[
Abstract
Using the FeynmanPines diagram technique, the energy spectrum of localized quasiparticles interacting with polarization phonons is calculated and analyzed in the wide range of energies at the finite temperature of the system. It is established that the general model of the system, besides the bound states known from the simplified model with an additional condition for the operator of quasiparticles number, contains the new bound states even for the systems with weak coupling. The contribution of multiphonon processes into the formation of renormalized spectrum of the system is analyzed. The reasons of the appearance, behaviour and disappearance of separate pairs of bound states depending on the coupling constant and temperature are revealed. \keywordsquasiparticles, phonon, Green’s function, mass operator
\pacs71.38.  k, 63.20.kd, 63.20.dk, 72.10.Di
Abstract
Методом дiаграмної технiки ФейнманаПайнса розраховано i дослiджено енергетичний спектр локалiзованих квазiчастинок, взаємодiючих з поляризацiйними фононами у широкiй областi енергiй при скiнченнiй температурi системи. Показано, що загальна модель системи крiм зв’язаних станiв, вiдомих зi спрощеної моделi з накладеною додатковою умовою на оператор повного числа квазiчастинок, навiть зi слабким зв’язком мiстить новi зв’язанi стани. Виявлена роль багатофононних процесiв у формуваннi перенормованого спектру системи. Встановлено причини появи, еволюцiї та зникнення окремих пар зв’язаних станiв у залежностi вiд величини енергiї зв’язку та температури. \keywordsквазiчастинка, фонон, функцiя Грiна, масовий оператор
201619443701 \doinumber10.5488/CMP.19.43701 Properties and temperature evolution of the spectrum of localized quasiparticles]Properties and temperature evolution of the spectrum of localized quasiparticles interacting with polarization phonons in two models M.V. Tkach, Ju.O. Seti, O.M. Voitsekhivska, O.Yu. Pytiuk]M.V. Tkach^{†}^{†}thanks: Email: ktf@chnu.edu.ua , Ju.O. Seti, O.M. Voitsekhivska, O.Yu. Pytiuk \addressChernivtsi National University, 2 Kotsyubinsky St., 58012 Chernivtsi, Ukraine \authorcopyrightM.V. Tkach, Ju.O. Seti, O.M. Voitsekhivska, O.Yu. Pytiuk, 2016
1 Introduction
The theory of the renormalized energy spectrum of a system of quasiparticles interacting with phonons in a wide range of energies (containing bound states) and coupling constants has been attracting a permanent attention [1, 2]. The increased interest to the theory of quasiparticles interacting with the quantized fields (photons, phonons) is caused by the practical and fundamental prospects of their utilization.
As an example of practical use we should mention the important role of phonon and photon assisted tunneling of electrons through the multilayer resonant tunneling nanostructures (RTS), where, due to the interaction with the fields, the new states between which the quantum transitions occur are observed causing the appearance of new transmitting canals of the system [3, 4]. These phenomena essentially effect the functioning of nanodevices (quantum cascade lasers and detectors), the main operating elements of which are the multilayer RTS [5, 6, 7].
Studying the hightemperature superconductivity, mezophysical phenomena, lowdimensional nanosystems one should solve the problems where the perturbation or variational methods cannot be used because the multiphonon or multiphoton processes of quasiparticles scattering play an essential or even the main role. Therefore, one should propose the new mathematical approaches or use the methods of quantum field theory in order to overcome the known problems of partial summing of the infinite ranges of Feynman diagrams. For example, within the new diagrammatic Monte Carlo method [8, 9, 10], the important problems of hightemperature superconductivity [11] have been solved, and the excited states of structure and structureless Fröhlich polaron [1, 2] have been studied exactly and consistently. Recently in [12, 13, 14, 15], a new powerful approach for the investigation of different quasiparticles interacting with phonons in homogeneous and inhomogeneous systems has been developed. It is based on the nonperturbative method of momentum average approximation. Using it, in the paper [15], all types of disorder for various types of electronphonon interaction were studied in detail. Here, it was shown that the obtained results well correlate with that obtained within the diagrammatic Monte Carlo method. Moreover, in [16], the modified method of FeynmanPines diagram technique has been used for the development of a physically correct theory of renormalized spectrum of the ground and first excited state of Fröhlich polaron in the regime of weak coupling at K taking into account the multiphonon processes.
A complicated mathematical approach of quantum field theory does not always give an opportunity to study the spectra of quasiparticles renormalized due to the interaction with phonons in the framework of the general realistic models without the use of uncontrolled approximations. For several systems, this problem is studied using some additional mathematical conditions, which have a proper physical interpretation simplifying the starting model after which the problem is solved exactly.
The above mentioned situation is well known in the theory [17, 18] of quasiparticles with narrow energy bands (or localized ones) interacting with polarization phonons, where the renormalized spectrum of the system is obtained using an additional condition for the operator of a complete number of quasiparticles, which is equal to the square of this operator. Physically, this condition is explained the one at which the quasiparticle either exists in a certain state or not, without considering the interaction with phonons. In this simplified model, the unitary transformation with further analytical calculation of Fourier image of quasiparticles Green’s function allowed us to obtain the exact energy spectrum [17] of all bound states of the system. It was shown that the renormalized spectrum, besides the ground level shifted into lowfrequency range, contains a set of equidistant levels (the distance is of one phonon energy order) both in low and highfrequency range independently of temperature.
In this paper, we obtain a renormalized spectrum of localized quasiparticles interacting with polarization phonons using the general model (without the above mentioned additional condition) for systems with weak coupling at a finite temperature. This problem is solved within the modified method of FeynmanPines diagram technique. It is shown that compared to the simplified model, the general model provides a richer energy spectrum containing new bound states with complicated behaviour depending both on the temperature and coupling constant.
2 Hamiltonian of the system. Theory of renormalized energy spectrum in two models
We consider the localized dispersionless quasiparticles (excitons, impurities and so on) interacting with dispersionless polarization phonons described by Fröhlich Hamiltonian
(1) 
where and are the energies of quasiparticles and phonons, respectively. In the range of their typical magnitudes for the bulk crystals and nanosystems ( meV, meV), these values can be arbitrary. The analytical form of the binding function is not essential because the energy of quasiparticlephonons interaction, as would be seen further, is consistently characterized by a coupling constant , independent of , which can be also arbitrary in natural range since the problem becomes zerodimensional. The quasiparticle operators of the second quantization () and () satisfy the Bose commutative relationships.
We study the problem of a renormalized spectrum of the system of quasiparticles interacting with phonons at arbitrary temperature () using the Hamiltonian (1) within two models.
a) The model of the system where the condition
(2) 
is fulfilled [17]. It means that the eigenvalue of these operators can be either 0 or 1 and is assumed in [17] to be the condition of existence (1) or absence (0) of ‘‘pure’’ quasiparticle state (without interaction with phonons).
b) The general model of the system where the number of quasiparticle states is not confined by any conditions.
It is well known, [17, 18, 19], that the renormalized energy spectrum of the system is obtained from the Fourier image of the quasiparticle Green’s function , in general case, through the Dyson equation
(3) 
related with the mass operator (MO) , which is calculated according to the rules of FeynmanPines diagram technique [17, 18] when the concentration of quasiparticles is small.
In the model (a) the Hamiltonian (1) is diagonalized exactly, using the known, [17], unitary transformation, and the poles of function are obtained, in its turn, defining the exact renormalized energy spectrum of the system
(4) 
Formula (4) proves that the spectrum of the system is stationary (without a decay), equidistant and independent of temperature. It contains a renormalized by interaction ground state with the energy shifted into the longwave region with respect to and bound highenergy () and lowenergy () states of the system.
The exact unitary transformation, that makes the Hamiltonian (1) diagonal, cannot be performed for the model (b), where the condition (2) is not fulfilled. Thus, one should use the FeynmanPines diagram technique [17, 18] in order to calculate . All energetic multipliers in MO are independent of quasimomentum because the energies (, ) are dispersionless, as far as they are carried out from all sums over . Consequently, in all MO terms, one can see the same value , essentially simplifying the diagram technique [18]. Within the convenient dimensionless variables and values
(5) 
the Dyson equation (3) is of the form
(6) 
Here, since the problem has become ‘‘zerodimensional’’, MO is defined by the infinite sum of ‘‘dumb’’ diagrams (without arrows at the dashed phonon lines and without numeric indices at the solid quasiparticles ones)
(7) 
with the known rules of their construction, from the diagram technique [18].
In order to write a consistent analytic expression with respect to MO (7), for each diagram of th order over the number of dashed lines, one should put in correspondence the sum of equal ‘‘dumb’’ diagrams with all possible directions of the arrows. Under the solid lines of these diagrams one should put the numbers, which are the sums of the numbers of dashed lines in the righthand side (with sign ‘‘’’) and in the lefthand side (with sign ‘‘’’), placed above the respective solid line. For example, the system of four diagrams with indices
(8) 
corresponds to the ‘‘dumb’’ diagram of the second order. The rules of conformity between diagrams and analytical expressions are simple:
(9) 
where is an average phonon occupation number.
Thus, the analytical expression for the arbitrary diagram with indices is written as a product of contributions of all its lines and tops. For example, the analytical expression
(10) 
corresponds to the index diagram of the third order. The analysis of the structure of the complete MO proves that it can be written in an analytical form
(11) 
with separated terms which describe the processes of quasiparticle scattering at phonons in the unmixed [] and all possible mixed (the terms in ) sequences. Herein, the term describes the interaction between quasiparticle and phonons in all unmixed processes, accompanied at first by the creation and then by the annihilation of phonons, while the term — vice versa. The sum of the rest of the terms in MO (11) describes the mixed processes of the phonon creation and annihilation in all possible sequences.
Therefore, MO , according to the FeynmanPines diagram technique, is an infinite sum of diagrams in all orders over the powers of with the arrows directed only to the right ( ). Therein, the diagrams with the crossing dashed lines give the same contribution as their equivalent diagrams without these crossing lines. Thus, has a rather simple diagram representation
(12) 
According to the rules of FeynmanPines diagram technique, it brings us to the exact representation of this MO in two equal but analytically different forms
(13) 
The same calculation of (with all lines ) yields two equal expressions
(14) 
We should note that the representation of in the form of a chain fraction converges to the exact value at all and faster than that in the form of the sum over . We should also note that as it is shown in [20] and proven by formulae (11)–(14) at K when MO has the exact representation in the form of a continuous chain fraction, the th and th links of which are related by the expression . It is interesting that the qualitatively similar continuous fractions appeared in the other nonperturbative theories for quasiparticles interacting with phonons, in particular, in the momentum average approximation for inhomogeneous systems, [15].
The terms of MO (11), which describe the mixed sequences of scattering processes
(15) 
have the following analytical form:
(16) 
(17) 
Here, the functions are consistently defined by the diagrams with differently directed phonon lines of the order 2 and 2+1, respectively. Thus, for example, the mixed diagrams of the second order (=1), define MO and the respective functions
(18) 
(19) 
Each MO of the third order [] contains 30 diagrams with three differently directed phonon lines. Thus, to avoid cumbersomeness, we present the final analytical expressions
(20) 
where
(21) 
The exact analytical expressions for the functions of the higher order are clearly determined by diagram technique, although the number of diagrams rapidly increases for the bigger order.
In general case, when there is no decay, the renormalized energy spectrum of the system of quasiparticles interacting with phonons is obtained from the solutions of dispersional equation
(22) 
In order to study the properties of such systems in the model (a) with the condition () and in general model (b), we are going to use and MO, respectively. Herein, for the model (a), we use the known [17] analytical expression for the Green’s function and Dyson equation in dimensionless variables and obtain the analytical expression for
(23) 
which is correct at arbitrary values of and .
In the general model (b) we use the MO
(24) 
where is the just defined MO which describes the unmixed sequences of the scattering processes which is correct for the arbitrary values , and as well as which describes the mixed sequences of the scattering processes of the second and third order. This is sufficient for the majority of bulk crystals and nanostructures where the magnitude of the electronphonon interaction energy is not bigger than the phonon energy and the temperature is in the range of the room one, so that .
Besides the renormalized energy spectrum of the system in both models, we are going to analyze the socalled phonon ‘‘coats’’ of quasiparticles, namely the average number of phonons () surrounding the quasiparticles in the respective states depending on the values and . It is known [21] that the average numbers of phonons () surrounding the quasiparticles in the states with the energies obtained from the dispersional equation (22) in general case are defined as
(25) 
As far as the spectrum of renormalized energies is exactly fixed by formula (2) in the model (a), is also calculated analytically exactly
(26) 
In the model (b), the complete MO contains the term , which in analytical form describes all unmixed scattering processes independently of the values and and of the rest of terms, which describe the mixed scattering processes, where besides the MOs defined in the second and third order, the higher orders demand the accounting of the bigger number of diagrams. Thus, in the model (b), we are going to analyze for the system with weak coupling ()
(27) 
where are the solutions of dispersional equation (22) with MO (24).
As far as both MOs and are right at arbitrary and , in order to compare with , we are going to study the properties of numbers, which can be analytically written as
(28) 
where are the solutions of the equation (22) with MO .
The developed theory gives the opportunity to calculate, reveal and analyze the common and different features of the renormalized spectra of the systems of quasiparticles interacting with polarization phonons in both models.
3 Analysis of the formation of the renormalized spectra of the system of localized quasiparticles interacting with polarization phonons
The temperature evolution and the reasons of differences between renormalized spectra of the system of localized quasiparticles interacting with polarization phonons in two models are advisable to be studied comparing the respective mass operators as functions of dimensionless energy varying in the range at different and .
The typical dependences of MO , model (a), and MO terms of unmixed processes, model (b), are shown in figure 2 as functions of . Both of them are defined by the exact analytical expressions which are correct at arbitrary and . Figure 2 proves that both functions are qualitatively similar and at K when , are even completely equal [17, 18, 20]. However, at K when , their behavior is different in actual regions of energy where the solutions of dispersion equations [] define the energy spectra. When , from (11), (15)–(17) it is clear that MO , thus , since the renormalized energy spectra in both models are the same (, ) and equidistant. They are formed by the interaction between quasiparticles and virtual polarization phonons in the processes of their gradual creation with further gradual annihilation.
From figure 2 it is clear that at the increasing temperature (), model (b), in the approximated MO where only unmixed sequences of scattering processes are taken into account, all modes of , which form the bound states of quasiparticles with one, two and more phonons with the energies (), shift into the lowenergy region while the mode which forms the ground renormalized state () and all states without one, two and more phonons () in the vicinity of the energies of these states — vice versa. Consequently, as it is clear from figure 2 (b) and table 1, the renormalized spectrum of the system becomes not equidistant if the temperature increases. In this approximation, in the model (b), the same states as in the model (a) are observed. However, the properties of temperature dependence of the spectra and, as it is revealed, the properties of average phonon numbers () in phonon ‘‘coats’’ of quasiparticles are different.
0  0.6  1.6  

0.2  0.537  1.522  
0.4  0.480  1.446 
The average number of phonons in phonon ‘‘coats’’ for different states of quasiparticles with the energies are presented in figure 2 as functions of the coupling constant at =0, 0.3. If =0, these numbers () are the same in both models and are obtained exactly analytically
(29) 
They have an interesting property: in each th state of the system, these numbers as functions of have one minimum at , where, figure 2 (c), their magnitudes (marked by stars) are equal to the magnitudes of the numbers of the neighbour state
(30) 
The average phonon numbers in each th state of quasiparticle asymptotically increase till one in the region . From figure 2 (c) it is clear that at the number of phonons in the ‘‘coat’’ decreases only for the renormalized ground state of quasiparticle when becomes smaller.
At nonzero temperatures (), besides the highfrequency states with the energies , one can observe the lowfrequency ones with the energies in both models. Now, the average phonon numbers () as functions of are essentially different in two models. These numbers were calculated using formulae (26)–(28), and the results are shown in figures 2 (a), (b), respectively. From figure 2 (a) it is clear that in the model (a) the numbers in quasiparticles phonon ‘‘coat’’ depend on in the similar way as it was for =0, but the positions of their minima are now fixed by the relationship
(31) 
and the magnitudes are fixed by the expression
(32) 
Thus, when the temperature increases, the magnitude also decreases. Herein, decreases as well, while increases. In all lowfrequency states at all , figure 2 (a), are nearly low maximal () but weakly shift to the direction of smaller with respect to their analogues at =0.
The average numbers of phonons in the ‘‘coats’’ of quasiparticles are presented in figure 2 (b) as functions of for several states of the system in the model (b). This figure proves that in the region the numbers oscillate in antiphase with the numbers . These oscillations are quasiperiodical and, according to the calculations, their period and amplitude decrease when increases. Comparing figure 2 (a) with figure 2 (b), one can see that in the approximation where in the complete MO only all unmixed processes [] are accounted at , the average numbers of phonons in quasiparticles ‘‘coats’’ [] in model (b) correlate well with their analogues [] in model (a).
Taking into account the analysis of the properties of the spectra and average numbers of phonons in the ‘‘coats’’ of localized quasiparticles interacting with polarization phonons we can conclude that the results of the exact model (a) according to their main features are the same as the results of model (b) in which all unmixed scattering processes are considered.
Now we are going to study the properties of the spectra and average phonon numbers in the states of the system of localized quasiparticles interacting with phonons in model (b), where in the complete MO , besides the unmixed processes described by MO , the mixed scattering processes of the second and third orders over the coupling constant are considered.
The dependences of MO at different and are presented in figure 3, which shows the formation and behaviour of the energy spectrum of the system in general model (b). Figures 3 (a)–(f) prove that besides the states revealed in the model (a) and in the model (b) without taking into account the mixed processes (the modified or even the disappeared ‘‘old’’ states), one can see completely ‘‘new’’ states, their energies being also obtained from the solution of dispersional equation (22). Of course, the separation of the states at ‘‘old’’ and at ‘‘new’’ bound states of the system is fully conditional, because all states equally belong to the system. However, such separation makes it possible to better reveal the reasons of a different behaviour of these states. In figure 3 one can identify the origin of all states of the system fixed by the solutions of equation (22).
The analysis of the terms and of the complete MO at shows, figure 3, that renormalized energy spectrum of the system, as a set of solutions of dispersional equation, is mainly formed by those of them that contain the poles in the respective region of energies . The analytical form of MO (11) proves that both its terms and are essential only in the vicinity of , while in highfrequency region, the prevailing contribution into the formation of the spectrum is performed by the terms and and in lowfrequency region — and , respectively. In the structures of MO and there prevail the terms proportional to (1+), describing the processes accompanied by creation of phonons, which are exactly the ones that form the highfrequency bound states of the system. In the structures of MO and there prevail the terms proportional to , describing the processes accompanied by annihilation of phonons, which are exactly the ones that form the lowfrequency bound states of the system.
Figure 3 also shows that in the regions of energies , where in the vicinity of the solutions of dispersional equation, the condition is fulfilled, the ‘‘old’’ states are formed and at the condition — the ‘‘new’’ states appear. From the physical considerations and according to the previous analysis one can conclude that the ‘‘old’’ states with renormalized energies are mainly formed by unmixed scattering processes and the ‘‘new’’ ones with renormalized energies , are formed by the mixed processes [figure 3 (f)]. When the solutions of dispersional equation exist and the condition = is fulfilled, there appear ‘‘new’’ degenerated states of the system with renormalized energies and with equal contributions of mixed and unmixed scattering processes.
Moreover, from figure 3 one can clearly see the properties of renormalized energies of quasiparticles interacting with polarizational phonons (in the range ) depending on the coupling constant () and temperatures being in the vicinity of room ones (). The energy of the ground state of the system is shifted into the lowfrequency region. Together with the energies () of ‘‘old’’ highfrequency bound states it forms a quasiequidistant spectrum with the difference between the energies being of one phonon order which weakly depends on the values and . Up to three ‘‘new’’ bound states can appear in the highfrequency region. One of them has the energy () and the other two with the energies and (; ). Depending on the relationships between the values and , all highfrequency states can exist, degenerate and disappear. Figure 3 proves that at the fixed , the existing highfrequency states vary in such a way that the differences between the energies of neighboring ‘‘new’’ and ‘‘old’’ states () or () decrease when the temperature () increases. At certain temperature, , the difference between the energies of onephonon states disappears since they degenerate into one state, which further disappears at a higher temperature. When temperature still increases, the pair of neighboring states with the energies and show a similar behaviour.
Comparing figure 3 (a) and 3 (b) one can see that the degeneration of the respective pairs of the energy levels with a further disappearance of the respective states is observed at a stronger interaction between quasiparticles and phonons () and at higher temperature (). This clear from physical considerations because the stronger is quasiparticlesphonons coupling, the harder it is to break it, thus, the temperature should increase.
Contrary to the highfrequency bound states, the lowfrequency ones with the energies , , , exist only at K. Their temperature dependence differs as well, figure 3. One can see that in the vicinity of the energy , only one ‘‘new’’ state with the energy is formed while the ‘‘old’’ one with the energy is absent because the contribution of unmixed scattering processes into MO prevails. In the vicinity , three bound states are observed: one ‘‘old’’ () and two ‘‘new’’ (, ), presented at the upper insert in figure 3. This figure and the tables prove that the lowfrequency spectrum of energies weakly changes at increasing temperature independently of .
The revealed differences in the behaviour of energy spectra of bound states of the system of quasiparticles interacting with phonons in two models are also seen in the dependences of average phonon numbers () in the phonon ‘‘coats’’ on and . Figure 4 shows that at the regime of weak coupling () at the fixed , the increasing temperature () strongly decreases the number only for the highfrequency state with the energy . This fact correlates with the obtained temperature dependences of neighbouring energy levels and , starting from their coexistence till degeneration and disappearance. The average number of phonons in the ground state weakly decreases at an increasing temperature while in all other states, the numbers almost do not depend on . Herein, in the vicinity of very small , they sharply increase when the interaction increases.
4 Main results and conclusions
Using the method of FeynmanPines diagram technique, we developed the theory of renormalized spectra of localized quasiparticles interacting with polarization phonons at finite temperatures in a wide range of energies containing the energies of the bound states of the system. The properties of renormalized spectrum of the system are analyzed and compared in two models: in the known model [17] in which the problem is solved exactly when the additional condition fulfills ( , where is the operator of quasiparticles number) and in the general model with the regime of a weak coupling between quasiparticles and phonons.
It is established that, contrary to the model with an additional condition, where there always exist bound stationary states of the system with equidistant energy spectrum independent of temperature, in the general model, the renormalized spectrum is found to be much richer and more complicated. This is caused by different formation of bound states in mixed and in unmixed sequences of the processes of quasiparticle scattering while interacting with phonons.
It is shown that in the general model, the unmixed processes of quasiparticle scattering, accompanied by the creation of phonons, form a group of bound states with quasiequidistant spectrum while the mixed processes form a group of states with nonequidistant spectrum in highfrequency region. The states located near the ground state are mainly formed by the mixed processes of quasiparticle scattering with annihilation of phonons causing a nonequidistant spectrum in the lowenergy region.
It is revealed that in the systems with weak coupling, if the temperature increases to the room one, the location of the energy levels weakly changes while in highfrequency region they gradually degenerate in pairs and then disappear.
Finally, we should note that the use of the computer method of construction and calculation of the higher order diagrams, which describe the mixed sequences of the scattering processes of quasiparticles interacting with phonons, would essentially broaden the range of energies containing the bound states of the system and outrun the frames of the weak coupling. Besides, the further development of FeynmanPines diagram technique would help to solve the wellknown urgent problems regarding the existence and properties of the excited states of electronphonon systems (in particular, polaron) at arbitrary temperatures.
References
 [1] Mishchenko A.S., Phys. Usp., 2005, 48, 887; \bibdoi10.1070/PU2005v048n09ABEH002632.

[2]
De Filippis G., Cataudella V., Mishchenko A.S., Nagaosa N., Phys. Rev. B, 2012, 85, 094302;
\bibdoi10.1103/PhysRevB.85.094302.  [3] Tkach M.V., Seti Ju.O., Voitsekhivska O.M., Condens. Matter Phys., 2012, 15, 33703; \bibdoi10.5488/CMP.15.33703.
 [4] Tkach M.V., Seti Ju.O., Voitsekhivska O.M., Acta Phys. Pol. A, 2013, 124, 94; \bibdoi10.12693/APhysPolA.124.94.
 [5] Lei W., Jagadish Ch., J. Appl. Phys., 2008, 104, 091101; \bibdoi10.1063/1.3002408.
 [6] Giorgetta F.R., Baumann E., Graf M., Yang Q., Manz C., Kohler K., Beere H.E., Ritchie D.A., Linfield E., Davies A.G., Fedoryshyn Y., Jackel H., Fischer M., Faist J., Hofstetter D., IEEE J. Quantum Electron., 2009, 45, 1039; \bibdoi10.1109/JQE.2009.2017929.
 [7] Katz S., Vizbaras A., Meyer R., Amann M.Ch., J. Appl. Phys., 2011, 109, 081101; \bibdoi10.1063/1.3566072.
 [8] Prokof’ev N.V., Svistunov B.V., Tupitsyn I.S., J. Exp. Theor. Phys., 1998, 87, 310; \bibdoi10.1134/1.558661.
 [9] Prokof’ev N.V., Svistunov B.V., Phys. Rev. Lett., 1998, 81, 2514; \bibdoi10.1103/PhysRevLett.81.2514.

[10]
Mishchenko A.S., Prokof’ev N.V., Sakamoto A., Svistunov B.V., Phys. Rev. B, 2000, 62, 6317;
\bibdoi10.1103/PhysRevB.62.6317.  [11] Mishchenko A.S., Phys. Usp., 2009, 52, 1193; \bibdoi10.3367/UFNe.0179.200912b.1259.
 [12] Berciu M., Phys. Rev. Lett., 2006, 97, 036402; \bibdoi10.1103/PhysRevLett.97.036402.
 [13] Berciu M., Fehske H., Phys. Rev. B, 2010, 82, 085116; \bibdoi10.1103/PhysRevB.82.085116.

[14]
Marchand D.J.J., De Filippis G., Cataudella V., Berciu M., Nagaosa N., Prokof’ev N.V., Mishchenko A.S.,
Stamp P.C.E., Phys. Rev. Lett., 2010, 105, 266605; \bibdoi10.1103/PhysRevLett.105.266605.  [15] Ebrahimnejad H., Berciu M., Phys. Rev. B, 2012, 85, 165117; \bibdoi10.1103/PhysRevB.85.165117.

[16]
Tkach M.V., Seti Ju.O., Voitsekhivska O.M., Pytiuk O.Yu., Condens. Matter Phys., 2015, 18, 33707;
\bibdoi10.5488/CMP.18.33707.  [17] Davydov A.S., Theory of Solids, Nauka, Moscow, 1976 (in Russian).
 [18] Tkach M.V., Quasiparticles in Nanoheterosystems. Quantum Dots and Wires, Chernivtsi University Press, Chernivtsi, 2003 (in Ukrainian).
 [19] Abrikosov A.A., Gorkov L.P., Dzyaloshinski I.E., Methods of Quantum Field Theory in Statistical Physics, Dover, New York, 2012.
 [20] Tkach N.V., Theor. Math. Phys., 1984, 61, 1220; \bibdoi10.1007/BF01035007.
 [21] Levinson Y.B., Rashba E.I., Sov. Phys. Usp., 1974, 16, 892–912; \bibdoi10.1070/PU1974v016n06ABEH004097.
Властивостi i температурна еволюцiя спектру системи локалiзованих квазiчастинок взаємодiючих з поляризацiйними фононами у двох моделях
М.В. Ткач, Ю.О. Сетi, О.М. Войцехiвська, О.Ю. Питюк
\addressЧернiвецький нацiональний унiверситет iм. Ю. Федьковича,
вул. Коцюбинського, 2, 58012 Чернiвцi, Україна