The parabolic equation (nonlinear Schrödinger equation) that appears in problems of stationary nonlinear beam propagation (self-focusing) is reconsidered. It is shown that an additional term, which involves changes of the propagation constant along the propagation direction, should be taken into account. The physical consequences of this departure from the standard approximation, which uses the parabolic equation, are discussed. A numerical simulation showing the difference between the new approach and the standard nonlinear Schrödinger equation is given as an example. © 1993 Optical Society of AmericaPeer Reviewe

Jirawit

Makhotkin

Matyi

Monaco

Nannarone

Nayak

Platonov

Serafinczuk

Spiga

Windt

Sertsu, M. G.

Giglia, A.

Brose, Sascha

Comisso, A.

Wang, Z. S.

Juschkin, Larissa

Nicolosi, P.

Publikationsserver der RWTH Aachen University

Optical and structural characterization of CeO2/B4C multilayers near boron K-edge energy

A search for novel materials for making multilayers of high reflectivity has been driven by the vigorous demand towards miniaturizing photonics. A typical consumer of high performance multilayers (MLs) is the extreme ultraviolet lithography (EUVL) based on the 13.5 nm laser produced plasma (LPP) source. To sustain “Moore’s law” and print fine features below 10 nm on integrated circuits (IC), source of radiation for the EUVL has to shift towards even shorter wavelengths where 6.x nm wavelength seems to be immediate successor. However, the 6.x nm EUV lithography needs MLs of reflectivity performance above 70 % to support high volume manufacturing (HVM). It is clear that more work is required particularly on the development of MLs with high reflectance, stable to thermal heat and sufficient lifetime. In this work new MLs of B4C/CeO2 are deposited, analyzed and characterized for the first time. Combinations of X-ray reflectometry (XRR) and EUV reflectance measurements near resonance edge of boron are analyzed to derive structural and optical parameters of MLs. ML coatings of B4C/CeO2 MLs have shown similar reflectance performance with the leading candidate MLs around 6.x nm wavelength. Analysis shows that interlayer diffusion is a major reason for low reflectivity performance. Cross-sectional scanning electron microscopy (SEM) images of the MLs have proved formation of interlayer diffusion

SERTSU, MEWAEL GIDAY

NICOLOSI, PIERGIORGIO

A. Giglia

S. Brose

A. Comisso

Z. S. Wang

L. Juschkin

Archivio istituzionale della ricerca - Università di Padova

Optical and structural characterization of CeO2/B4C multilayers near Boron K-edge energy

RWTH Publications

M. G. Sertsu

P. Nicolosi

Crossref

Akhmediev, N.

Ankiewicz, A.

Soto Crespo, J. M.

Digital.CSIC

March 15, 1993 / Vol. 18, No. 6 / OPTICS LETTERS 411Does the nonlinear Schrodinger equation correctlydescribe beam propagation?Nail Akhmediev and Adrian AnkiewiczOptical Sciences Center, Institute of Advanced Studies, Australian National University, Canberra, ACT 2601, AustraliaJose Maria Soto-CrespoInstituto de Optica, Consejo Superior de Investigaciones Cientificas, Serrano 121, 28006 Madrid, SpainReceived November 17, 1992The parabolic equation (nonlinear Schrodinger equation) that appears in problems of stationary nonlinear beampropagation (self-focusing) is reconsidered. It is shown that an additional term, which involves changes of thepropagation constant along the propagation direction, should be taken into account. The physical consequencesof this departure from the standard approximation, which uses the parabolic equation, are discussed. Anumerical simulation showing the difference between the new approach and the standard nonlinear Schr6dingerequation is given as an example.The effects of self-trapping and self-focusing oflight beams in nonlinear media were predictedin the early 1960's.1-3 The evolution of lightbeams in self-focusing media has been described bythe parabolic equation [the nonlinear Schr6dingerequation (NLSE)] since the first studies devotedto this question.4 5 This equation takes diffractionand nonlinearity into account in a simple way anddescribes the field evolution with high accuracy,unless time dependence and dispersion are involved.6Thus, the parabolic equation is a convenient ap-proximation; it provides the possibility of using apowerful tool such as the inverse-scattering method7for its investigation. In fact, a variety of exactsolutions can be obtained for the one-dimensionalNLSE by using even simpler approaches.8 Thisequation, with variable coefficients adjusted for alayered medium, has been used widely for describingnonlinear wave propagation in optical waveguidesand interfaces.9 "14 It is also important to notethat many fast and convenient calculation methodshave been developed15 for numerical simulations ofsolutions of the parabolic equation.Unfortunately, this equation has limitations thathave not been discussed before and that areconnected with the approximation of slowly varyingamplitude. As can be seen in what follows, somephysical implications of this equation can even bemisleading and turn out to be in contradictionwith the general theory of wave propagation. Thequestion arises: Is approximation by the parabolicequation good enough to describe nonlinear guided-wave phenomena in their full complexity?In this Letter we show that the parabolic equationis a good approximation, unless stationary (in thelongitudinal direction) solutions (like self-trapping2and stationary nonlinear guided waves9 -'4 ) or so-lutions close to them are considered. If the beamhas any longitudinal variation during propagation, as0146-9592/93/060411-03$5.00/0happens in most cases of interest, then the equationshould be completed by an additional term describinglongitudinal field oscillations. This additional termallows us to present a clear physical interpretation ofthe conserved quantities involved.For simplicity we start from the scalar waveequation for a three-dimensional field E(x,y,z) in amedium":E.d, + Eyy + Ezz - e(x, IEI) alE = o~~ ±E~~2 c2t (1)where E is a scalar (y-component) optical fieldand e(x, IEI) is the intensity-dependent dielectricpermittivity:e(x, IEI) = e,(x) + ci(x)1E12 .Here e1(x) is the linear part of the transverse profileof the dielectric permittivity of the layered mediumand a(x) is the transverse profile of the nonlinearsusceptibility. In order to include layered media inthis analysis we allow e and a to depend on x. Thisis relevant to problems of nonlinear guided waves.9 -14In the particular case of a homogeneous medium, theyare constants. The averaged dielectric permittivitydoes not depend on time. The field is assumed to bestationary (in time) and monochromatic:E = 0(x,y,z)exp(-i&)t).For convenience, we normalize the coordinates x, y,and z by using the free-space wave number k = co/c:(2)XI zz + VXx ++ el(X) /I + a(x)Iti2i = 0.We seek a solution of Eq. (2) of the formqi(x,z) = B(x,y,z)exp[i~p(z)].We assume that the amplitude function B(x,y,z) isslowly varying and that all fast oscillations are in-cluded by means of the phase function sp(z). Usually,© 1993 Optical Society of America(3)412 OPTICS LETTERS / Vol. 18, No. 6 / March 15, 1993in the approximation of slowly varying amplitude, weset p (z) = /3z + spo, with /3 = constant. In this case,fast oscillations are still implicitly included in thefunction B(x,y, z). However, the second derivative ofthis function is then not small and cannot be droppedcompletely.There can be some degree of arbitrariness in sep-arating the fast oscillatory part from the functionB(x,y,z) if the beam divides into two or more beamsduring propagation. In this instance it is more con-venient in numerical simulations to keep /3 constant,as is usually done. The correction to the real value of,/ (separate for each beam) can then be extracted fromthe results by calculating the period of longitudinaloscillations of B(x,y,z) at the center of each beam.On the other hand, the correct initial separationproduces physically important consequences as wellas crucial differences in numerical results, as weshow below.We assume that we have only one beam as asolution of Eq. (1), so that the function IB(x,yz)Ihas only one maximum at any fixed z and that itapproaches zero at x = o. Substituting Eq. (3) intoEq. (2), we obtainB,, + Bx + By + 2impB, + i~p22B-q(Z2B + e,(x)B + a(x)IB12B = 0. (4)The term B,, can be omitted from Eq. (4), as isusual in the slowly varying amplitude approximation.However, this can only be done if B(x,y,z) does notinclude any fast field oscillations in the z direction.With our definition, the rapidly oscillating part of thesolution is included by means of the function so(z) insuch a way that the function B(x,y, z) maintains con-stant phase at the center of the beam where IB(x,y, z)Ihas its maximum. If the beam center is located at(x,y) = (0,0 ) then we can define the function so (z) insuch a way thatarg[B(x = O,y = 0,z)] = constant, (5)where B(0,0,z) has been written as IB(0,0,z)l xexp[i arg B(0, 0, z)]. This in turn means that theratio of the imaginary to the real part of B(0, 0,z),i.e., Im[B(0, 0, z)]/Re[B(0, 0, z)], remains constant.Equation (5) defines the functions o(z) and B(x,y,z)uniquely.Let us now define the function /3 asfi(z) = d, (6)dzThis is the instantaneous propagation constant at agiven cross section z. This function is also defined ina unique way. Now we can write Eq. (4) in the form2ifiBz + ifizB + Bc, + B - f_ 32B+ el(x)B + a(x)IB 12B = 0. (7)In the case of constant 1i, this equation obviouslycoincides with the standard parabolic equation forstudying the propagation of nonlinear guided waves.The second term in Eq. (7), which can be of the sameorder as the first one, makes it different from theusual parabolic equation.Now let us turn to physical differences that ap-pear when we take this term into account. Consider,for example, the invariants of Eq. (7). By multiply-ing Eq. (7) by B*, taking the complex conjugate ofthis expression, and subtracting and integrating, weobtaind (/) = 0, (8)where I is the energy invariant for the standardparabolic equation [i.e., Eq. (7) without the secondterm]:I= EIB(x,y,z)I 2dxdy. (9)We can see now that the product HI, rather thanjust I, is the conserved quantity during propagation:/8(z)I(z) = constant. (10)This product Sz = jIi is proportional to the integratedenergy flow'6 in the z direction, i.e., to the z compo-nent of Poynting vector S = E X H integrated overthe cross section. It can also be called power1 orpower flow'8 crossing a given surface z = constant.This is the result that we would expect physically, be-cause in the general theory of wave propagation, theenergy flow is the quantity that has to be conservedin media without gain or loss. However, in the stan-dard approximation by the parabolic equation, thisconservation law is incomplete, and only the energyintegral I is conserved, as rapid oscillations are ne-glected when the term B,, is dropped. Of course, inthe case of constant /3, the energy invariant I itselfis conserved. This can happen only for stationarysolutions of Eq. (2). But in that case it is a trivialresult, as the function B(x,y) itself then does notdepend on z, and so neither will any integral of it.For any other solutions, we have to take into accountrapid field oscillations along the z axis.Let us now consider the second quantity conservedfor the parabolic equation, namely the Hamiltonian.For simplicity we restrict ourselves to the case of atwo-dimensional field B(x, z). It is now proportionalto the y component of the electric field. By multiply-ing Eq. (7) by dB*/dz, taking the complex conjugateof this expression, and adding and integrating overx, we obtainif dx/(z(BzB*-Bz*B) - 2f dx if/iIB12d 12 + (,B2 2= .dJ LIRI2 -,E,)1B1 - B 0.IB4(11)The sum of integrals in Eq. (11) is proportional tothe energy density of the optical field integrated overx per unit z. The first two integrals are the part ofthe energy density connected with the x component ofthe magnetic field (HX2). These two integrals becomeMarch 15, 1993 / Vol. 18, No. 6 / OPTICS LETTERS 41310C',NaM1l I l l I I I I I I . . I V l ' I . . ..l l l l - l -~~~~~~~~~~~~~~~~~~~~~~~~~~~~~~~0:-~~~~~~~~~~~~~~~~~~~~~~~I,I10 ' / j~~~~~~~~~~~~~~~~~~~~~~~~I I I 0 20 40 60 80 100zFig. 1. On-axis intensity versus normalized axial dis-tance z for the Gaussian initial condition (z = 0) ofEq. (12) found by using the standard NLSE (dashedcurve) and by using Eq. (7) (solid curve). Parameterschosen for these simulations are e1 = 24.50015104,,/(0) = 5.0, and a = 1.0.zero when ,3 is constant in the standard parabolicapproximation. Then the third integral is conservedalong z. It still can be considered as the energydensity per unit z. So, in the absence of currents,the integrated energy density is conserved along z.If /z is nonzero, then the whole Eq. (11) cannotbe represented in the form of a conservation law.The consequence is that the Hamiltonian [the thirdintegral in Eq. (11)] is no longer conserved.In order to show that the new equation gives re-sults that are different from the standard NLSEbut are consistent with the solutions of the waveequation, we present here one example of a nu-merical simulation to compare the two approaches.For this short communication we choose the moststriking example where the standard NLSE fails togive a correct result,'9 namely catastrophic beamcollapse in the two-transverse-dimensional NLSE.We have developed a modification of the Crank-Nicholson scheme that maintains a constant phaseof B(x,y, z) at (x,y) = (0,0) to simulate the solutionsof Eq. (7). We have verified during simulations thatthe invariant given by Eq. (10) is conserved to highaccuracy for a variety of initial conditions. Figure 1shows the on-axis intensity of the cylindrically sym-metric beam that initially (z = 0) has a Gaussianshape:B(x,y,z = 0) = exp( 8 ) (12)This initial condition has a power flow that is abovethe critical value and thus results in collapse whenthe standard NLSE is used. The parameters of thesimulation are given in the figure caption. It is seenfrom this figure that the standard NLSE leads tocollapse and that the on-axis field goes to infinityat finite z (-62.5). The solution of Eq. (7) deviatesfrom it for on-axis intensities IB(0, 0, z)12, which arebetween approximately 5 and 10, and then returnsto a more smooth beam propagation beyond the pointof collapse. This result is in qualitative agreementwith the numerical results of Refs. 19 and 20, wherethe authors use nonparaxial algorithms for simula-tion of the solution of the wave Eq. (2) to describebeam self-focusing. Thus the NLSE leads to an er-roneous physical conclusion.In summary, we have shown that the standardapproximation, which uses the parabolic equationand which is employed widely in the analysis ofnonlinear self-focusing and self-guiding, should becompleted with an additional term that takes intoaccount the variation of the propagation constantalong the propagation direction.Nail Akhmediev thanks Ewan Wright for fruit-ful discussions at the First Nonlinear Guided-Wave-Theory Workshop, Orlando, Florida, April 1992, andduring the Integrated Photonics Research Conferencein New Orleans, Louisiana, April 13-16, 1992.References1. G. A. Askar'yan, Zh. Eksp. Teor. Fiz. 42, 1567 (1962)[Sov. Phys. JETP 15, 1088 (1962)].2. R. Y. Chia, E. Garmire, and C. H. Townes, Phys. Rev.Lett. 13, 479 (1964).3. V. I. Talanov, Izv. Vyssh. Uchebn. Zaved. Radiofiz. 7,564 (1964) [Radiophysics 7, 254 (1964)].4. P. L. Kelley, Phys. Rev. Lett. 15, 1005 (1965).5. V. E. Zakharov, V. V. Sobolev, and V. S. Synakh, Zh.Eksp. Teor. Fiz. 60, 136 (1971) [Sov. Phys. JETP 33,77 (1971)].6. V. E. Zakharov and A. M. Rubenchik, Zh. Eksp. Teor.Fiz. 65, 997 (1973) [Sov. Phys. JETP 38, 494 (1973)].7. V. E. Zakharov and A. B. Shabat, Zh. Eksp. Teor. Fiz.61, 118 (1971) [Sov. Phys. JETP 34, 62 (1972)].8. N. N. Akhmediev, V. M. Eleonskii, and N. E. Kulagin,Theor. Math. Phys. 72, 809 (1987) [Teor. Mat. Fiz(USSR) 72, 183 (1987)].9. C. T. Seaton, G. I. Stegeman, and H. G. Winful, Opt.Eng. 24, 593 (1985).10. G. I. Stegeman, E. M. Wright, N. Finlanson, R. Zanoni,and C. T. Seaton, IEEE J. Lightwave Technol. 6, 953(1988).11. D. Mihalache, M. Bertolotti, and C. Sibilia, in Progressin Optics, E. Wolf, ed. (North-Holland, Amsterdam,1989), Vol. XXVII, pp. 229-313.12. N. N. Akhmediev, in Modern Problems in CondensedMatter Sciences, H.-E. Ponath and G. I. Stegeman,eds. (North-Holland, Amsterdam, 1991), Vol. XXIX,pp. 289-321.13. A. D. Boardman, P. Egan, T. Twardowski, and M.Wilkins, in Nonlinear Waves in Solid-State Physics,A. D. Boardman, M. Bertolotti, and T. Twardowski,eds. (Plenum, New York, 1990), pp. 1-50.14. S. Maneuf, R. Desailly, and C. Froehly, Opt. Commun.65, 193 (1988); J. S. Aitchinson, A. M. Weiner, Y.Silberberg, M. K. Oliver, J. L. Jackel, D. E. Leaird,E. M. Vogel, and P. W. E. Smith, Opt. Lett. 15, 471(1990).15. T. R. Taha and M. J. Ablowitz, J. Comput. Phys. 55,203 (1984).16. M. Born and E. Wolf, Principles of Optics, 6th ed.(Pergamon, Oxford, 1980).17. A. W. Snyder and J. D. Love, Optical WaveguideTheory (Chapman and Hall, London, 1983).18. H. A. Haus, Waves and Fields in Optoelectronics(Prentice-Hall, Englewood Cliffs, N.J., 1984).19. M. D. Feit and J. A. Fleck, J. Opt. Soc. Am. B 5, 633(1988).20. J. T. Manassah and B. Gross, Opt. Lett. 17, 976 (1992).