differs essentially from analogous term in the for- mula presented in [10]. Here we see the time parameter T ≫ 1 is found in the denominator. As was mentioned earlier, this parameter has a deep sense: as you move farther the source of the particles, its intensity on the grating becomes weaker. For exception of this effect, the term (21) does not exert influence on the interference pattern. Therefore, for short we will write this normalization factor as A . coefficients at k $^{2}$d2 emergent at decomposition ( x − kd ) 2 = x 2 − 2 kxd + ( kd ) $^{2}$. The point is that the terms at k $^{2}$d2 lead messed phases on infinity, due to which summation of that exponents gives zero contribution. Other sums with coefficients at x 2 and 2 kxd can be easily computed. As a result, intensity of the particle beam in the far-field region is as follows Let a screen, on which a monochromatic beam of the particle scatters, has N slits ( n = 0 , 1 , 2 , · · · , N − 1) located at equal distance from each other, as shown in Fig. 4. Here we have an origin of coordinates placed in the center of the slit grating. In this frame of reference, n -th slit has a position x$_{0}$ = ( n − ( N − 1) / 2) d , where d is a distance between slits. Further it is measured in units multiple to the wavelength λ . We need now to compute contributions of all paths passing from the source through all slits in the screen and farther to a point of observa- tion ( x, z ). Per se, we have to execute superposi- tion in the observation point of all Gaussian wave packets (20) from all slits n = 0 , 1 , 2 , · · · , N − 1. Such a superposition reads and probability density in the vicinity of the ob- servation point ( x, z ) is Hereinafter, the superscript 1 at x is dropped. Before we will take up interference effects in the near-field region and behavior of Bohmian trajectories here, let us consider an asymptotic limit of the formula (23) in the far-field region. With this aim in mind, we preliminarily replace the term ( n − ( N − 1) / 2) d in Eq. (22) by kd , where k runs ( − ( N − 1) / 2 , · · · , ( N − 1) / 2). Next, at summation we will neglect contribution of Let us now compare intensities of radiation from N slits in the far-field region computed by Eq. (23) and according to the approximated for- mula (24). Fig. 5 shows, in gray palette, a dis- tribution of the probability density (23) formed by radiation from N = 7 slits grating in the far- field region. Thermal neutrons are adopted here as incident particles on the N -slit grating. The wavelength is λ = 0 . 5 nm. Large red arrows in this figure point out directions of radiation of principal maxima having a big intensity. Short blue arrows, in turn, point out directions of sub- sidiary maxima having a low intensity. All near- It turns, this parameter is equivalent to the instantaneous Gaussian width presented in [8]. Emergence of the wavelength λ , in the above stated formulas, (25) and (26), is due to the de Broglie relation binding the momentum p$_{z}$ with the wave vector k$_{z}$ of the pilot wave, namely, ¯ hk$_{z}$ = h/λ = mv$_{z}$ = mz/τ . The parameter A is determined by Eq. (21), and σ$_{z}$ has a form Here terms ζ ( x, z ) and I$_{0}$ ( x, z ) read 7 III. ORDERED SEQUENCE OF THE SLITS | Ψ( x, z ) 〉 = 1 N N − 1 ∑ n =0 ψ$^{(}$x,$^{(}$n − N − 1 2 ) d, z$^{)}$, (22) p ( x, z ) = 〈 Ψ( x, z ) | Ψ( x, z ) 〉 . (23) σ$_{z}$ = σ$^{√}$ √ √ 1 + ( zλ 4 πσ 2 ) 2 . (26)          ζ ( x, z ) = xd zλ 4 πσ 2 2 σ 2 z , I$_{0}$ ( x, z ) = A 2 N $^{2}$σ$_{z}$ exp$^{{}$ − x 2 2 σ 2 z } . (25) I ( x, z ) = I$_{0}$ ( x, z ) sin$^{(}$ Nζ ( x, z ) 2 ) 2 sin$^{(}$ ζ ( x, z ) 2 ) 2 . (24)