Оператор давления для осциллятора Пёшля-Теллера

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1. Formation of the Model Some decades ago P¨oeschl and Teller [1] introduced a family of anharmonic PT-potentials U(), which allowed the exact solutions of the one-dimensional Schr¨odinger equation in the coordinate, or -representation [2, 3]. One of the most interesting member of the PT-family is the symmetric trigonometric potential, which is even in the variable , where - < < . U(, ) = U(-, ) = U0 tg2[()], (1) () = /2. At = the potential becomes singular, which physically means the presence of a pair of impenetrable walls. They confine the movement of the non-relativistic particle with positive constant mass . The parameters U0 and are also positive, though the limits U0 0 and are also allowable and will be considered properly. The presence of the walls is of specific interest for the future thermodynamic description of this model, placed into some thermostat. In contrast to ordinary harmonic oscillator (HO) for the PT-oscillator (PTO) it is possible to introduce the pressure operator ˆ(ˆ, ˆ, ) which according to Hellmann and Feynman [4, 5] is connected with the energy operator or the Hamiltonian (ˆ, ˆ, ) = ( ) + U(, ) by the formal relation: . (2) Strictly speaking, one should differentiate in (2) with the volume U = , where is dimension of the coordinate space, where = 1 will be held here everywhere. The important point is that the operation may be fulfilled only after the operator ˆ has acted upon some wave function - as a rule, upon the eigenfunction () of ˆ with eigenvalue (see, e.g., the detailed analysis in [4, 5]). The importance of this sequence of operations is directly connected with the account of boundary conditions ( ) = 0 at all values of . In this case the formal definition (2) acquires more definite sense: (3) Note, that in this paper we won’t be engaged with the eigenfunctions ( ) - it is sufficient to know that all of them contain the factor cos , which ensures the fulfillment of zero boundary condition at the walls = ± = ±. Following (7) one may see, in particular, that if the energy spectrum () is a uniform function of (e.g. () ∼ - > 0) so that () = )︁ (), or in the operator form: where ˆ() = (4) is the (linear) density of the energy; the last relation is the well known barocaloric equation of state for the ideal gas. Note that by obtaining (4) we have used Euler’s uniformity property d () = () valid for any real value of 2. Exact Energy and Pressure Spectra It is remarkable that the complication potential (2), leads to an exact solution of the Schr¨odinger equation with potential (1) with fully discrete positive energy levels () > 0 including the ground levels 1() : (5) obviously, the spectrum () is unbounded from above. Two terms in (5) look like the free particle in the box and harmonic oscillator respectively: (6) note, that (6) doesn’t contain terms of higher order in that quadratic one. The quantity () is equal to the well known minimal kinetic energy of the in the box with dimensions [-, ] : (7) The () quantity is the frequency of some HO, and depends upon () in much more complicated way than (7)). In this paper we won’t be engaged with the eigenfunctions () - it is sufficient to know that all of them contain the factor cos , which ensures the fulfillment of zero boundary condition at the walls = ± 2 = ±. Complicated method: , (8) . (9) Obviously, that the formal structure of the parameter () resemble the kinetic energy of the free relativistic particle with rest mass in (() is the like , where is the particle’s momentum) () ≥ 0 () = 0 only at the point = = 0 in the limit → ∞). Following the definition (3), one finds from (5) the exact diagonal matrix elements of the pressure operator (2): (10) (11) the Euler’s uniformity property: , (12) where we have used Euler’s The expressions (HO) and ( HO) are rather complicated since () is non-uniform function of pressure operator () for PTO is in general not proportional to the energy operator (), but in extreme case (FP and H-parts) this property is restored. At fixed , the relative contribution of the FP and HO depends upon and it’s determined by the ratio: . (13) Clearly, at () 1, () i.e for lower energy levels, the HO-part dominates, whereas at () 1, (), i.e, for higher energy levels, the FP-part dominates. This is easy to understand, because at 0 and held constant the growth of the particle’s energy makes the potential (1) more and more the limiting potential U(, ) = () + ( + ), which characterizes the FP in the box. In the last case we obtain he fully free particle without any “box”, so the particle’s energy is not quantized at all. The same limit at fixed is achieved at 0 = 0. Moreover, the FP-limit full at fixed is achieved also at the limiting point () = 0 or = 0, because in this case the potential (1) also is identically equal to zero. However, one should note that the limit of small, but finite () 1 resembles more not the FP-, but the HO-case. 3. FP- and HO-Limits for the Energy and Pressure Spectra It is instructive to consider the expressions (5) and (10) at fixed values of in two basic limiting cases, i.e. FP in the box and HO-limits. 3.1. FP in the Box Limit: = const, 0 → 0, () → ∞ In this case, () is large compared to 0, so (()) = 0 () ≪ 1, thus: Due to the general definition (8), the effective frequency is of the form: and tends to zero with 0. For the pressure operator ˆ in this limit the whole term (11) is negligible, so for ˆFP the linear operation, equation of state (4) holds, where = 2 and ˆFP 3.2. HO-Limit: 0 = const, → ∞, () ∼ () → 0 In this case, () ∼ 2() is small compared to the effective frequency in the lowest order HO-approximation п() = () ∼ 02() here: is a large quantity. More precisely, from (8) follows that further, using again (8), one obtains . (15) Here (16) is of order (), while the second and third term in (15) are of the order 2() and 3() accordingly. The pressure operator ˆ in this limit may be found from (15) by noticing that both terms in the rhs of the equation make contributions of opposite sign, but of the same (lowest) order (). Indeed, in this limit ()() ≈ ()() = п˜() and (17) Combining relations (16) and (17)) one finds for the pressure operator ˜HO, as well as for ˜FP, the linear operator equation of state (4) holds, but now with = 1 and effective Hamiltonian: which describes some “confined” HO. 4. Approximations for the Energy Spectrum 1. Quasi-Classical Approximation (QC) It is instructive to compare the exact energy spectrum (5) with its QC-counterpart, for which the quantization rule states that for = 1, 2, 3, . . . , (18) here .J() is the classical action for the PT oscillator with the potential energy (1) while (, ) is the classical momentum , (19) obviously, 0() as . The Bohr-Sommerfeld quantization takes the explicit form: (20) so that the QC energy spectrum will be of the same form as in (5)-(6). The only difference is that the exact quantity () in the QC-case will be substituted by it’s QC-analogy . It is easy to verify that, all the basic features of the PT-oscillator remain just the same (up to some numerical factors). 2. Perturbation Theory Consider the expansion of the potential: , (21) which is plausible when both () and are small. The leading term in (21) may be written down as the usual HO-potential: where the frequency ˜2() is the same as defined by (15). It may seem rather unpleasant that ˜2() goes to zero with () at → ∞, and so one may ask for the usual constant HO-frequency 0 = ( = const). Such a result may be achieved simply by means of the potential intensity U0 ( )-2(). Note, that in this case as the limit point (). One arrives strictly to the usual HO-oscillator (but not the PT-oscillator). Indeed, the suggested rescaling can’t save “all the next order terms in the expansion” (21). Moreover, at this limiting point the notion of pressure (the operator as well as it’s spectrum becomes meaningless, so that we don’t use this “scaling trick” - as well as the point () = 0 in the followings though the HO-limit () 1 is quite appropriate) . Consider now the term of the lowest order () 4 in (21) as the weak an harmonics them the energy spectrum is of the form [2, 3]: , (22) ∆() = where = 0, 1, . . .. Making the shift → ( - 1): (23) Two effects are evident once from (23). Firstly, the linear in part of ∆() brings for the non-perturbated spectrum ˜HO() equal to [ ()], which agrees with the correction of the same order in (2) the full expansion. Secondly, the quadratic in n part reproduces the term FP() from the exact energy spectrum (6). Unfortunately, the next approximation (e.g. of orders ()6 and/or ()8 tend to spoil these nice results. In particular, they bring in () so, “non-physical” terms of orders 3, 4, etc. and also deform the term ()2, which should not be affected at all. 5. Conclusion In this paper the quantum-mechanical properties of the strongly non-linear quantum oscillator in the P¨oeschl-Teller model were considered. In Sec. 1 the formulation of the model was given and its relations with two well known models - i.e., the free particle in the box and the harmonic oscillator were considered. Sec. 3 was devoted to the analysis of the fully discrete spectrum of the model; also, using the Hellman-Feynman theorem the pressure operator was obtained and analyzed. namely, both the “free particle in the box” and “harmonic oscillator” limits were given the detailed investigation. Finally, in Sec. 4 some approximations for the energy spectrum are considered - namely, the quasi-classical one as well as the perturbation theory in the region near the harmonic one - i.e., were the anharmonic terms are relatively small. All the results obtained here will be used for the thermodynamic calculations in the nearest future publication.

Об авторах

Юрий Григорьевич Рудой

Российский университет дружбы народов

Автор, ответственный за переписку.
Email: rudikar@mail.ru

Кафедра теоретической физики и механики

ул. Миклухо-Маклая, д. 6, Москва, Россия, 117198

Енок Олуволе Оладимеджи

Российский университет дружбы народов

Email: nockjnr@gmail.com

Кафедра теоретической физики и механики

ул. Миклухо-Маклая, д. 6, Москва, Россия, 117198

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