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## Brazilian Journal of Physics

*Print version* ISSN 0103-9733

### Braz. J. Phys. vol. 28 n. 3 São Paulo Sept. 1998

#### http://dx.doi.org/10.1590/S0103-97331998000300009

**Eigenmode frequencies calculations in the charge-density-wave states of 2H-TaSe_{2}**

*.*

A. Ribeiro Filho, E. M. do Nascimento and

D. S. de Vasconcelos

*Instituto de Física, Universidade Federal da Bahia*

*Campus de Ondina, 40.210-340, Salvador, Ba, Brazil*

**Received 8 June, 1998. Revised version received on 17 August, 1998 **

We have performed some calculations involving two eigenmode frequencies of

2H-TaSeWe have obtained a good comparison with some well established Raman scattering data for the commensurate and incommensurate charge-density-wave phases in this compound. We outline an approximated method to compute the determinantal equation._{2}.

Subject Classification: 64.70. Rh; 77.80.Bh; S1.63

#### I Introduction

Many experimental and theoretical works with charge-density-waves *(CDW*) phase transitions in layered dichalcogenide transition metals, like *2H-TaSe2*, have emphasized the importance of the phenomenological McMillan-Landau theory [1] -[8], which was successful in introducing the notion of discommensuration defect or soliton-like behaviour of the incommensurate *CDW* near the incommensurate-commensurate "lock-in" phase transition, despite the existence of alternative theoretical models[9]. The compound *2H-TaSe _{2}* has a layered structure; in each layer a hexagonal sheet of Ta ions is sandwiched between two hexagonal sheets of

*Se*[10] ions. Moncton et al[11] , from the initial neutron diffraction study found, as the temperature is lowered, an initial onset phase transition to an incommensurate

*CDW*phase at 122

^{o}

*K*followed by another phase transition to a commensurate

*CDW*phase at 90

^{o}

*K*.

The order parameter fluctuation modes for the charge-density-waves in incommensurate systems have been studied by various authors and, in the case of *2H-TaSe _{2}*, there has been a great deal of work due to the complexity of its phase transition picture. The understanding of the incommensurate superlattice of this substance, has been improved following the experimental work performed by Steinitz and Genossar[12] who inferred that in the range between 122

^{o}

*K*and 90

^{o}

*K*, this superlattice presents two different phases. The first one with hexagonal symmetry exhibits at 112

^{o}

*K*a first-order phase transition to an orthorhombic stripe phase, which subsequently 'locks-in' at 90

^{o}

*K*. Chen at al[13] have stressed that 'on cooling', X-ray diffraction studies show that the

*CDW*, although incommensurable, remains hexagonal and it is generally believed that a honeycomb array of narrow discommensurations [5] can also describe the incommensurate phase. Despite this possibility those authors have admitted that the hexagonal symmetry in the incommensurate superlattice of this compound is retained on a larger scale. Other writers [9], have introduced an alternative model, where they have proposed three types

*(I, II, III*) of orthorhombic stripe incommensurate

*CDW*phases, as well three types

*(I,II,III)*of double honeycomb domain structure for the high-temperature incommensurate superlattice of a single layer having the

*2H-TaSe*structure. Although we do not study this model here, we emphasize that these three distinct types of incommensurate phases correspond to three types

_{2}*(I, II, III*) of commensurate phases of a single layer of this compound. There is experimental evidence that both the type-

*I*and type-

*II*commensurate phases occur in this substance [11], [15]. From this approach only the type-

*I*can be obtained from McMillan's phenomenological model. Those authors [14] have also showed how the layers could be stacked to give both hexagonal and orthorhombic structures.

In spite of these new theoretical approaches, our interests, in this work, have been in following McMillan's model, which is simpler and describes very well the distinct incommensurate and commensurate phases of this substance. In section *II* will perform calculations involving the commensurate *CDW* phase, maintaining the early notation [7], [8], outlining eigenmode frequencies calculations in the hexagonal commensurate *CDW* phase, comparing these results with those, of incommensurate* CDW* phase, obtained previously [7] and providing new analytical results, a little different from ones of McMillan [8] because he omitted the contribution of the term, in his free energy expression, that computes the amplitude fluctuation modes (or amplitudons). That writer only discussed phase fluctuation modes (or phasons). In section *III* we present some analytical calculations of the eigenmode frequencies (E_{2g}, A_{1g}) for the range of temperature decreasing from 122^{o}*K*, performing a limited numerical illustration and using a set of phenomenological parameters, in order to fit the two dominating modes, mentioned above, reported by Steigmeier et al [16], in his Raman scattering studies. They observed two dominating modes at 49cm^{-1} (E_{2g}) and 82cm^{-1} (A_{1g}), at 6^{o}*K*, which were also confirmed by Sugai et al [17].

#### II Theory

Let us consider the hexagonal commensurate phase of* 2H-TaSe _{2}*, which is characterized by the space group

*D*. The McMillan-Landau free energy density[8] presents, in this case, a cubic ''lock-in'' energy term. This term is associated with the strong contribution to the lattice potential energy from the electrons due to the Peierls energy gap in band structure[18].

_{6h}-6/mmmNow following the standard procedure we expand the order parameter as [7].

(*j* = 1,2,3), where in the presence of excitations

(*j* = 1,2,3) and the _{j} are the static charge-density-wave vectors. With f_{1} = f_{2} = f_{3} = f_{0} and knowing that in this case q_{j} = k_{j}, being k_{j} the shortest reciprocal lattice vectors in the hexagonal symmetry, we write the new McMillan-Landau free energy for the hexagonal commensurate phase as

where we see the contribution of the cubic 'lock-in' energy term, which is present in the mentioned phase. In order to maintain a comparison between the notation used by Holy et al [18] and McMillan [8] papers with our expression above, we note the following correspondence with their parameters and variables: a_{o} º A; b_{1} º 2B = 2B_{l}exp[i3(_{j}-)·]; (3c_{o}+2d_{o}) º D; b_{o} º -E = Re[exp(i3q_{o})], and f_{j} º f_{l}^{j} = f_{l}^{j}. The minimization of the static free energy with respect to f_{o} gives

with Q_{1} = |_{i}| and k_{1} = |_{i}| .

Now we compute the phonon frequencies and we use the expansion (2), such that this procedure corresponds to the addition of small phase and amplitude distortions to static distortion. Using Eq. (4) we expand (3) in powers of f_{jq} from (2) and keeping only second order terms, and following McMillan's procedure we compute the eigenmodes, writing in terms of the coupled modes and find

where

In order to avoid some difficulties in solving the complete 6 x 6 characteristic determinantal equation to compute the fluctuation eigenmodes, we have only considered the particular situation where is parallel to _{1}. Such situation results from the contribution of the cross q-linear term given by Eq. (9) above, which does not occur in the hexagonal incommensurate case [7]. Performing some algebraic manipulations, we are able to rewrite the original matrix as the product of two other matrices with dimensions 4 x 4 and 2 x 2 respectively. The advantage of this calculation is that the 2 x 2 determinantal equation gives directly expressions for the E_{2g} and E_{1u} eigenmode frequencies; and the 4 x 4 matrix provides the eigenmodes E_{2g}, A_{1g}, E_{1u}, B_{1u}, avoiding the degeneracy problem of the doublet amplitudons or phasons respectively. With this procedure, we find the following results,

where we have defined

Equation (12) gives the frequencies of the modes with symmetry E_{2g} at q = 0, and we also see that the quadratic contribution in e_{o} results from the cross q-linear term. As we have written before[7] the expressions (10) and (11) represents , being w the mode frequency and M^{*} = 206au. E_{2g} and E_{1u} are the symmetry characters of the irreducible representations of the group D_{6h}-6/mmm.

Our 4 x 4 determinantal equation can be written as

where we have defined: a =3(b_{o}-^{1}/_{2}b_{1})f_{o}+3c_{o}f_{o}^{2}+e_{o}Q_{1}^{2}q^{2}; a^{¢} = 3(b_{o}+3b_{1})f_{o}+e_{o}Q_{1}^{2}q^{2}; b =3(b_{o}-b_{1})f_{o}+3c_{o}f_{o}^{2}+(e_{o}+3f_{o})Q_{1}^{2}q^{2}; b^{¢} = 3(b_{o}+3b_{1})f_{o}+(e_{o}+3f_{o})Q_{1}^{2}q^{2}; c = -3b_{o}f_{o}+(3c_{o}+2d_{o})f_{o}^{2}; c^{¢} = 3b_{o}f_{o}; d = -e_{o}(k_{1}-Q_{1})Q_{1}^{2}q.

In these calculations we see from V^{+}, V^{-} and V^{±} expressions that a, b, c, are directly connected with amplitudons; a^{¢}, b^{¢}, c^{¢}, with phasons, and d with the cross term.

In reality the exact solution of the determinantal equation (14) is not straightforward and we have used an approximated method in order to calculate the last four non-degenerate fluctuation eigenmodes. We can outline this procedure rewriting that equation as

being l_{i} the eigenvalues and A, B and C are expressed in terms of a, a^{¢}, b, b^{¢},...,d, as we will discuss in the appendix. We will derive the following expression for the four eigenvalues,

where j = 1,2,3,4 and l_{5} = l_{1}, l_{6} = l_{2} and l_{7} = l_{3}. Despite this expression is not evaluated here, meanwhile it indicates how the analytical expression can be obtained for the eigenvalues with symmetries A_{1g}, E_{2g}, B_{1u}, E_{1u}, respectively, to order q^{2}. We do not consider the case of perpendicular to _{1}, because this has more severe algebraic difficulties, and we cannot obtain similar simplification. If we consider the particular case of q = 0 the determinantal equation (14) can be solved to obtain the following expression: A_{1g}:-3(b_{o}+b_{1})f_{o}+(15c_{o}+8d_{o})f_{o}^{2}; E_{2g}:3(b_{o}-b_{1})f_{o}-(3c_{o}+4d_{o})f_{o}^{2}; B_{1u}:9(b_{o}+b_{1})f_{o}; E_{1u}:9b_{1}f_{o}. These last expressions are similar in outline but differ in detail from those reported by Holy at al [18]. We must stress that it is not possible to make a complete comparison because those authors used a different free energy for their commensurate phase calculations in *2H-TaSe _{2}*.

#### III Numerical Results

In this section we present the results of a numerical illustration of eigenmode frequencies (E_{2g}, A_{1g}) of *2H-TaSe _{2}*. We have used the normalized coordinates and defined previously [7], and we have assumed the phenomenological parameters b

_{o}= , b

_{1}= 1.2, c

_{o}= , d

_{o}= -3.9 and f

_{o}= 0. We have used a quadratic expression, a

_{o}= a

^{¢}(T

^{2}-T

_{o}

^{2}), as the definition of Landau parameter a

_{o}in terms of temperature, with a

^{¢}= 2.35 x 10

^{-4}. If the standard Landau expression, a

_{o}= a

^{¢}(T-T

_{o}), is used at low temperatures regime, we find that the order parameter and mode frequencies have a linear component in their dependence temperature as T® 0, in violation of the third law of Thermodynamics [7]. Our quadratic expression has the usual linear form for T close to T

_{o}but it also produces the thermodynamically correct behaviour as T® 0. For the case of the hexagonal commensurate phase, there is a visible variation of the frequencies of these optical phonons with temperature but it is not strongly.

We must emphasize that our calculations are in fact an approximation to the exact ones, because the analytical calculations involving the normal mode frequencies in this commensurate phase are not straightforward, due to the cross q-linear term V^{±}. We have also performed numerical computations in the region of the incommensurate-commensurate ''lock-in '' phase transition, obtaining the order parameter's behavior as the temperature changes over the complete range between 122^{o}*K* and 0^{o}*K*. We consider the experimental 'on cooling ' situation, where the orthorhombic stripe incommensurate phase for this compound does not occur, that is, in the range of temperature between 122^{o}*K* and 90^{o}*K*, the unique phase is the hexagonal incommensurate phase.

Let as consider the equations of minimization of the static free energy for the incommensurate case [7] with respect to f_{o},

and the similar for the commensurate case (4) that give the analytical expressions for the order parameter for the hexagonal incommensurate (f_{inc}) and commensurate (f_{c}) phases respectively. Then, using the new definition of the Landau parameter a_{o}, we rewrite V(f_{o}) for the case of both phases as,

and

where e^{¢} represents 4e_{o}[Q_{1}^{2}(k_{1}-Q_{1})^{2}].

The numerical problem is to find a set of phenomenological parameters that produce the incommensurate-commensurate "lock-in'' transition temperature at 90^{o}*K* , that is, the point where V_{inc}^{o} = V_{c}^{o}. To illustrate this procedure, we have used the same values of b_{o}, b_{1}, c_{o} and d_{o} introduced by Ribeiro Filho[7] and take e^{¢} = 0.779. The next step is to solve numerically the equation V = V_{c}^{o}(T)-V_{inc}^{o}(T) = 0, T being the "lock-in'' temperature. These calculations can be performed when we substitute Eqs. (17) and (4) in V_{inc}^{o} and V_{c}^{o}, respectively. The expression for V is an equation V(a^{¢}) = 0 that gives the values of a^{¢} for a particular set of phenomenological parameters. If we use the parameter mentioned above we obtain a^{¢} = 2.35 x 10^{-4}. Figs. (1) and (2) show the free energies V^{o} relative to the incommensurate and commensurate phases and the order parameter (f_{o}) versus temperature for *2H-TaSe _{2}*. Further numerical computations have been made in order to fit the theoretical results for eigenmode frequencies to light scattering data. We have concentrated on the experimental results of Raman scattering reported by Steigmeier et al [16], that are an important contribution to the understanding of the commensurate charge-density-wave phase of 2H-TaSe

_{2}. They observed two dominating modes at 49cm

^{-1}(E

_{2g}) and 82cm

^{-1}(A

_{1g}), at 6

^{o}

*K*, which were confirmed by Sugai et al [17]. We have performed a limited numerical calculation of these two eigenmode frequencies (E

_{2g}, A

_{1g}), normalizing the Steigmeier et al results to T = 0

^{o}

*K*. We retain the same values for parameters b

_{o}, b

_{1}, c

_{o}, d

_{o}and calculate a

^{¢}and e

^{¢}algebraically, with a

_{o}defined before. Then, after some straightforward manipulations with the order parameter and frequency expression of A

_{1g}and E

_{2g}, we write for the range of temperature between 0

^{o}

*K*and 90

^{o}

*K*,

Figure 1. Free energies, relative to the incommensurate (-- ·) and commensurate (-) phase for a single layer of the

2H-TaSeas a function of temperature with all parameters given in the text._{2}

Figure 2. Order parameter (f_{0}) versus temperature for *2H-TaSe _{2}*, with all parameters given in the text.

where ; and

where w_{E}^{¢} =3(b_{o}-b_{1}) and w_{E}" = -(3c_{o}+4d_{o}); with w_{A1g}(0) and w_{E2g}(0) being the experimental values of Steigmeier et al, and f_{c}(T) has been obtained from the minimization of the static commensurate free energy.

In order to get an approximate picture of these modes for the incommensurate phase [7], we have written for the range between 90^{o}*K* < *T* < 122^{o}*K*, the eigenmode frequencies as

and

Equations (20-23) are plotted in Fig. (3) and give a reasonable picture of the Steigmeier et al experimental work (1976).

Figure 3. Frequencies of the

CDWmodels of 2H-Ta Se_{2}versus temperature. Fitting from Steigmeier et all for A_{1g}(-) and E_{2g}(-- ·) modes, with all parameters given in the text.

#### IV Conclusions

In this work we have reported calculations of eigenmode frequencies for an assumed hexagonal commensurate charge-density-wave phase of *2H-TaSe _{2}*, despite the controversy whether such phase is orthorhombic [6] rather than hexagonal [11]. Fung et al (1981) found that the commensurate phase is not hexagonal but rather a network of orthorhombic domains and that the hexagonal symmetry observed in scattering experiments was due to domain averaging. Another interesting contribution to the orthorhombic-hexagonal controversy has been given by Walker and Jacobs[14] that introduced an alternative free energy functional for the CDW states in

*2H-TaSe*. Those writers have classified three distinct (I, II, III) commensurate

_{2}*CDW*states with hexagonal (type-I layers) and orthorhombic (type-II, III layers) symmetries. In fact the experimental study of the incommensurate and commensurate superlattices of this compound has been intense during recent years, and there is the possibility that new symmetry's interpretations can be improved in the next future.

We have also performed some numerical computations in order to give an approximated picture of some experimental results for this compound. The analytical results for commensurate *CDW* phase can be correlated with those ones of the incommensurate phase[7]. We have assumed 'on-cooling' experimental situation where only the hexagonal incommensurate phase is present in the range of temperature between 122^{o}*K* and 90^{o}*K*. In the case of the commensurate superlattice we have neglected any orthorhombic symmetry, retaining the original picture of the hexagonal symmetry existing throughout the commensurate phase. In spite of the limitations of this numerical illustration, it shows the advantage of the McMillan-Landau theory in providing a unified description of the charge-density-wave phases of this compound. We have written some normalized expressions for eigenmode frequencies in order to fit the Raman scattering (E_{2g}, A_{1g}) data obtained by Steigmeier et al[16]. It is important to stress that these two previously identified hexagonal E_{2g} modes can be then be thought of as superpositions of A_{g} and B_{lg} orthorhombic modes, while the two previously identified A_{lg} modes become A_{g} orthorhombic modes[19]. These correlations between the two symmetry possibilities are very interesting because they create a link between the experimental results of those authors that found hexagonal or orthorhombic symmetries. Finally, we must emphasize that we have obtained, from Fig. 3, a reasonable fitting from the Raman scattering data obtained by Steigmeier et al.

**Acknowledgment**

One of us (A. R. F.) would like to thank the support of "Conselho Nacional de Desenvolvimento Cientifí co e Tecnológico "(CNPq) and the Brazilian agency CAPES through the "CDI-Programa Suplementar de Apoio à Qualificação Docente''.

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#### V Appendix

In this section we discuss the calculation of eigenmodes from the determinantal equation (14) using an approximated method outlined below. We rewrite it as

with a, a^{¢}, b, b^{¢}, c, c^{¢}, d, as defined before. After performing straightforward algebraic manipulations, we write Eq. (24) as

where

and

where we have neglected the quartic d-contribution. In order to get approximate solution of (25), we consider first the case when d vanishes in (24). So, we have two uncoupled 2x2 determinantal equations A = 0 and P = 0, which after diagonalization could be written as

In this case, using the same procedure outlined before and substituting a, a^{¢}, b, b^{¢}, c, c^{¢}, d, in (26) and (27) we find

If we compare (29 - 32) with the expressions of A_{1g}, E_{2g}, B_{1u} and E_{1u}, given in section II, we identify these modes as follows: l_{1}® A_{1g}; l_{2}® E_{2g}; l_{3}® B_{1u}; and l_{4} ® E_{1u}. When we consider d ¹ 0 in (25) we retain only terms to order q^{2}. After some algebraic manipulation we can rewrite (25) as

where

Equation (33) produces for instance the approximate value l_{1}^{¢} of the eigenmode l_{1}, where l_{1}^{¢} = l_{1}+e with e ~ O(q^{2}). In this case when we substitute l = l_{1}^{¢}, we get

and to lowest order in q^{2},

Following the same procedure, we can write a general expression for these eigenvalues:

with j = 1,2,3,4, and l_{5} = l_{1}, l_{6} = l_{2}, l_{7} = l_{3}. The values of l_{j} are given by equations (29-32).