Peculiarities of Laue Diffraction of Neutrons in Strongly Absorbing Crystals

# Peculiarities of Laue Diffraction of Neutrons in Strongly Absorbing Crystals

A. Ya. Institute for Nuclear Research, NAS of Ukraine,
03680, prospect Nauki 47, Kiev, Ukraine
V. V. Institute for Nuclear Research, NAS of Ukraine,
03680, prospect Nauki 47, Kiev, Ukraine
V. Yu. Institute for Nuclear Research, NAS of Ukraine,
03680, prospect Nauki 47, Kiev, Ukraine
###### Аннотация

Well-known Kato’s theory of the Laue diffraction of spherical x-ray waves is generalized to the case of the neutron diffraction in strongly absorbing crystals, taking into consideration both the potential and the resonant scattering of neutrons by nuclei as well as a realistic angular dispersion of incident neutrons. The saddle-point method is applied for estimation of the angular integrals, being more adequate in the case of strongly absorbing crystals than the usually used stationary-phase approximation. It is found that the intensity distribution of the diffracted and refracted beams along the basis of the Borrmann triangle significantly depends on the deviation of the neutron energy from the nuclear resonant level. When comparing our calculations with the Shull’s experimental data on neutron diffraction in silicon we regard also the role of finite width of the collimating and scanning slits.

\English

Dzyublik

Mykhaylovskyy

Spivak

## 1 Introduction

The neutron scattering is one of the most powerful tools for investigation of the crystal structure and its magnetic properties (see, e.g., Refs. [1-6]). For interpretation of experimental data, obtained in very thin films, it is sufficient to apply the kinematical scattering theory, while for thick targets, where the multiple scattering of neutrons by atoms becomes significant, one has to use already its dynamical version. Such a dynamical scattering theory has been developed for the elastic diffraction in perfect crystals of both neutrons [7-9] and Mössbauer rays [10-13], treating them as plane waves. Its generalization to the case of inelastic diffraction at the crystals subject to external alternating fields was given in Refs. [14, 15].

In the case of two-wave diffraction it was predicted the effect of suppression of reactions and inelastic channels [8, 10], observed later in numerous Mössbauer diffraction experiments (see, e.g., the reviews [16, 17]) as well as in the neutron diffraction experiments [18, 19], studying the reaction in the cadmium sulphide crystal, abandoned with the nuclei Cd having the resonant level 0.178 eV.

Although there is close analogy of the suppression of nuclear reactions with the anomalous transmission of x-rays (the Borrmann effect) [20-25], the resonant nuclear scattering provides principally new character of the anomalous absorption of neutrons or -photons. Namely, in the scattering of x-rays by atomic electrons, when the Bragg condition is fulfilled, there is only partial suppression of inelastic scattering. At the same time, in the case of resonant nuclear scattering, choosing the corresponding geometry of the experiment, one can achieve complete suppression of the inelastic and reaction channels. This effect is explained by the dynamical scattering theory, which predicts that the energy exchange between the refracted and diffracted waves inside the crystal ensures splitting each of them into two waves with different wave vectors. One such wave is weakly absorbed and another strongly.

Notice once more that in Refs. [7-15] the electromagnetic waves and neutrons were described by plane waves. At the same time, in typical experiments on the Laue diffraction the incident waves first pass a narrow slit and only afterwards penetrate into the crystal (see Fig.1). In this case the incident neutrons are described already by a wave packet written as the integral over the angle. Moreover, both the refracted and diffracted waves travel inside the crystal within the region, confined by so-called Borrmann triangle [20-25]. The distribution of diffracted beam intensity along the basis of the Borrmann triangle oscillates due to interference of two waves, transmitting the crystal with different wave vectors. The same interference provides also the familiar Pendellösung effect [20-24].

Kato [26-29] developed a theory for such a diffraction, assuming the angular dispersion of incident x-ray waves to be much larger than a small diffraction interval of the order of several seconds of arc. Although Kato told about the diffraction of spherical waves emitted by a point-like source, in reality he considered the cylindrical waves, emitted by the thread-like source. More exactly, the collimating entrance slit has been regarded like the continuous line of such point emitters, stretched along the slit.

Shull [30-32] used the Kato’s theory in order to interpret the results of his Laue diffraction experiments of neutrons in perfect crystals of silicon and germanium. Measuring the period of interference oscillations for the diffracted neutron beam he determined with high precision the coherent scattering lengths of neutrons by the nuclei of silicon [30] and germanium [32]. These experiments were repeated later by Abov and Elyutin [5, 6].

Worth noting also the papers [33-37], studying the Laue diffraction of neutrons in large silicon crystals at the Bragg angle close to . In these conditions the authors observed anomalous absorption and slowing down of neutrons. Moreover, they hoped to verify the equivalence principle of the inertial and gravitational masses on the example of such microscopic object as neutron and achieve higher accuracy .

Previously we analyzed the symmetric Laue diffraction of divergent neutron beams [38] in strongly absorbing crystals, taking into account both the potential and resonant neutron scattering by nuclei. Following Kato [26-29], we took the angular dispersion of the incident neutrons much exceeding the characteristic angular interval , where the diffraction proceeds. In other words, a real angular distribution of neutrons in this approximation was replaced by a constant. The analogous theory for the symmetric Laue diffraction of the Mössbauer radiation has been developed in [39].

In the present paper we study general case of the Laue diffraction, when the reflecting crystal planes are canted at arbitrary angle with respect to the crystal surface. For the first time the angular distribution of incident neutrons is included into consideration with dispersion , which may be of the order of the diffraction angular range . For calculation of the angular integrals, which determine the neutron wave packet inside a thick crystal, we use the saddle-point method. It is more adequate for strongly absorbing crystals than the stationary-phase method, which has been used previously in the theory of x-rays diffraction in weakly absorbing crystals [24]. Note that in the Kato’s approximation, when the function is replaced by a constant, these angular integrals are calculated exactly [24]. However, in our approach due to the factor we need estimations of the integrals by means of the saddle-point approximation for thick enough crystals.

We consider typical experimental situation (see, e.g., [30-32]), when the neutrons pass first through the entrance slit cut in a shield and then move inside the crystal within the Borrmann triangle. We assume that all the neutrons fall perpendicularly to the collimating slit, which in turn is parallel to the reflecting crystal planes. First we shall regard the slit as a thread-like emitter. In this case the neutron waves have a cylindrical symmetry with the symmetry axis along the slit. And in the fourth section we analyze the role of finite width of both slits used in experiments.

## 2 Basic formulas

Let the incident neutrons at be described by the initial wave packet

 Ψin(r,t)=∫dκ(2π)3f(κ)eiκr−iEt/ℏ, (1)

where are the wave vectors of neutrons, is their energy and the mass. The product is interpreted as a probability of finding the neutron with the wave vector lying in the interval beside . For brevity, we omit the spin factor, which does not affect the coherent scattering by nonmagnetic crystal with unpolarized nuclei.

We introduce the right-hand coordinate frame with the origin on the entrance surface in the middle of the collimating slit. The axis is directed inside the crystal perpendicularly to its surface and the axis along the slit (see Fig.1). One introduces also the frame with the axis parallel to the reflecting crystal planes and axis coinciding with . It is obtained from by rotation through the angle around the axis . Here for clockwise rotation and otherwise. The angle between the neutron wave vector and the axis is , the incidence angle on the reflecting planes is and the Bragg angle

Besides, we introduce the angles and between the axis and the sides of the Borrmann triangle, corresponding to transmitting and diffracted rays ( and ).

Let the divergent beam of neutrons move in the plane perpendicularly to the slit and be spread over the angle . Then , while the components of along the axes are

 κ(θ)={κcosφ,κsinφ,0}, (2)

where .

The wave function (1) may be rewritten as

 Ψin(r,t)=∫∞0Ge(E)ΨinE(r)e−iEt/ℏdE, (3)

where characterizes the energy distribution of incident neutrons, the function

 ΨinE(r)=∫π−πGa(θ)eiκ(θ)rdθ (4)

describes neutrons with fixed energy . We approximate the angular distribution by the Gaussian function with maximum at the angle close to the Bragg angle :

 Ga(θ)=1(√2πσ)1/2exp{−(θ0−θ)24σ2}, (5)

where

 σ2=⟨(θ0−θ)2⟩ (6)

denotes the mean-square angular dispersion of neutrons. Usually , that enables us to spread the integration limits over from to . If much exceeds the diffraction interval , then can be replaced by a constant.

The energy distribution is also described by the Gaussian function:

 Ge(E)=1(√2πσe)1/2exp{−(E−¯E)24σ2e}. (7)

We shall consider scattering of the neutron wave by atomic nuclei in the crystal, ignoring influence of the electrons. Then the coherent scattering of neutrons by an elementary cell of the crystal from the state to is determined by the amplitude

 F(κ,κ′)=∑jeiQρj¯fj(κ,κ′), (8)

where is the scattering wave vector, the radius-vector defines equilibrium position of the th atom within the elementary cell, is the coherent scattering amplitude of low-energy neutrons by the th nucleus:

 ¯fj(κ,κ′)=−¯bje−Wj(Q)+¯fresj(κ,κ′), (9)

where is the coherent scattering length of neutrons by the th nucleus, is the square root of the Debye-Waller factor, is the coherent resonant scattering amplitude. In vicinity of an isolated resonance it is given by

 ¯fresj(κ,κ′)=−cj(2Ie+12Ig+1)Γn2κ0 (10)
 ×∑{n′s}⟨(exp[−iκ′uj]){n0s}{n′s}(exp[iκuj]){n′s}{n0s}E−E0−∑sℏωs(n′s−n0s)+iΓ2⟩,

where is the probability of finding the resonant isotope in the th site, is the spin of the ground state of the initial nucleus and the spin of the excited state of the compound nucleus, is the energy of the resonant level, is the total width, consisting of the partial widths for neutron , radiation and possibly fission decay channels, is the displacement of the th nucleus from the equilibrium position, and are sets of phonon numbers in the initial and final states of the crystal, are the phonon frequencies, the brackets denote averaging over the initial states of the crystal lattice.

The sum in Eq.(10) can be transformed to the integral:

 ∑{n′s}⟨...⟩=−ie−Wj(κ)e−Wj(κ′) (11) ×∫∞0dtℏei(E−E0)t/ℏ−Γt/2ℏ+φj(t),

where is the Lamb-Mössbauer factor,

 φj(t)=∑sℏ2MjNωs××[yjs¯nseiωst+y∗js(¯ns+1)e−iωst] (12)

and

 yjs=(κvjs)(κ′v∗js), (13)

is the mass of the th atom, is the number of elementary cells, is the average number of phonons of the th normal vibration with polarization .

In the framework of the Debye model of the crystal with one atom per the elementary cell, ignoring anisotropy of vibrations, one can rewrite this expression as (see also [40])

 φj(t)=32(p⋅p′)M(kBΘD)3∫ωmax0ℏ2ωdω (14) ×[¯nωeiωt+(¯nω+1)e−iωt],

where and are the initial and final momenta of neutrons, is the Debye temperature, is the maximal frequency of phonons.

In such Debye approach the parameter is given by [41]

 W(κ)=3RkBΘD(TΘD)2∫ΘD/T0[1ez−1+12]zdz, (15)

where represents the recoil energy of the nucleus with mass .

In the approximation of fast collisions, when , the expression (11) reduces to

 ∑{n′s}⟨...⟩=e−Wj(Q)E−E0+iΓ2. (16)

This approximation is well fulfilled for low-lying resonances. Specifically, for the CdS crystal with parameters of the neutron resonance  eV,  meV,  meV [42] and K one has .

## 3 The wave function

According to collision theory [43] every plane wave of the wave packet (4) is scattered independently of each other, giving rise to the wave function . Therefore the neutron wave packet, born by the incident wave Eq. (4) takes the form

 ΨE(r)=∫∞−∞dθGa(θ)ψκ(θ)(r), (17)

In the two-wave case the wave inside the crystal as , where is the crystal thickness, consists of the refracted wave with the wave vector and the diffracted one with the wave vector , where denotes a reciprocal lattice vector. The components of the vectors and along the entrance surface coincide. Therefore the vectors with can be written as

 kν(θ)=κν(θ)+δ(θ)n,κ1(θ)=κ0(θ)+h, (18)

where is the unit vector along the axis .

As a consequence, the wave function inside the crystal transforms to

 ΨE(r)=∑ν=0,1Ψ(ν)E(r), Ψ(ν)E(r)=∫∞−∞dθGa(θ)ψκν(θ)(r), (19)

with given by

 ψκν(θ)(r)=∑ι=1,2C(ι)ν(θ)eiκν(θ)r+iδι(θ)x. (20)

Following [8] we introduce the notations

 k0(θ)=κ[1+ε0(θ)],k1(θ)=κ[1+ε1(θ)]. (21)

The parameters are related by

 ε1=α/2+γ1ε0/γ0, (22)

where

 α=2κ(θ)h+h2κ2,γν=cosφν. (23)

The means the refractive index for the incident wave .

Recall that are the angles between the vectors and the axis . The angle indicates deviation from the exact Bragg condition corresponding to . For neutrons with fixed energy [21]

 α=2sin2θBΔθ, (24)

where

 Δθ=θ\scriptsize{B}−θ. (25)

The corrections to the wave numbers in the medium are related with the parameters by

 δ(θ)=κε0(θ)/γ0. (26)

The amplitudes and the wave vectors are determined by the system of fundamental equations of the dynamical scattering theory [24]. For the two-wave case in notations of Ref. [8] they are written as

 (k2(θ)/κ2(θ)−1)C0=g00C0+g01C1, (k21(θ)/κ2(θ)−1)C1=g10C0+g11C1. (27)

The scattering matrix is defined by the expression

 gμν=4πκ2v0F(κν,κμ),μ,ν=0,1, (28)

where stands for the volume of the elementary cell.

The system of two equations (3) has the following solution [8]:

 ε(1,2)0=14[g00+βg11−βα]±14{[g00+βg11 (29) −βα]2+4β[g00α−(g00g11−g01g10)]}1/2,

where

 β=γ0/γ1. (30)

Henceforth the root with sign plus is associated with and minus with .

It is more convenient to express them in terms of new deviation parameter

 η=12(βg01g10)1/2(α−α0), (31)

where the angular shift

 α0=g11−g00/β. (32)

Note that is already a complex number.

Then the parameters take simple form

 ε(ι)0=12g00−12√g01g10β[η+(−1)ι+1√1+η2] (33)

and , defined by Eq.(26), may be written as

 δι(η)=κg002γ0−πΛL[η+(−1)ι+1√1+η2], (34)

where

 ΛL=2πγ0κ√g01g10β (35)

means the Pendellösung distance in the case of weakly absorbing crystals (see, e.g., [24]).

For the Laue diffraction () the amplitudes of the waves satisfy the following boundary condition at :

 ∑ι=1,2C(ι)0(θ)=1,∑ι=1,2C(ι)1(θ)=0. (36)

Being expressed in terms of the variable , they take the form

 C(ι)0(η) =12[1+(−1)ιη√1+η2], C(ι)1(η) =(−1)ι2(g10g01)12√β1+η2. (37)

Let us express the angular distribution as a function of . By means of Eqs. (24) and (31), one finds first the relation between the departures and :

 θB−θ=Δϑη−ΔθB, (38)

where

 Δϑ=1sin2θB√g01g10β,ΔθB=−α02sin2θ\scriptsize{B}. (39)

Here has a sense of the characteristic diffraction range, corresponding to variation of from zero to unity.

According to (3) the maximal amplitude of the diffracted neutron wave is achieved at , i.e. if

 θ=θ′B,θ′B=θB+ΔθB. (40)

From here we see that can be interpreted as the Bragg angle shifted by .

Assuming that the incident beam is oriented along the corrected Bragg angle, , we rewrite the angular distribution as

 Ga(θ)→Ga(η)=1(2π¯¯¯¯¯η2)1/4exp⎧⎨⎩−η24¯¯¯¯¯η2⎫⎬⎭, (41)

where the mean-square width

 ¯¯¯¯¯η2=(σ/Δϑ)2. (42)

From definition of it follows also that

 Ga(θ)dθ=−√ΔϑGa(η)dη. (43)

The neutron intensity distribution over the basis of the Borrmann triangle is usually analyzed with the aid of the scanning slit, located on the rear surface and directed along the axis z. Let be the radius vector of any point inside this slit, while be the coordinate of the midpoint E on the side AB of the Borrmann triangle. Following [24] we determine the reduced coordinate of this point as

 p=ΔySL, (44)

where is the length of the line segment AB, is the coordinate of the point relative to the midpoint E. The definition (44) is equivalent to

 p=2ΔyS/Dtanφ0−tanφ1, (45)

which in the case of symmetric diffraction, , reduces to the definition of , given in Refs. [22, 26]:

 p=tanϵtanθ\scriptsize{B}, (46)

where is the angle between the reflecting planes and the direct line CS, connecting the entrance slit and the point (see Fig. 1).

It remains now to expand the plane wave in the point in powers of . Keeping the linear terms in the expansion of and introducing the notation we get

 eiκ(θ)r=exp[iκDsinφ0(1−ys/Dtanφ0)Δθ] (47) ×exp{iκ0r}.

With the help of relations

 tanφ0+tanφ1=sin2φnγ0γ1 (48)

and

 tanφ0−tanφ1=sin2θBγ0γ1, (49)

 φ0+φ1=2φn,φ0−φ1=2θB, (50)

we find that

 ΔyS/D=12γ0γ1[sin2φn+psin2θB]. (51)

Substitution of this formula into (47) after some trigonometric manipulations gives

 exp{iκ(θ)r}=exp{iκD4γ1(1−p)α0} ×exp{iπDΛL(1−p)η}eiκ0r. (52)

Taking also into account Eq. (34), we are led to the following expression for the waves in the exit slit:

 exp{iκ(θ)r+iδι(θ)D}=Φ(p;E) (53) ×exp{−iπDΛL[pη+(−1)ι+1√1+η2]}eiκ0r,

where we used the abbreviation

 Φ(p;E)=exp{iκD4[g00γ0+g11γ1+p(g00γ0−g11γ1)]}. (54)

Substituting (3) into Eqs. (3), (20) and introducing the notations

 N=πD|ΛL|, (55)
 Sι(η)=−i(|ΛL|/ΛL)[pη+(−1)ι+1√1+η2], (56)

one finds the integral representation for the wave function in the point :

 Ψ(ν)E(r)=−Φ(p;E)√Δϑ (57)
 ×∫CdηGa(η)∑ι=1,2C(ι)ν(η)eNSι(η)eiκνr,

where the integration path in the complex plane is a direct line, defined by the condition Im

For a crystal, whose thickness , the large parameter allows us to estimate the integral over with the aid of the saddle-point method (see, e.g., [44]). Here we assume that as well as are smooth functions. First from the equation one finds the saddle points:

 η(ι)0=(−1)ιp√1−p2. (58)

Since the integrand in (57) is an analytical function one can deform the integration contour on the complex plane . This contour should cross the th saddle point along the line which indicates a steepest decent of the function . Along such a line Im const and the function Re  is maximal in the point . These requirements are satisfied if the line is directed with respect to the real axis at the angle

 ϑι=±π2−12arg\leavevmode\nobreak S′′ι(η0), (59)

where the second derivative of in the saddle point equals

 S′′ι(η0)=i(−1)ι(|ΛL|ΛL)(1−p2)3/2. (60)

Inserting (60) into (59) one finds that at

 ϑι=(−1)ιπ4+arg√ΛL. (61)

Evaluating the integral (57) with the aid of the saddle-point method, one has

 Ψ(ν)E(r)=−√ΔϑGa(η0)Φ(p;E) ×∑ι=1,2C(ι)νeNSι(η0)√2πN|S′′ι(η0)|eiϑιeiκνr, (62)

where the amplitudes in the saddle points are

 C(ι)0=12(1+p), (63) C(ι)1=(−1)ι2(g10g01β)12√1−p2,

while the angular factor

 Ga(η0)=1(2π¯¯¯¯¯η2)1/4exp⎧⎨⎩−14¯¯¯¯¯η2p2|1−p2|⎫⎬⎭. (64)

Substituting (60), (61) and (63) into (3), one gets the wave function of neutrons in the point inside the scanning slit. For the refracted neutrons the wave function is

 Ψ(0)E(r)=12A0(p)(1−p2)1/4(1+p1−p)12Φ(p;E) (65)
 ×√2ΛLD[eiζ(p)+e−iζ(p)]eiκ0r

and for the diffracted those

 Ψ(1)E(r)=12A1(p)(1−p2)1/4Φ(p;E) (66)
 ×√2ΛLD[eiζ(p)−e−iζ(p)]eiκ1r,

where

 ς(p)=πDΛL√1−p2+π4. (67)

and the amplitudes are

 A0(p)=−√ΔϑGa(η0),A1(p)=(g10g01β)12A0(p). (68)

The corresponding intensities of the monochromatic neutron beams are determined by

 Iν(p;E)=|Ψ(ν)E(p)|2. (69)

Introducing the notation

 1ΛL=1τL+i1σL, (70)

we get the following intensity distribution of the refracted beam through the basis of the Borrmann triangle :

 I0(p;E)=|A0(p)|2√1−p2(1+p1−p)e−μD2|ΛL|D (71)
 ×[sinh2(πDσL√1−p2)+cos2(πDτL√1−p2+π4)],

while for the diffracted beam distribution one has

 I1(p;E)=|A1(p)|2√1−p2e−μD2|ΛL|D (72)
 ×[sinh2(πDσL√1−p2)+sin2(πDτL√1−p2+π4)].

Here

 μ=12[μ0γ0+μ1γ1+p(μ0γ0−μ1γ1)], (73)

and are the absorption coefficients for neutrons incident far from the Bragg condition , no diffraction), but having the wave vectors and , respectively. They are determined by

 μν=κImgνν=σt(κν)/v0, (74)

where is the total cross section for scattering and absorption of neutrons by an elementary cell, which have in the initial state the wave vector . In accordance with the optical theorem [45]

 σt(κν)=4πκImF(κν,κν). (75)

Outside the Borrmann triangle in close vicinity to the points these intensities are

 I0(p;E)=|A0(p)|2√p2−1∣∣∣1+p1−p∣∣∣e−μD2|ΛL|D (76)
 ×[sinh2(πDτL√p2−1)+sin2(πDσL√p2−1+π4)],

and

 I1(p;E)=|A1(p)|2√p2−1e−μD2|ΛL|D (77)
 ×[sinh2(πDτL√p2−1)+cos2(πDσL√p2−1+π4)],

Outside the Borrmann triangle the intensity of the diffracted neutrons (77) in strongly absorbing crystal first quickly falls down and then begins to grow with increasing due to the hyperbolic sine. But in this region our approach is not valid, since the departure becomes too large.

In order to illustrate the role of the resonant scattering we have done numerical calculations for the symmetric Laue diffraction in an isotropic crystal containing single resonant nucleus in every unit cell. We neglected the potential scattering amplitude compared to the resonant one. The latter was described by Eq. (16) with the Debye-Waller factor . In this approximation the absorption coefficient, depending on the detuning of the resonance , is written as

 μ(x)=μres1+x2, (78)

where is the resonant value of the absorption coefficient, given by

 μres=4πκ2v0(2Ie+12Ig+1)ΓnΓ. (79)

As to the functions and , they are determined by the following expressions:

 1τL=−μres2πγ0xe−W(Q)1+x2,1σL=μres2πγ0e−W(Q)1+x2. (80)

Intensities of the diffracted and refracted beams as functions of , calculated in units of with and are presented in Figs.  2, 3 for and in Figs. 4, 5 for more thick crystal with .

## 4 Averaged intensities

Remind that up to now we dealt with the waves ejected from the thread-like source with the coordinates and changing from to . And now we shall analyze the role of finite width of the entrance slit, regarding it as a sum of the parallel thread-like sources, spread over the interval , which corresponds to variation of the coordinate in the interval of the width . In the case of symmetric diffraction .

The neutron wave in any point of the scanning slit is a superposition of the waves emitted by every such thread and afterwards passing the crystal region, confined by their own Borrmann triangle. The resulting waves in the point will be

 ~Ψ(ν)E(p)=∫Δp/2−Δp/2Ψ(ν)E(p+ξ)dξ, (81)

The corresponding integral intensity

 ~Iν(p)=∫∞0|Ge(E)|2|~Ψ(ν)E(p)|2dE. (82)

Besides, when the scanning slit has the width , the intensity should be integrated over from to , where denotes the coordinate of the slit’s middle. So the flux of neutrons per unit time, emerging from the scanning slit in the th direction, is determined by

 Jν(¯p)=¯v∫¯p+Δp/2¯p−Δp/2~Iν(p)dp, (83)

where is the velocity bound to the average energy :

 ¯v=ℏ¯κ/m,¯κ=√2m¯E/ℏ. (84)

We compared our results with the data of Shull [30], who had observed the symmetric Laue diffraction of neutrons at (111) planes of silicon crystal. It has the diamond structure with the crystal constant  Å  and contains 8 atoms in the elementary cell [46]. A spacing of the adjacent (111) planes equals . The corresponding scattering amplitudes are

 F(κ0,κ0)=F(κ1,κ1)=−8¯b, (85) (F(κ0,κ1)F(κ1,κ0))1/2=4√2⋅¯be−W(Q), (86)

where the scattering vector and is an integer. We took .

In numerical calculations of the intensity we used the following experimental parameters: the wave length  Å, crystal thickness  cm, the coherent scattering length  cm and the factor [30]. The calculated dependence of