The model and numerical simulation

Errors in wiggler magnetic field and electron beam steering can degrade the FEL performance.

We will assume that each wiggler segment is shimmed to have vanishing first and second magnetic field integrals and focus on the variations of the wiggler parameter K due to magnetic field errors or transverse misalignments among segments. Using the 1D FEL equations, Yu and Krinsky, studied the effect of wiggler errors (Yu and Krinsky, Reference Yu and Krinsky1992) on FEL performance.

When the undulator strength parameter has an error ΔK = K − K ₀, the phase change (Huang and Kim, Reference Huang and Kim2007) can be written as

(1)$$\eqalign{\displaystyle{{{\rm d}\theta } \over {{\rm d}z}} &= k_{\rm u}-\;k_{\rm s}\;\displaystyle{{1 + ({(K_0 + \Delta K)}^2/2)} \over {2\gamma ^2}} \cr & \approx \;2k_{\rm u}-\;k_{\rm u}\;\displaystyle{{K_0\Delta K} \over {1 + (K_0^2 /2)}}.} $$

Here, the first term describes the ideal motion, and the second term is the amount of the phase kick due to small changes in K.

We have introduced a magnetic correlation length L _c = N_cλ_u which is assumed to be much shorter than the approximate field amplitude gain length. Then the net phase shift per gain length is

(2)$$\Delta {\rm \theta} = {\rm \;} \mathop \sum \limits_{n = 1}^{2L_{{\rm 3G}}/L_{\rm c}} N_{\rm c}\displaystyle{{2{\rm \pi} K_0\Delta K_n} \over {1 + K_0^2 /2}}\;, $$

For 2 L _3G/L_c ≫ 1, Δθ has a zero mean and a variance

(3)$$ \lt \; \lpar {\Delta {\rm \theta}} \rpar ^2 \gt \; = \; \displaystyle{{L_{{\rm 3G}}} \over {L_{\rm c}}}\left( {\; N_{\rm c}\; \displaystyle{{2{\rm \pi} K_0^2} \over {1 + (K_0^2 /2)}}\; \displaystyle{{\sigma_K} \over {K_0}}\;} \right)^2.$$

where σ _K is the rms value of ΔK _n.

The 3D gain length (Xie, Reference Xie2000) of a FEL has expressed as

(4)$$L_{{\rm 3G}} = {\rm \;} L_{1{\rm g}}\lpar {1 + \; {\rm \Lambda}} \rpar .\; $$

The correction factor Λ has been obtained by 3D numerical studies.

(5)$${\rm \Lambda} = {\rm F\;} (X_{\rm \gamma}, {\rm \;} X_{\rm d},{\rm \;} X_{\rm \varepsilon} )$$

where,

(6)$$X_{\rm \gamma} = 4{\rm \pi \;} \displaystyle{{L_{1{\rm g}}} \over {{\rm \lambda} _{\rm w}}}{\rm \;} \displaystyle{{{\rm \sigma} _{\rm \gamma}} \over {\rm \gamma}}, {\rm \;} \; \; X_{\rm d} = {\rm \;} \displaystyle{{L_{1{\rm g}}} \over {L_{\rm r}}},{\rm \;} \; \; X_{\rm \varepsilon} = {\rm \;} \displaystyle{{L_{1{\rm g}}} \over {\rm \beta}} {\rm \;} \displaystyle{{4{\rm \pi \varepsilon}} \over {\rm \lambda}} {\rm \;} $$

with σ _γ is the energy spread, and ε is the emittance.

(7)$$L_{\rm r} = \; \displaystyle{{{\rm \pi} w_0^2} \over {\rm \lambda}}. $$

L _r is the Rayleigh range.

The extended 3D equations describing the effect of the wiggler errors due to the phase shift, the 3D gain length, energy spread, and emittance in FEL interaction of the lower and higher energy electron beams with oscillator may be written as

(8)$$\eqalign{\displaystyle{{{\rm d}\vartheta {[x,y,\bar{z}]}_j} \over {{\rm d}\overline {\rm z} }} =& [\gamma [x,y,\bar{z}]_j-\gamma _r[x,y,\bar{z}]] \cr & + k_{{\rm s}\;}\varepsilon _n/2\;\overline {\gamma _1} \;k_{\rm u}\overline {\rho _1} \;\overline \beta ,} $$

(9)$$\displaystyle{{{\rm d\varphi} {[x,y,\bar{z}]}_j} \over {{\rm d} \bar {\rm z}}}} = [{\rm \Gamma} [x,y,\bar{z}]_j-{\rm \Gamma} _{\rm r}[x,y,\bar{z}]] + k_{{\rm s\;}} \varepsilon _n/2\overline {{\rm \gamma} _n} k_{\rm u}\overline {{\rm \rho} _n} { \bar {\rm \beta},} $$

The scaled lower and higher electron-energy parameters in the phase Eqs (8) and (9) are defined as

(10)$${\rm \gamma} [x,y,\bar{z}]_j\equiv ({\rm \gamma} _j-\overline {{\rm \gamma} _1} )/{\rm \;} \overline {{\rm \rho} _1} {\rm \;} \overline {{\rm \gamma} _1} $$

(11)$${\rm \Gamma} [x,y,\bar{z}]_j\equiv ({\rm \gamma} _{\rm j}-\overline {\gamma _n} )/\overline {{\rm \rho} _n} \; \overline {{\rm \gamma} _n} $$

with the relation $\overline {{\rm \gamma} _n} \; = {\rm \;} \sqrt {n{\rm \;}} \overline {{\rm \gamma} _1} $, and the normalized emittance of ε_n.

The coupling of the lower-energy electrons to both the fundamental and the harmonic fields are seen in Eq. (12). From Eq. (13), the higher-energy electron couples only to the harmonic field A_H (its fundamental field).

(12)$$\displaystyle{{{\rm d\gamma} [{[x,y,\bar{z}]}_j} \over {{\rm d} \bar{\rm z}}}} = -\mathop \sum \limits_{h.{\rm odd}}^n F_{\rm h}\lpar {A_{\rm L}{\rm e}^{ih\vartheta {[x,y,\bar{z}]}_j} + c.c.} \rpar ,$$

(13)$$\displaystyle{{{\rm d\Gamma} {[x,y,\bar{z}]}_j} \over {{\rm d}\bar{\rm z}}}} = \; -c_1F_1\lpar {A_H{\rm e}^{ih\vartheta {[x,y,\bar{z}]}_j} + c.c.} \rpar ,$$

where j = 1,…, N are the total number of electrons, h = 1, 3, 5, … are the odd harmonic components of the field, and F _h,k are the usual differences of Bessel function factors.

The field A _L is seen from Eq. (14) to be driven only by the lower energy electron beam. Equation (15) demonstrates that the harmonic field has two driving sources: The lower and higher energy electron beams.

(14)$$\left( {\displaystyle{{\partial^2} \over {\partial x^2}} + \displaystyle{{\partial^2} \over {\partial y^2}} + 2i\; k_{\rm s}\displaystyle{\partial \over {\partial} {\bar{\rm z}}}}} \right)A_{\rm L}\lsqb {x,y,\bar{z}} \rsqb = {\rm \;} {\rm S}_{h\vartheta}, $$

(15)$$\left( {\displaystyle{{\partial^2} \over {\partial x^2}} + \displaystyle{{\partial^2} \over {\partial y^2}} + 2i\; k_{\rm s}\; \displaystyle{\partial \over {\partial {\bar{\rm z}}}}} \right)A_H\lsqb {x,y,\bar{z}} \rsqb = (S_{\rm \varphi} + S_{n\vartheta} ),$$

where

(16)$$S_{h\vartheta} = F_k{\rm e}^{-ik\vartheta \lsqb {x,y,\bar{z}} \rsqb },$$

(17)$$S_{\rm \varphi} = c_2F_1{\rm e}^{-i{\rm \varphi} [x,y,\bar{z}]},$$

(18)$$c_1 = \displaystyle{1 \over {n^{1/4}}}\left( {\displaystyle{{{\rm \rho}_n} \over {{\rm \rho}_1}}} \right)^{3/2},$$

(19)$$c_2 = n^{1/4}\left( {\displaystyle{{{\rm \rho}_n} \over {{\rm \rho}_1}}} \right)^{3/2},$$

(20)$$\bar{z} = 2k_{\rm u}{\rm \rho} z{\rm,} $$

where, h refers to all odd harmonics h < n, I is the beam current, and the subscripts 1 (n) refer to the parameters of the lower (higher) energy beam.

The analysis of the system has been carried out using the method of numerical simulations with collective variables (Bonifacio and McNeil Reference Bonifacio and McNeil1988; Bonifacio et al., Reference Bonifacio, Pelligrini and Narducci1984).

The parameters of our simulation were wiggler period 2.5 cm ; a number of periods of 80; beam currents (I _b) 75 and 25 A for n = 3 and 5, respectively; curvature radius of 450 ~ 520 cm ; and a resonator length of 8.0 m. The simulation used our extended 3D simulation code, which describes the effects of two-electron beams with different energies, that is, 13.4 MeV (higher beam) and 6 MeV (lower beam). The seed field at the lower electron beam energy is modeled by defining its initial scaled intensity at the beginning of the FEL interaction |A _L1(${\rm \bar{z}}$ = 0)|² = (1 + I) exp[−(x ² + y ²)/0.5] × 10⁻⁸ to be two orders of magnitude greater than that of the harmonic. The multi-particle and multi-pass simulations were performed for a particle number of 300 and a pass number of 200. In the simulations, the minimum waist position of the radiation is at the center of the cavity. The radiation spot size (w ₀) at the minimum waist, higher harmonics (k, n = 3 and 5) and the number of macro-particles (j = 300) were used in the simulation.

An evaluation of the effect of the beam's emittance was performed for the case of the coupled two-beam oscillator with a phase shift errors 0–4 radian as shown in Figure 1. For the maximum emittance of the higher beam at ε_n = 60 mm · mrad, the saturation intensity|A|²decreases by approximately 3% relative to those of the minimal emittances of ε_n = 20 mm · mrad of the two-beam system as shown in Figure 1. However, the harmonic field intensity of both beams with phase shift errors is decreased significantly compared with that of both electron beam without phase shift errors for varying emittances and it was decreased by approximately 11% in the case of both beams with phase shift errors.

Fig. 1.

Evolution of the harmonic radiation field intensity, for varying emittance of 20, 40, and 60 mm·mrad, for a phase shift errors of 0–4 radian (both beams).

An evaluation of the effect of the beam's emittance was performed for the case of the coupled two-beam oscillator with for a wiggler error of ΔK = 10⁻⁴ as shown in Figure 2. For the maximum emittance of the higher beam at ε_n = 60 mm · mrad, the saturation intensity|A|²decreases by approximately 9% for n = 3 relative to those of the minimal emittances of ε_n = 20 mm · mrad of the two-beam system as shown in Figure 2.

Fig. 2.

Evolution of the harmonic radiation field intensity, for varying emittance of 20, 40, and 60 mm·mrad, for a wiggler error of ΔK = 10⁻⁴ (both beams).

Figure 3 shows the evolution of the harmonic intensity for the case of the coupled two-beam oscillator with and without wiggler errors for varying Gaussian energy spreads σ_E.

Fig. 3.

Evolution of the maximum harmonic intensity in the two-beam oscillator for Gaussian energy spreads from ${\rm \sigma} _{\rm E} = 0{\rm \;\ to\;} {\rm \sigma} _{\rm E} = 0.6{\rm \%} $ in the higher energy beam with and without wiggler errors.

For an energy spread of the higher beam of ${\rm \sigma} _{\rm E} = 0.6{\rm \%} $ for the case of the coupled two-beam oscillator with wiggler errors, the saturation intensity |A|² decreases by approximately 11% relative to that of the energy spread of ${\rm \sigma} _{\rm E} = 0.2{\rm \%} $ the higher beam as shown in Figure 3.

However, for an energy spread of ${\rm \sigma} _{\rm E} = 0.6{\rm \;\ \%} $ for the case of both beam with wiggler error of δK = 10⁻⁴, the saturation intensity |A|² decreases significantly by 23% relative to that of both beam without energy spread and without wiggler error.

The field distribution of 3D Hermite-Gaussian beams (Wu and Lu, Reference Wu and Lu2002) for the higher-order modes is described at the plane z ₀  = 0 as:

(21)$$A_{m,n}\lpar {x_0,y_0,z_0 = 0} \rpar = \; H_m\left( {\displaystyle{{x_0} \over {w_{0x}}}} \right)H_n\left( {\displaystyle{{y_0} \over {w_{0y}}}} \right){\rm exp}\left[ {-\left( {\displaystyle{{x_0^2} \over {w_{0x}^2}} + \; \displaystyle{{y_0^2} \over {w_{0y}^2}}} \right)} \right]$$

where H _m and H _n denotes the Hermite polynomial of order m and n, w _0x and w _0y are waist widths in the x and y-direction, respectively.

The field error is assumed to be much smaller than the field itself, ΔK < K ₀, where ΔK and K ₀ denote the maximum error amplitude and the nominal value of the undulator parameter, respectively. The phase error (Li et al., Reference Li, Faatz and Pflueger2008) for periodic errors on phase shake is

(22)$${\rm \delta \theta} = \displaystyle{{k_{\rm u}} \over {\; 1 + \; K_0^2 \; \;}} \mathop \int \limits_0^z 2K_0\Delta K\; f\lpar {z^{\rm^{\prime}}} \rpar {\rm d}z^{\rm ^{\prime}}\;. $$

where f(z) describes the error shape, |f(z)| ≤ 1. f(z) is a periodic function with periodic length λ_δ and f(z) = f(z + λ_δ). If z is normalized, z _n = z/λ_δ.

(23)$$\eqalign{ {\rm \delta \theta} & = \displaystyle{{k_{\rm u}} \over {\; 1 + \; K_0^2 \; \;}} \; 2K_0\Delta K\; {\rm \lambda} _{\rm \delta} \mathop \int \limits_0^{z_n} \; f\lpar {z_n^{\rm^{\prime}}} \rpar {\rm d}z_n^{\rm ^{\prime}} = {\rm \;} \displaystyle{{2k_{\rm u}K_0^2} \over {\; 1 + \; K_0^2 \; \;}} \; \displaystyle{{\Delta K} \over {K_0}}\; {\rm \lambda} _{\rm \delta} g(z_n)} $$

Since the error function is periodic, the integration can be restricted to one error period length and a SASE-FEL always radiates at a wavelength for which <δθ> = 0..

Therefore the rms phase shake is given by

(24)$${\rm \sigma} _{{\rm \delta \theta}} = \; \displaystyle{{2k_{\rm u}K_0^2} \over {1 + K_0^2}} \; \displaystyle{{\Delta K} \over {K_0}}\; {\rm \lambda} _{\rm \delta} \; \sqrt {\mathop \int \limits_0^1 g^2\lpar {z_n} \rpar {\rm d}z_n\;} \; {\rm =\ \alpha \;} \displaystyle{{2k_{\rm u}K_0^2} \over {1 + K_0^2}} \; \displaystyle{{\Delta K} \over {K_0}}\; {\rm \lambda} _{\rm \delta}. {\rm \;} $$

This equation is valid for all kinds of periodic errors. Different gap profiles are described by the coefficient α. The strength is given by ΔK.

The radiation amplitudes of the 1^st-order, 3^rd-order, and 5^th-order for the wiggler error with an emittance of ε_n =10, 20, and 30mm·mradand energy spread of 0 ~ 0.5% in the two-beam oscillator system are shown in Figures 4–6, respectively. The higher-order modes have lower radiation amplitudes relative to the fundamental mode in the higher energy beam with the wiggler error, emittance, and energy spread.

Fig. 4.

(Color online) Evolution of the radiation field intensity |A|² for the (a) fundamental, (b) 3^rd-, and (c) 5^th-order modes for wiggler error dk = 0.0 without an emittance and without energy spread.

Fig. 5.

(Color online) Evolution of the radiation field intensity |A|² for the (a) fundamental, (b) 3^rd-, and (c) 5^th-order modes for wiggler error dk = 0.0001 with an emittance of ε_n = 10 mm · mrad and energy spread of 0.3%.

Fig. 6.

(Color online) Evolution of the radiation field intensity |A|² for the (a) fundamental, (b) 3^rd-, and (c) 5^th-order modes for wiggler error dk = 0.0001 with an emittance of ε_n = 30 mm · mrad and energy spread of 0.5%.

For wiggler error ΔK = 0.0001 with an emittance of ε_n = 30mm · mradand energy spread of 0.5% in the two-beam oscillator system, the saturation intensity |A|² at the fundamental mode decreased by 31% in the 3D simulation relative to those of the fundamental modes for the wiggler error ΔK = 0.0 without an emittance and without energy spread in the two-beam oscillator system.

However, for the rms phase shake in wiggler errors with sinus (α = 0.113), constant (α = 0.144) and parabolic type (α = 0.970) in the two-beam oscillator system, the saturation intensity |A|² at the fundamental mode decreased by approximately 4% only in the 3D calculations relative to those of the fundamental modes without wiggler errors for the case without an emittance and without energy spread as shown in Figure 7.

Fig. 7.

(Color online) Evolution of the radiation field intensity |A|² for rms phase shake error with sinus type (a), with constant type (b), and with parabolic type (c) for without an emittance and without energy spread.