. This means that a strongly stretched pulse can have the same small chirp as a barely stretched pulse, even though the pulse lengths are quite different [25]. Wigner distributions of the laser pulses for different values of x are shown in Figure 9.


Figure 8. Chirp as a function of stretch factor, x = σLL0. From Equation (36).


Figure 9. Wigner distributions of a chirped laser pulse with fixed bandwidth with x and C values from Equation (36).

The quadratic coefficient of the bunching phase is,

ϕ2=2mCσkL2.    (38)

The chirp is multiplied by the harmonic. Because the laser pulse length changes, the bandwidth σkE is also a function of the stretch factor x,

σkE2=12(1σz4+8m4/3σkL4x4)1/2.    (39)

Inserting (38) into (22), one can see that if the pulse is stretched such that 23m2/3(x2-1)>1, then there exists a finite length electron beam that minimizes the bandwidth, given approximately by (25),

(σz)min31/42σkLmC.    (40)

The optimum electron beam length is the smallest at the maximum chirp, C = 1/2, and is also less than σL0 unless the harmonic chirp is smaller than one, mC < 1. This can occur for both barely stretched or strongly stretched pulses. The minimum relative bandwidth from Equation (23) is then,

(σν)min=2σνL31/4Cm.    (41)

Figure 10 shows how the bandwidths evolve for different σz.


Figure 10. Scaled bandwidth vs. electron beam length for different values of a fixed-badwidth laser stretched with a linear chirp at m = 50.

Note that if the electron beam also has quadratic curvature, the laser chirp can be set to negate the bandwidth broadening if C=-ηh2/mσνL2, similar to [4]. Consider the example of the 4 GeV (σE = 0.45 MeV) beam at LCLS-II using EEHG to reach harmonic m = 130 of a 260 nm laser. Assuming σz = 15 μm (50 fs), and quadratic electron beam curvature h2=1×10-4 in the beam core, the transform-limited laser pulse to minimize the bandwidth from (30) is also 50 fs (assuming η = 1/2). This yields a relative bandwidth from (32) of (σν)min8×10-5. However, chirping the laser slightly C=-ηh2/mσνL2-1/4, (stretching the pulse by about 3%), the bandwidth is reduced by 2 and is at the transform limit.

Finally, it is useful to look at a practical example in which the electron beam is long compared to the length of the second laser, irrespective of the chirp (e.g., FERMI). The total relative bandwidth from Equation (20) is then

σν24σνL23x2m4/3[1+34m2/3(x2-1)].    (42)

Inspection reveals that σν grows with increasing x for high harmonics, so the minimum bandwidth is obtained only when the laser chirp is zero. The scaling with the harmonic number clearly differs according to whether the laser is fully compressed or stretched,

σv{σvL/m2/3(x=1)σvL/m1/3(x1).    (43)

Figure 11 illustrates the bandwidth growth between the two regimes.


Figure 11. Relative bandwidth as the fixed-bandwidth second laser is stretched for different harmonics, assuming σz → ∞. Exact solutions are solid lines, and approximate solutions from Equation (42) are dashed lines. The disagreement with exact solutions is attributed to the super-Gaussian approximation for g(z).


Finite laser pulse length effects in EEHG FEL seeding are investigated. We have derived an approximate super-Gaussian form for the laser modulation g(z) and used it to calculate the spectral bandwidth of the harmonic bunching peak. The effects of nonlinear longitudinal variations in the e-beam energy and the laser temporal phase are studied by way of a general phase term φ(z). From the series expansion, the impact on the bandwidth and the TBP of the different order phase contributions is determined. All orders of the temporal phase contribute, in direct contrast to the spectral phase where the odd orders are negligible. Conditions on obtaining the minimum bandwidth are derived, which is shown to exceed the transform-limited bandwidth by at most 2, depending on the order of the nonlinearity.

Author Contributions

The author confirms being the sole contributor of this work and has approved it for publication.

Conflict of Interest Statement

The author declares that the research was conducted in the absence of any commercial or financial relationships that could be construed as a potential conflict of interest.


This work was supported by the U.S. Department of Energy Contract No. DE-AC02-76SF00515 and the U.S. DOE Office of Basic Energy Sciences under award number 2017-SLAC-100382. The author would like to thank L. Giannessi for helpful discussions.

Supplementary Material

The Supplementary Material for this article can be found online at:


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Keywords: FEL (free electron laser), EEHG, echo, seeded, xray, chirp, nonlinear, harmonic

Citation: Hemsing E (2019) Minimum Spectral Bandwidth in Echo Seeded Free Electron Lasers. Front. Phys. 7:35. doi: 10.3389/fphy.2019.00035

Received: 03 October 2018; Accepted: 26 February 2019;
Published: 22 March 2019.

Edited by:

Arya Fallahi, Foundation for Research on Information Technologies in Society, ETH Zurich, Switzerland

Reviewed by:

Ilia L. Rasskazov, University of Rochester, United States
Masoud Mehrjoo, Helmholtz Association of German Research Centers (HZ), Germany

Copyright © 2019 Hemsing. This is an open-access article distributed under the terms of the Creative Commons Attribution License (CC BY). The use, distribution or reproduction in other forums is permitted, provided the original author(s) and the copyright owner(s) are credited and that the original publication in this journal is cited, in accordance with accepted academic practice. No use, distribution or reproduction is permitted which does not comply with these terms.

*Correspondence: Erik Hemsing,