PHYSICAL REVIEW B 79, 125101 共2009兲

Infrared spectra of the low-dimensional quantum magnet SrCu2(BO3)2:
Measurements and ab initio calculations
C. C. Homes,1,2,* S. V. Dordevic,1,3 A. Gozar,1 G. Blumberg,4,5 T. Rõõm,5 D. Hüvonen,5 U. Nagel,5 A. D. LaForge,6
D. N. Basov,6 and H. Kageyama7
1

Department of Condensed Matter Physics and Materials Science, Brookhaven National Laboratory, Upton, New York 11973, USA
2Laboratoire Photons et Matière, UPR-5 CNRS, ESPCI, 10 Rue Vauquelin, 75231 Paris Cedex 5, France
3Department of Physics, The University of Akron, Akron, Ohio 44325, USA
4
Department of Physics and Astronomy, Rutgers University, Piscataway, New Jersey 08854, USA
5National Institute of Chemical Physics and Biophysics, Akadeemia tee 23, 12618 Tallinn, Estonia
6
Department of Physics, University of California-San Diego, San Diego, La Jolla, California 92093, USA
7
Department of Chemistry, Graduate School of Science, Kyoto University, Kyoto 606-8502, Japan
共Received 16 June 2008; revised manuscript received 28 November 2008; published 4 March 2009兲
The reflectance of the insulating quasi-two-dimensional quantum magnet SrCu2共BO3兲2 has been examinedover a wide temperature and frequency range for light polarized parallel 共a axis兲 and perpendicular 共c axis兲 tothe copper- and boron-oxygen sheets. The spectra have been measured for temperatures below the structuralphase transition Ts = 395 K for both polarizations; above Ts a limited study of the in-plane properties wasundertaken in the far-infrared region only. Several new modes appear in the reflectance just below Ts along thea and c axes, while others are visible only for T Ⰶ Ts. Below Ts, the intensity of some of the new modes
displays little or no temperature dependence, while the intensity of some vibrations increases dramatically withdecreasing temperature. Ab initio calculations have been performed for the room-temperature phase using
density-functional theory, and the frequencies and atomic characters of the infrared-active phonons at the zone
center were obtained using the direct method. The agreement between the calculated and experimentallyobserved frequencies is quite good, and assignments of the modes are discussed. The vibrational features thatare observed only at low temperature appear to be magnetic in origin.
DOI: 10.1103/PhysRevB.79.125101

PACS number共s兲: 63.20.⫺e, 71.15.Mb, 72.15.Jf, 74.25.Gz

I. INTRODUCTION

The low-dimensional quantum magnet SrCu2共BO3兲2 hasreceived a considerable amount of attention recently for its
unusual magnetic properties.1–10 In this system the zeromagnetic-field spin gap of ⌬ = 3 meV separates the singlet
ground state from the excited triplet states. The crystal has atetragonal symmetry in which the copper, boron, and oxygen
atoms are organized in two-dimensional sheets. The S = 1 / 2
spins lie on the copper sites in the layers to form interacting
spin dimers that are orthogonally connected.11 This exotic
spin-exchange topology results in an almost perfect realization of the Shastry-Sutherland model.12 It has been suggested
that this material is close to a quantum critical point that
separates the gapped short-range dimer phase from a gaplesslong-range antiferromagnetically ordered Néel state.4–6
Some evidence has been found in the magnetic susceptibility
for a closing of the gap under hydrostatic pressure.3
The magnetic properties of this material have been investigated in detail using several different experimental techniques, including magnetic susceptibility,1–3 nuclear magnetic resonance,1,2 thermal conductivity,13 specific heat,14
and ultrasonic attenuation;15,16 all give results that are consistent with the thermal excitation of triplet states across thespin gap. Below about 20 K the population of excited magnetic states begins to diminish and well-defined direct transitions between the singlet ground state and the lowest excited triplet states are observed in electron-spin resonance17
and inelastic neutron scattering.18–20 There have also been anumber of optical studies. Raman scattering,21–24 infrared
1098-0121/2009/79共12兲/125101共12兲

transmission, and magnetoabsorption studies25,26 have all
been able to observe several excitations across the spin gap;
magneto-optical studies have revealed a significant field dependence for the transitions across the spin gap.23,26 Thesestudies all draw attention to the coupling between the spins
and the lattice, and in particular the ability of optical methods to probe this behavior; however, a detailed infrared studyof this material has not yet been performed. Strong spinphonon interactions are expected to manifest themselves as
either anomalous frequency shifts with the onset of magnetic
order or the appearance of Fano-type asymmetric line
shapes.27–35
In this work we have measured the reflectance of
SrCu2共BO3兲2 for different polarizations over a wide temperature and frequency range below the structural phase transition Ts = 395 K 共Ref. 36兲; above Ts only the in-plane properties were examined. The measurements have been
performed on the crystals from the same batch as those usedin recent Raman scattering23 and infrared25,26 experiments,
allowing for direct comparison of results. The infrared spectra reveal an insulating character along both crystallographic
directions, allowing a large number of phonon modes to be
identified in both the ab-plane and c-axis spectra. The evolution of the vibrational spectra in this material is rather unusual; some new modes develop just below Ts, while others
are visible only below ⬃250 K, and one peculiar mode at
443 cm−1 共55 meV兲 appears only below ⬃20 K. In addition, some vibrational modes increase in intensity with decreasing temperature, contrary to the expectation that the oscillator strength should remain constant.

125101-1©2009 The American Physical Society

PHYSICAL REVIEW B 79, 125101 共2009兲

HOMES et al.

(a)
Sr
Cu
B
O(1)
O(2)

(b)

FIG. 1. 共Color online兲 The unit cell of SrCu2共BO3兲2 in the 共a兲high-temperature I4 / mcm phase with coplanar copper and boron
sheets, and 共b兲 the low-temperature body-centered-tetragonal I4̄2m
setting with a = b = 8.982 Å and c = 6.643 Å, showing the bucklingof the copper- and boron-oxygen planes and loss of inversion symmetry 共detailed structural parameters for the low-temperature phase
may be found in Table II兲. The sheets describe the a-b planes, while
the orthogonal direction is the c axis. The Sr atoms 共yellow兲 lie
between the Cu 共blue兲 and B 共green兲 sheets; the four-fold coordinated Cu atoms form a distorted square with the O共1兲 atoms 共red兲,
while the three-fold coordinated B also lies on the corner of a distorted square formed by the Cu and O共2兲 atoms 共magenta兲.

to an I4̄2m space group 共D2d point group兲, in which the
sheets buckle and the structure loses its inversion
symmetry.11,36 The room-temperature structure is shown in
Fig. 1共b兲. This transition leads to an abrupt jump in the magnetic susceptibility at Ts 共Ref. 4兲; however, the structure continues to evolve well below Ts and the fractional coordinates
continue to show changes down to T ⱗ 200 K 共Ref. 36兲.
Large single crystals of SrCu2共BO3兲2 have been grown by
a traveling solvent floating zone method.37 The crystals examined consisted of one with a cleaved a-b face and anotherwhich was oriented, cut, and polished to reveal an a-c facewith an optically flat surface and a bright mirrorlike finish.
Typical sample dimensions are ⬃1 ⫻ 2 mm2, with somewhat
irregular perpendicular dimensions. The reflectance of thecrystals of SrCu2共BO3兲2 has been measured between 5 and295 K 共below Ts兲 at a near-normal angle of incidence from
⬃20 to 18 000 cm−1 using an in situ evaporation technique38
with typical resolutions of 1 or 2 cm−1. A more detailed
temperature dependence up to 400 K 共T ⬎ Ts兲 has been performed only in the far-infrared region for light polarized in
the planes. For the crystal with an a-b face, the light was notpolarized. In the case of the crystal with an a-c face, thereflectance has been measured using an s-polarized geometry
for light polarized along the a and c axes. The s-polarized
geometry has been employed because it has been demonstrated that it reduces the contamination from other crystallographic directions.39

III. RESULTS

To better understand the nature of the lattice vibrations inthis complex material, ab initio calculations have been performed using density-functional theory, and the frequencies
and atomic characters of the zone-center 共q = 0兲 modes in theroom-temperature structure have been determined using thedirect method. The relative intensities of the infrared-activemodes have also been calculated. The agreement between thepredicted and observed frequencies is quite good. The modes
that appear below Ts correspond to the predicted frequenciesof the weak symmetry-allowed infrared modes. While there
is no direct evidence for spin-phonon coupling in any of theinfrared modes, there is evidence for a redistribution of
charge within the unit cell at low temperature. In addition,
the unusual temperature dependence of the 443 cm−1 modesuggests that it is probably a combination of a strong infrared
mode and a magnetic excitation.

II. EXPERIMENT

SrCu2共BO3兲2 has a tetragonal symmetry in which layersof 共BO3兲3− groups and Cu2+ ions are separated by closedshell Sr2+ atoms. The a-b direction is along these planes 共inplane兲 and c-axis direction is perpendicular to them 共out ofplane兲. At high temperature, this compound is in the I4 / mcm
space group 共D4h point group兲 in which the copper and boron
sheets are planar. The high-temperature phase is shown in
Fig. 1共a兲, projected along the planes. Below Ts = 395 K thesystem undergoes a displacive second-order phase transition

The reflectance of SrCu2共BO3兲2 below 2000 cm−1 at 5
and 295 K for light polarized along the a and c axes is shownin Figs. 2共a兲 and 2共b兲, respectively. Due to the insulating
character of this compound, the reflectance is dominated by
the infrared-active vibrations, many of which sharpen considerably with decreasing temperature. In addition, some
new features become visible in both polarizations only at low
temperature.
The real and imaginary parts of the dielectric function
have been calculated from a Kramers-Kronig analysis of thereflectance,40 for which extrapolations are supplied for ␻→ 0 , ⬁. At low frequency, the reflectance is assumed to continue smoothly to R ⬇ 0.2; at high frequency, the reflectanceis truncated at a cut-off frequency and above this point a
free-electron approximation has been assumed 共R ⬀ ␻−4兲. The
Kramers-Kronig analysis yields accurate information in the
low-frequency region; however, the nature of the line shapes
共profile and amplitude兲 observed in the imaginary part of thedielectric function above several hundred cm−1 are very sensitive to the choice of cut-off frequency and the nature of thehigh-frequency extrapolation. It seems likely that the frequency interval available in this experiment is insufficiently
large for the Kramers-Kronig relation to yield accurate results over the entire region. For this reason, in order to quantitatively analyze the temperature dependence of phononmodes, we have chosen to fit the reflectance spectra to amodel for the complex dielectric function 共˜⑀ = ⑀1 + i⑀2兲 consisting of Lorentz oscillators,

125101-2

PHYSICAL REVIEW B 79, 125101 共2009兲

INFRARED SPECTRA OF THE LOW-DIMENSIONAL…

FIG. 2. 共Color online兲 The
temperature dependence of the reflectance of SrCu2共BO3兲2 versus
the log of the frequency for 共a兲light polarized in the a-b planes
and 共b兲 light polarized along the caxis in the region of the infraredactive vibrations.

˜⑀共␻兲 = ⑀⬁ + 兺
j

␻2p,j
,
2
␻ j − ␻2 − i␥ j␻

共1兲

where ␻ j, ␥ j, and ␻ p,j are the frequency, width, and effective
plasma frequency of the jth vibration; ⑀⬁ is the highfrequency contribution to the dielectric function. The complex dielectric function is related to the complex refractive
index ñ = n + ik,
n=
and
k=

冋冑

册

共2兲

冋

册

共3兲

1/2
1
共 ⑀21 + ⑀22 + ⑀1兲
2

1/2
1
共冑⑀21 + ⑀22 − ⑀1兲,2from which the reflectance at a normal angle of incidence
can be calculated,R=

共n − 1兲2 + k2.
共n + 1兲2 + k2

共4兲

The insulating nature of the spectra precludes any freecarrier contribution. The model reproduces the data very
well, and the results of the fits to the reflectance at room
temperature and 5 K for light polarized in the a and c axes
are listed in Table I.
IV. DISCUSSION AND ANALYSIS
A. Vibrational features

The irreducible vibrational representations for both thehigh- and low-temperature phases of SrCu2共BO3兲2 have beenpreviously examined22,24 and will only be briefly discussed.
In the high-temperature I4 / mcm phase, the presence of inversion symmetry allows the vibrations to be divided intoeven 共g兲 and odd 共u兲 species, yielding the vibrational representation⌫HT = 5A1g + 6A2g + 5B1g + 5B2g + 6Eg + A1u+ 5A2u + 4B1u + B2u + 11Eu ,including A2u + Eu acoustic modes. All of the even modes are

Raman active. The odd A2u and Eu modes are infrared active
along the c axis and the planes, respectively. Below thestructural phase transition at 395 K in the I4̄2m phase, theinversion symmetry is lost and it is no longer possible tolabel a species as even or odd. The irreducible vibrational
representations at low temperature are⌫LT = 9A1 + 7A2 + 6B1 + 10B2 + 17E,
including B2 + E acoustic modes. Effectively all of the 47
optical modes are Raman active.24 The nine B2 and 16E
modes are infrared active with dipole moments along the caxis and the a-b planes, respectively.
It is clear from the irreducible vibrational representations
that many more infrared-active modes should be observed in
the a-b planes than along the c axis, and this is indeed what
we observe in Fig. 2. Along the c axis at room temperature,
we observe seven out of the nine possible B2 modes. At low
temperature these modes narrow considerably, and a sharp
new mode is observed at 150 cm−1 共Table I兲. Within the a-b
planes, the spectra are considerably more complicated. At
room temperature, we observe only 10 out of the 16 possible
E modes. At low temperature, in addition to the narrowing ofmost vibrational modes, new features are observed at 125,
223, 231, and 443 cm−1, yielding a total of 14 modes. The
detailed temperature dependence of the reflectance for lightpolarized along the a axis in the 120– 170 cm−1 region isshown in Fig. 3共a兲; the reflectance has been modeled using
the complex dielectric function in Eq. 共1兲, and the fitted
widths, frequencies, and effective plasma frequencies 共theoscillator strength is proportional to ␻2p,j兲 of the modes as afunction of temperature are shown in Fig. 4.
The behavior of the low-frequency vibrational modes may
be seen more clearly in the imaginary part of the dielectric
function 共related to the optical absorption兲 shown in Fig. 3共b兲that has been determined from a Kramers-Kronig analysis of
the reflectance. Above Ts only one broad mode at about
142 cm−1 is observed. Below Ts the 157 cm−1 mode is immediately visible; however, the modes at 125, 223, and231 cm−1 共shown in Figs. 2 and 3兲 only become visible below about 250 K 共well below Ts兲. The imaginary part of thedielectric function for the mode at 443 cm−1, shown in detail125101-3

PHYSICAL REVIEW B 79, 125101 共2009兲

HOMES et al.

TABLE I. The vibrational parameters for oscillator fits to the reflectance SrCu2共BO3兲2 for light polarized
in the a-b planes and along the c axis at 295 and 5 K, where ␻ j, ␥ j, and ␻ p,j are the frequency, width, andeffective plasma frequency of the jth vibration. The value for the high-frequency contribution to the dielectric
constant has been determined to be ⑀⬁,a = 3.4 for the a-b planes and ⑀⬁,c = 2.7 along the c axis. All units arein cm−1, except for the dimensionless oscillator strength S j = ␻2p,j / ␻2j ; a value of zero indicates S j ⬍ 0.01.
E储a
295 K

5K

␻j
1307
1226
934
719
693
659

␥j
16.4
4.4
4.4
3.4
5.8
6.3

␻ p,j
763
601
52
34
105
220

共S j兲
共0.34兲
共0.24兲
共0.01兲
共0.00兲
共0.02兲
共0.11兲

425
318

6.5
12.2

386
254

共0.82兲
共0.64兲

150
142

5.2
4.7

94
140

共0.39兲
共0.97兲

␻j
1308
1228
934
721
693
661
443
424
319
231
223
157
141
125

␥j
11.9
2.7
4.5
2.2
4.6
3.9
4.0
4.1
5.4
2.0
2.5
0.7
1.8
1.0

␻ p,j
751
610
62
47
116
231
35
394
257
29
23
76
150
49

共S j兲
共0.33兲
共0.25兲
共0.01兲
共0.00兲
共0.03兲
共0.12兲
共0.01兲
共0.86兲
共0.65兲
共0.02兲
共0.01兲
共0.23兲
共1.13兲
共0.15兲

203
29
30
350
40
331
49
126

共0.02兲
共0.00兲
共0.00兲
共0.26兲
共0.01兲
共2.46兲
共0.11兲
共1.58兲

E储c
295 K

5K

1349
956
694
682
449
211

11.1
5.2
5.7
2.4
5.7
10.1

139
19
30
360
30
318

共0.01兲
共0.00兲
共0.00兲
共0.27兲
共0.01兲
共2.27兲

97

4.8

121

共1.55兲

in Fig. 5, has a more unusual temperature dependence withan onset of absorption only below ⬃20 K, similar to anotherin-plane mode observed at 52 cm−1 in magnetoabsorption
experiments.25 In contrast, the modes above about 500 cm−1
in either polarization vary little with temperature 共Table I兲.
The behavior of the three modes in the 120– 170 cm−1
region may be considered as a template for other activatedmodes in this material, which along with the 443 cm−1 mode
will be examined in more detail below. As Figs. 3共b兲 and 4共a兲
indicate, above Ts only one vibrational mode at about
141 cm−1 may be identified; just below Ts a new mode splits
off of the main feature, narrowing rapidly and increasing infrequency with decreasing temperature until it may beclearly resolved at about 157 cm−1 for T Ⰶ Ts. The originalmode at 142 cm−1 narrows with decreasing temperature but
otherwise displays little temperature dependence. It is interesting to note that in Fig. 4共c兲 the 142 cm−1 mode undergoes
an abrupt decrease in oscillator strength below Ts. However,
below Ts the sum of the oscillator strengths of the 141 and

1347
955
696
683
448
211
150
100

7.7
4.3
2.2
1.9
3.1
4.2
2.7
0.5

157 cm−1 modes 共dotted line兲 is roughly equal to that of thesingle mode above Ts, indicating that there is a conservationof oscillator strength between these modes across the structural phase transition. This suggests that above Ts bothmodes are optically active; however, they are degenerate infrequency.
Below about 250 K a weak mode is visible in Fig. 3共a兲 at⬃121 cm−1, increasing to 125 cm−1 at low temperature. The
size and temperature dependences of the widths of the modes
between 120 and 170 cm−1 are all comparable, as shown in
Fig. 4共b兲, narrowing with decreasing temperature. However,unlike the two modes at slightly higher frequency which display effectively no temperature change in oscillator strength
below Ts, the strength of the 125 cm−1 mode increases
gradually below about 250 K, as shown in Fig. 4共c兲. A similar trend has been observed for the c-axis B2 mode at
150 cm−1. This behavior is unusual because while it is common for the frequency and width of a new mode that develops below a structural phase transition to change with de-125101-4

PHYSICAL REVIEW B 79, 125101 共2009兲

INFRARED SPECTRA OF THE LOW-DIMENSIONAL…

FIG. 3. 共Color online兲 The detailed temperature dependence of
共a兲 the reflectance of SrCu2共BO3兲2 above and below the structuralphase transition at Ts = 395 K for light polarized along the a axis in
the region of the three low-frequency E lattice vibrations and 共b兲 theimaginary part of the dielectric function. The asterisk in the upper
panel denotes the appearance of a shoulder in the reflectance at low
temperature. The experimental resolution is 2 cm−1, except below
100 K, where it is 1 cm−1. Note: the frequency intervals in theupper and lower panels are different.

creasing temperature, the oscillator strength is expected toremain constant. We remark here that the rather gradual nature of the phase transition may make it difficult to initiallyobserve weak new modes; however, while some changes
might be explained by the evolution of the structure, below⬃200 K no further changes are expected in this material as
it has essentially achieved its final geometry.36
The activation of some modes at low temperature is evenmore exaggerated in the case of the 443 cm−1 mode, which
is seen only as a weak antiresonance superimposed on amuch stronger feature in the in-plane reflectance in Fig. 2共a兲at 5 K. The temperature dependence of the imaginary part ofthe dielectric function for the 443 cm−1 mode is shown below 50 K in Fig. 5共a兲. The intensity of this mode has been
estimated from the area under the curve 共spectral weight兲
assuming a linear background; the relative intensity is shownin Fig. 5共b兲. This feature may only be identified below 20 K,
which happens to coincide to the temperature at which magnetic transitions from the singlet to triplet states are first observed.
The behavior of these modes, and the development of the443 cm−1 mode below ⬃20 K, indicates that in order toassign these features we must first understand the characterof the vibrations. To obtain this information, we have undertaken a first-principles calculation of the lattice dynamics of

FIG. 4. 共Color online兲 The temperature dependence of the fitted
vibrational parameters of SrCu2共BO3兲2 for light polarized along thea axis for the 共a兲 fundamental frequencies ␻ j, 共b兲 widths ␥ j, and 共c兲
effective plasma frequencies ␻ p,j for the in-plane modes in the120– 170 cm−1 region. The solid circles track the mode visible in
the high-temperature phase designated as the 141 cm−1, while theopen squares and circles represent vibrational modes at 125 and157 cm−1, respectively, that are observed below Ts 共dashed line兲.
The dotted line represents the sum of the oscillator strengths obtained through addition in quadrature of the effective plasma frequencies for the two modes at 141 and 157 cm−1. The errors associated with the fitted results are comparable to the size of thesymbols.

the low-temperature phase, which we describe in Sec. IV B.
B. Calculation of phonon modes

The phonon frequencies were determined from first principles using the direct method,41 in which the dynamical matrix is derived from the Hellmann-Feynman force constantsarising when a single atom is displaced from its equilibrium
position. The forces are calculated using density-functional
theory with local-density approximation 共LDA兲 exchangecorrelation potential. The calculations for SrCu2共BO3兲2 werelimited to the low-temperature I4̄2m space group with 44
atoms in the unit cell.
The initial step in this procedure is to determine the equilibrium volume and geometry for which the forces on each
atom in the unit cell are minimized. The ab initio calculations on SrCu2共BO3兲2 were performed using the fullpotential linearized augmented plane-wave 共FP-LAPW兲
method42 with local-orbital extensions43 in the WIEN2K
implementation.44 In this treatment it is assumed that thematerial is paramagnetic and that the spins do not interact;

125101-5

PHYSICAL REVIEW B 79, 125101 共2009兲

HOMES et al.

FIG. 6. Calculated total energy for the formula unit
SrCu2共BO3兲2 in the low-temperature I4̄2m space group as a function of volume with constrained c / a ratio. The calculated equilibrium volume of 260 Å3 / f.u. is in good agreement with experimental value of 263 Å3 共Ref. 36兲. The dotted line is a fit to the
Murnaghan equation of state 共Ref. 47兲.
FIG. 5. 共Color online兲 The detailed temperature dependence of
共a兲 the imaginary part of the dielectric function of SrCu2共BO3兲2 forlight polarized in the a-b planes in the region of the mode at
443 cm−1 below 50 K and 共b兲 the relative intensity of the mode at
443 cm−1 below 35 K.

however, since the spins in the ground state are in fact correlated this approach may overlook forces generated by the
coupling of spins. Within the scope of this calculation such
effects are assumed to be weak, although this is not necessarily the case.45,46 Studies with different Monkhorst-Packk-point meshes indicated that a 2 ⫻ 2 ⫻ 2 mesh was sufficientfor good energy convergence. During the geometry optimization, the c / a ratio was fixed to the experimentally determined value.36 Further geometric optimization was achievedby refining the atomic fractional coordinates within the unit
cell until the total force on each of the atoms is typically lessthan 0.1 mRy/a.u. The results of the volume and geometry
optimization are summarized in Table II. The geometry optimization yields values for the lattice constants that are ingood agreement with the experimentally determinedvalues.36 The calculated total energy versus volume is illus-

trated in Fig. 6. A bulk modulus of ⬃170 GPa is extracted
by fitting to the Murnaghan47 equation of state.
The electronic band structure that is calculated from thisoptimized geometry reveals a nonzero density of states at the
Fermi level, primarily from the Cu 3d orbitals 共with a small
contribution from O 2p兲, indicating metallic behavior. This is
in contrast to the observed insulating character of this material, suggesting that a hybridized functional consisting of
LDA plus an on-site repulsion U is required to accurately
reproduce the band structure. Oscillator fits to the highfrequency reflectance for light polarized in the planes suggestthat the charge-transfer gap is ⌬0 ⯝ 0.7 eV, indicating that
this system should be viewed as a Mott insulator.48 In asystem such as this one where there are many valence electrons, there are many fully occupied bond states that contribute significantly to the binding energy between atoms, andtherefore the forces; these are not directly related to the density of states at the Fermi level that determine the transport
properties. Therefore, LDA alone has been deemed sufficient
to calculate the forces.

TABLE II. Experimental and theoretical lattice constants and atomic fractional coordinates for the optimized structure of SrCu2共BO3兲2 for the low-temperature body-centered-tetragonal I4̄2m space group 共44
atoms in the unit cell and 5 nonequivalent displacive particles兲. Note that in the optimized structure c / a has
not been allowed to vary.

a 共Å兲
c 共Å兲
1
Sr 共0 2 0兲Cu 共xyz兲B 共xyz兲O1 共xyz兲O2 共xyz兲0.1146
0.29470.40030.3279Experimenta

Theory 共LDA兲

8.982
6.643

8.882
6.569

0.1146
0.29470.40030.14530.28840.24000.20000.2568aReference 36.

125101-6

0.11710.29770.40430.33090.11710.29770.40430.14700.28430.24030.20530.2569

PHYSICAL REVIEW B 79, 125101 共2009兲

INFRARED SPECTRA OF THE LOW-DIMENSIONAL…

To determine the phonons at the zone center, a 1 ⫻ 1 ⫻ 1
supercell is sufficient. To obtain a complete set of HellmannFeynman forces, a total of 12 independent displacements are
required; we have considered symmetric displacements
which doubles this number, resulting in 24 separate structure
files. In this case, displacement amplitudes of 0.04 Å wereused. Typical values for the displacements range from 0.02 to
0.06 Å; however, the displacements should be small enoughto ensure that the response is still linear. The introduction of
displacements also has the effect of lowering the symmetryof the system. For these calculations a 2 ⫻ 2 ⫻ 2 k-point mesh
was again chosen. After each structure has converged using
the criteria that the total forces on each atom are less than
0.02 mRy/a.u., the residual forces are collected for each setof symmetric displacements and a list of the HellmannFeynman forces are generated. Using the program PHONON,49
the cumulative force constants deconvoluted from theHellmann-Feynman forces are introduced into the dynamical
matrix, which is then diagonalized in order to obtain thephonon frequencies.
The relative intensities have been estimated by calculating
the net dipole moment of the atomic displacements

␮i = 兺 Zⴱj wij ,共5兲jwhere Zⴱj is the Born effective charge of the jth atom in theunit cell and wij is its displacement in the ith direction. The
square of each sum is considered to estimate the relative
intensity for light polarized in the direction of that axis. In
this instance, Zⴱj is simply assumed to be the full ionic charge
for each atom.
The calculated E and B2 phonon frequencies for q = 0 arecompared in Table III with the corresponding infrared-active
vibrations observed at 5 K; the calculated relative intensities
are listed and compared with the experimentally measured
quantities 共recall that the oscillator strength is proportional to␻2p,j兲. The overall agreement between experiment 共T Ⰶ Ts兲
and theory is excellent, typically within a few percent, andthere is good agreement between the observed strength of thevibrations and the calculated relative intensities. The atomic
intensity for each vibrational mode is also listed 共this quantity is the sum of the square of the vibrational amplitude ofeach atom over the allowed degrees of freedom兲. The atomic
intensity characterizes the nature of the vibration. In compiling the experimentally observed frequencies in Table III,
there are two E modes calculated to be at 76 and 112, as well
as a B2 mode at 313 cm−1, that are not observed in the infrared reflectance spectra; this is not too surprising as thecalculated relative intensities of these modes are predicted tobe very weak. However, there are promising candidates in
the Raman spectra22,23 for these modes 共indicated by parenthesis in Table III兲. While most of the vibrational assignments have been relatively straightforward, the modes at 693
and 721 cm−1 present a problem. The vibrations have been
assigned to the modes calculated to be at 669 and 670 cm−1;
these modes are nearly degenerate in frequency and have asimilar vibrational character. In addition, both modes are expected to be relatively strong. However, the experimentallyobserved modes are relatively weak, and the strength of the721 cm−1 mode in particular appears to be somewhat sample
dependent.
The relative atomic displacements for the 16 infraredactive E modes are shown in Fig. 7 for the upper copper- andboron-oxygen sheets in order to provide a visual representation of the atomic intensities listed in Table III and to illustrate the character of the modes more clearly. A dividing linein the character of the E 共B2兲 modes occurs at about
500 cm−1. The modes observed at 661, 693, 721, 934, 1228,
and 1308 cm−1 are predicted to consist almost entirely ofboron and oxygen displacements, and the modes observed at
424 and 443 cm−1 are predicted to consist mainly of copperand oxygen displacements. The modes observed at 231 and319 cm−1 retain a boron-oxygen character. The remaining
low-frequency E modes vary greatly in nature. The modes
observed at 157 and 223 cm−1 are predicted to be primarily
copper-oxygen vibrations, while the mode observed at
141 cm−1 is similar but has a significant strontium character.
The mode observed at 125 cm−1 is predicted to be mainly astrontium-oxygen vibration. The remaining two lowfrequency E modes are calculated to have zero intensity andare observed using Raman spectroscopy at 80 and 112 cm−1;
these modes are predicted to involve displacements ofmainly the strontium and copper atoms. It is important tonote that the atomic displacements shown in Fig. 7 are notnecessarily restricted to the copper- and boron-oxygen
sheets; out-of-plane displacements are also observed. However, there are two sheets in the unit cell and the resultant
dipole moment is found to lie solely within the a-b planes.
From Fig. 3 and Table I we note the general absence ofany strong phonon frequency shifts through the phase transition or at low temperature 共typically only a few cm−1兲 orasymmetric phonon line shapes; this suggests that insofar as
the infrared-active modes are concerned, the spin-phonon
coupling in this compound is quite weak.
C. Low-frequency modes

It is interesting to once again examine the nature of thethree modes at 125, 141, and 157 cm−1 at low temperature,
where the character of the 125 cm−1 mode is quite different
than the other two. The strong fundamental mode at
141 cm−1 consists of Sr/Cu-O共1兲 motions, while the
157 cm−1 mode consists mainly of Cu-O共2兲 displacements;
however, a common feature of the 141 and 157 cm−1 modesis the torsional motion of different aspects of the copperoxygen plaquette. The 125 cm−1 vibration is mainly a Sr–
O共1兲/O共2兲 mode that involves a rocking motion of the boronand copper-oxygen plaquettes 共in which the boron and copper are essentially stationary兲. The low-frequency mode at
125 cm−1 is distinctly different from the other two in that it
does not involve significant copper-oxygen interactions. Perhaps the most peculiar aspect of the 125 cm−1 mode is theincrease in oscillator strength with decreasing temperature.
The intensity of an oscillator should be independent of temperature, as we observe for the 141 and 157 cm−1 modes inFig. 4共c兲; variations in the intensity are usually associatedwith changes in the coordination or structure, or in the formal charges on the ions. While the 125 cm−1 mode is indeed

125101-7

PHYSICAL REVIEW B 79, 125101 共2009兲

HOMES et al.

TABLE III. The experimentally observed 共T ⬃ 5 K兲 and calculated phonon frequencies at the zone centerof the infrared 共and Raman兲 active E and B2 modes for SrCu2共BO3兲2 in the tetragonal I4̄2m setting; theestimated numerical uncertainty in the calculation is roughly 5%. The E modes are active in the a-b plane,
while the B2 modes are active only along the c axis. 共Those modes that are seen only in the Raman results areshown in parenthesis for the E modes at 80 and 112 cm−1 and the B2 mode at 317 cm−1.兲 The relative
intensities of the modes have been calculated from the modulus of the induced dipole moments ␮2i . The
character of the mode is illustrated by the atomic intensities shown to the first two significant figures.
Atomic intensityMode␻obs a共cm−1兲

␻calc
共cm−1兲

兩␮2i,calc兩
共rel.兲

Sr

Cu

B

O共1兲

O共2兲

E
E
E
E
E
E
E
E
E
E
E
E
E
E
E
E
B2
B2
B2
B2
B2
B2
B2
B2
B2

1308 s1228 s934 vw
721 vw
693 w
661 m
443 vw
424 s
319 m
231 vw
223 vw
157 vw
141 w
125 vw
共112兲
共80兲
1347 m
955 vw
695 vw
682 s
447 vw
共317兲
211 s
150 vw
101 w

1355
1268
932
670
669
609
442
392
299
222
204
172
140
129
112
76
1361
956
641
642
423
313
212
165
99

0.83
1.00
0.00
0.26
0.10
0.03
0.00
0.21
0.01
0.00
0.01
0.01
0.03
0.01
0.00
0.00
0.02
0.00
0.00
1.00
0.00
0.00
0.13
0.00
0.00

0.00
0.00
0.00
0.00
0.00
0.00
0.00
0.00
0.03
0.03
0.01
0.02
0.57
0.21
0.37
0.51
0.00
0.00
0.00
0.00
0.00
0.00
0.09
0.16
0.48

0.00
0.00
0.00
0.05
0.06
0.02
0.23
0.28
0.02
0.11
0.60
0.18
0.16
0.06
0.53
0.32
0.00
0.01
0.04
0.00
0.30
0.62
0.28
0.12
0.26

0.74
0.72
0.00
0.43
0.36
0.10
0.04
0.06
0.23
0.11
0.03
0.01
0.03
0.04
0.00
0.04
0.72
0.01
0.14
0.79
0.11
0.03
0.14
0.00
0.00

0.18
0.01
0.35
0.30
0.36
0.26
0.10
0.17
0.12
0.08
0.17
0.18
0.20
0.38
0.02
0.02
0.21
0.40
0.16
0.06
0.22
0.06
0.10
0.50
0.23

0.08
0.27
0.65
0.22
0.22
0.62
0.63
0.49
0.60
0.67
0.19
0.61
0.04
0.31
0.08
0.11
0.07
0.58
0.66
0.15
0.37
0.29
0.39
0.22
0.03

a
The qualitative descriptions of the strengths of the modes have been sorted in the following manner: very
weak 共vw兲, ␻ p,j ⬍ 100 cm−1, weak 共w兲, ␻ p,j ⬍ 200 cm−1, and medium 共m兲, ␻ p,j ⬍ 300 cm−1; all other modes
are labeled as strong 共s兲.

associated with a structural phase transition, studies indicatethat both the unit-cell dimensions and the fractional coordinates change very little below 200 K 共Ref. 36兲, precisely the
point where this mode begins to gather strength. It is possiblethat a redistribution of charge within the unit cell may be
responsible for the increase in oscillator strength of thismode; however, one would also expect to see commensuratechanges in the oscillator strengths of other modes with decreasing temperature. Such a condition is expressed throughthe relation50
4␲⑀

共Zⴱe兲2兺j ␻2p,j = Vc ⬁ 兺k Mk k ,共6兲

where 兺kZⴱk = 0, Vc is the unit-cell volume, and j and k index
the lattice modes over all polarizations and the atoms withmass M k, respectively. It is clear from an inspection of Table
I that there is slightly more oscillator strength at T Ⰶ Ts thanfor T ⯝ Ts. While the presence of several light ions prevents
any estimate of the effective charge for a specific ion, theincrease in oscillator strength supports the view that the material may become increasingly ionic at low temperature.
Whatever mechanism is responsible for the increase in oscillator strength of the E mode at 125 cm−1, it is likely that thisis also responsible for the similar behavior of the E modes at
223 and 231 cm−1, as well as the B2 mode at 150 cm−1
which display a similar temperature dependence 共see TableI兲.
We note in passing that in Fig. 3共a兲 the doubly-degenerate
E mode at 141 cm−1 appears to develop a weak shoulder at
low temperature 共asterisk兲. This may suggest a further weak
structural distortion that results in an additional lowering of125101-8

PHYSICAL REVIEW B 79, 125101 共2009兲

INFRARED SPECTRA OF THE LOW-DIMENSIONAL…

1308 (1355)

1228 (1268)

934 (932)

721 (670)

693 (669)

661 (609)

443 (442)

424 (392)

319 (299)

231 (222)

223 (204)

157 (172)141 (140)125 (129)112 (112)

80 (76)

FIG. 7. 共Color online兲 The calculated relative atomic displacements in the a-b planes for the 16 infrared-active E modes in SrCu2共BO3兲2;
only the upper copper-boron sheet in the unit cell is shown. The observed frequency is shown below the displacements, with the calculated
frequency indicated in parenthesis. The color scheme used to depict the atoms is taken from Fig. 1.

the symmetry and the removal of the degeneracy of thismode. However, at this time we are not aware of any highresolution structural studies at low temperature that would
support this claim.51
D. 443 cm−1 mode

The imaginary part of the dielectric function is shown inthe vicinity of the mode at 443 cm−1 in Fig. 5共a兲 and therelative intensity in Fig. 5共b兲. Interestingly, there is no indication of a feature at this frequency above ⬃20 K; below
this temperature this feature narrows and hardens only
slightly. There are several possible explanations as to theorigin of this feature; one is that it is simply the weak E
mode calculated to be at 442 cm−1. It is also possible that
this feature is a combination of two other vibrations, such as

the E mode at 319 cm−1 and a B1 mode at 124 cm−1, which
sum to 443 cm−1; note that in the D2d point group E⫻ 共A1 , A2 , B1兲 = E, so this combination is an allowed infraredactive mode, although it is expected to be very weak. A third
possibility is that this feature originates from the splitting of
the strong E mode at 424 cm−1 due to a symmetry-breaking
process; however, the lack of similar features in other strong
modes makes this unlikely. These scenarios, while all areplausible to varying degrees, do not explain the unusual temperature dependence of this mode. The fact that the temperature dependence of the intensity of this feature is almost
identical to those of the magnetic excitations, as well as themore general dc susceptibility,20 suggests a possible magnetic origin for this feature. Since the exchange couplings
J ⯝ 70 cm−1 we may rule out a purely magnetic excitation. It
is possible that this mode is a combination of the strong

125101-9

PHYSICAL REVIEW B 79, 125101 共2009兲

HOMES et al.

424 cm−1 mode and a magnetic excitation, with the closest
candidate being the singlet at ⯝21.5 cm−1 observed in infrared magnetoabsorption26 and high-field electron-spin
resonance.17 While the temperature dependence of this mode
points to a magnetic origin, to properly determine whether
this feature is a phonon or a combination of a phonon and amagnetic excitation, the magnetic-field dependence of thefeature at 443 cm−1 should be investigated. Finally, we
noted earlier in text that the temperature dependence of the443 cm−1 mode was very similar to another in-plane mode
observed at 52 cm−1; however, there is compelling evidence
that the 52 cm−1 feature is a pure magnetic mode.25
V. CONCLUSIONS

The reflectance of insulating SrCu2共BO3兲2 is dominatedby the symmetry-allowed infrared lattice vibrations aboveand below the structural phase transition. In agreement withgroup theory, a number of new modes are observed below Ts.
Ab initio calculations were performed using densityfunctional theory with LDA and the direct method to determine the frequencies, atomic character, and relative intensities of the infrared-active E and B2 modes for the roomtemperature phase 共T ⬍ Ts兲 of this compound. The agreement

between the calculated and experimentally observed frequencies 共Table III兲 is excellent, and all the predicted modes havebeen identified.
The intensity of most of the infrared-active modes displays little temperature dependence 共Table I兲. However, several modes, in particular an E mode at 125 cm−1 and a B2
mode at 150 cm−1, become visible only for T Ⰶ Ts and display a steadily increasing oscillator strength with decreasing
temperature. This unexpected result suggests that a redistribution of charge within the unit cell occurs at low temperature. The absence of any large frequency shifts or asymmetric phonon line shapes suggests that, at least as far as theinfrared-active vibrations are concerned, the spin-phonon
coupling in this compound is very weak.
A weak mode at 443 cm−1 is observed only at low temperature and displays a similar temperature dependence tothe magnetic excitations. This is similar to a feature at
52 cm−1, previously observed in the infrared magnetoabsorption that has been identified as an electric-dipole transition in the dimer spin system. It is likely that the 443 cm−1
feature is a combination of a strong E mode at 424 cm−1 anda magnetic excitation. However, additional study of themagnetic-field dependence of this mode is required to determine if this is simply a phonon or a combination of a phonon
and a magnetic excitation.

TABLE IV. The experimentally observed 共T ⬃ 5 K兲 and calculated phonon frequencies at the zone centerof the A1, B1, and A2 Raman-active modes for SrCu2共BO3兲2 in the tetragonal I4̄2m setting; the estimatednumerical uncertainty in the calculation is roughly 5%. The character of the mode is illustrated by the atomic
intensities shown to the first two significant figures.

Mode
A1
A1
A1
A1
A1
A1
A1
A1
A1
B1
B1
B1
B1
B1
B1
A2
A2
A2
A2
A2
A2
A2

Atomic intensity

␻obs
共cm−1兲

␻calc
共cm−1兲

Sr

Cu

B

O共1兲

O共2兲

1360
950

1379
881
649
640
489
268
209
93
⬃0
1237
651
390
312
270
113
1267
593
457
300
227
196
156

0.00
0.00
0.00
0.00
0.00
0.00
0.00
0.00
0.00
0.00
0.00
0.00
0.00
0.00
0.00
0.00
0.00
0.00
0.07
0.01
0.91
0.01

0.00
0.01
0.00
0.00
0.40
0.30
0.52
0.20
0.57
0.00
0.02
0.08
0.31
0.01
0.58
0.00
0.00
0.17
0.01
0.00
0.01
0.81

0.71
0.00
0.75
0.20
0.05
0.00
0.09
0.16
0.04
0.72
0.03
0.01
0.16
0.00
0.08
0.71
0.03
0.00
0.23
0.01
0.02
0.00

0.19
0.38
0.06
0.26
0.08
0.54
0.13
0.29
0.07
0.00
0.58
0.22
0.14
0.00
0.06
0.01
0.73
0.09
0.12
0.00
0.01
0.05

0.10
0.61
0.19
0.54
0.47
0.16
0.26
0.35
0.32
0.28
0.37
0.69
0.39
0.99
0.28
0.28
0.24
0.74
0.57
0.98
0.05
0.13

473
285
198
122
60
706
386
323
283
125

156

125101-10

PHYSICAL REVIEW B 79, 125101 共2009兲

INFRARED SPECTRA OF THE LOW-DIMENSIONAL…
ACKNOWLEDGMENTS

The authors would like to thank A. Akrap, B. D. Gaulin, J.
Hancock, W. Ku, and T. Timusk for useful discussions. This
work was supported by Grant-in-Aid for Scientific Research
on Priority Areas from MEXT of Japan 共Contract No.
19052004兲. Work at UCSD is supported by NSF Grant No.
DMR 0705171; work at BNL is supported by the Office of
Science, U.S. Department of Energy 共DOE兲 under Contract
No. DE-AC02-98CH10886.

APPENDIX: RAMAN MODES

The Raman-active A1, B1, and A2 modes have also been
calculated. The experimental values from the literature22,23,36
are compared with the calculated frequencies in Table IV.
The lack of high-frequency data results in a list of assigned
frequencies that is not as comprehensive as in Table III. In
general, the agreement between the calculated and observed
frequencies appears to be quite good. In particular, the modewith A1 symmetry observed at very low frequency just below
Ts that hardens to about 60 cm−1 at low temperature22,36 islikely the lowest-frequency A1 mode. Similarly, the Raman
mode at 124 cm−1 that had previously been assigned as an
overtone22 of this vibration now appears to be the next highest A1 mode, although it must be said that the agreement withthe calculated frequencies is less than ideal 共better agreement

would likely be achieved through the use of larger supercells
in the calculations兲.
The assignment of the A2 mode at 156 cm−1 is unusual as
this mode is silent if phonon coupling alone is considered.
However, if other processes are taken into account 共i.e., spinorbit interaction, etc.兲 then the resonant Raman-scattering
process coupling to the antisymmetric A2 modes is generally
not forbidden. It is also possible that the mode at 156 cm−1
is not an A2 mode at all but a combination of the fully symmetric A1 mode at 122 cm−1 and an A2 species triplet excitation at roughly 36 cm−1 共in the D2d point group A1 ⫻ A2
= A2兲. However, this assignment remains rather speculative.
While there is little evidence for spin-phonon coupling in
the infrared-active modes 关see for instance Fig. 3共b兲, wherethe vibrations show a continuous hardening below 30 K兴, theA1 mode observed at ⬃60 cm−1 does show a slight softening
below about 15 K 共Ref. 22兲. Indeed, our own unpublished
Raman results52 for this compound not only verify the softening in the A1 mode at ⬃60 cm−1 but also identify a similarsoftening in another A1 mode at 198 cm−1. However, an A1
mode at 122 cm−1 shows little change in frequency at low
temperature. The difference in behavior of these modes may
arise from the fact that the A1 mode at 122 cm−1 is predicted
to have a mixed copper- and boron-oxygen characters, while
the A1 modes at ⬃60 and 198 cm−1 have a primarily copperoxygen character, suggesting that the weak softening of thesevibrations at low temperature may be due to spin-phonon
coupling.

047202 共2001兲.

*homes@bnl.gov
1 H. Kageyama, K. Yoshimura, R. Stern, N. V. Mushnikov, K.

14 G. A. Jorge, R. Stern, M. Jaime, N. Harrison, J Bonca, S. E.

Onizuka, M. Kato, K. Kosuge, C. P. Slichter, T. Goto, and Y.
Ueda, Phys. Rev. Lett. 82, 3168 共1999兲.
2 H. Kageyama, K. Yoshimura, R. Stern, N. V. Mushnikov, K.
Onizuka, M. Kato, K. Kosuge, C. P. Slichter, T. Goto, and Y.
Ueda, J. Phys. Soc. Jpn. 68, 1821 共1999兲.
3 H. Kageyama, N. V. Mushnikov, M. Yamada, T. Goto, and Y.
Ueda, Physica B 329-333, 1020 共2003兲.
4 S. Miyahara and K. Ueda, Phys. Rev. Lett. 82, 3701 共1999兲.
5 Zheng Weihong, C. J. Hamer, and J. Oitmaa, Phys. Rev. B 60,
6608 共1999兲.
6 E. Müller-Hartmann, R. R. P. Singh, C. Knetter, and G. S. Uhrig,
Phys. Rev. Lett. 84, 1808 共2000兲.
7 A. Koga and N. Kawakami, Phys. Rev. Lett. 84, 4461 共2000兲.
8K. Kodama, M. Takigawa, M. Horvatić, C. Berthier, H.
Kageyama, Y. Ueda, S. Miyahara, F. Becca, and F. Mila, Science
298, 395 共2002兲.
9
S. Miyahara and K. Ueda, J. Phys.: Condens. Matter 15, R327
共2003兲.
10 M. Takigawa, S. Matsubara, M. Horvatic, C. Berthier, H.
Kageyama, and Y. Ueda, Phys. Rev. Lett. 101, 037202 共2008兲.
11 R. W. Smith and D. A. Kesler, J. Solid State Chem. 93, 430
共1991兲.
12 B. Sriram Shastry and B. Sutherland, Physica B & C 108, 1069
共1981兲.
13 M. Hofmann, T. Lorenz, G. S. Uhrig, H. Kierspel, O. Zabara, A.
Freimuth, H. Kageyama, and Y. Ueda, Phys. Rev. Lett. 87,

Shawish, C. D. Batista, H. A. Dabkowska, and B. D. Gaulin,
Phys. Rev. B 71, 092403 共2005兲.
15 S. Zherlitsyn, S. Schmidt, B. Wolf, H. Schwenk, B. Lüthi, H.
Kageyama, K. Onizuka, Y. Ueda, and K. Ueda, Phys. Rev. B 62,
R6097 共2000兲.
16 B. Wolf, S. Zherlitsyn, S. Schmidt, B. Lüthi, H. Kageyama, andY. Ueda, Phys. Rev. Lett. 86, 4847 共2001兲.
17 H. Nojiri, H. Kageyama, Y. Ueda, and M. Motokawa, J. Phys.
Soc. Jpn. 72, 3243 共2003兲.
18 H. Kageyama, M. Nishi, N. Aso, K. Onizuka, T. Yosihama, K.
Nukui, K. Kodama, K. Kakurai, and Y. Ueda, Phys. Rev. Lett.
84, 5876 共2000兲.
19 O. Cépas, K. Kakurai, L. P. Regnault, T. Ziman, J. P. Boucher, N.
Aso, M. Nishi, H. Kageyama, and Y. Ueda, Phys. Rev. Lett. 87,
167205 共2001兲.
20
B. D. Gaulin, S. H. Lee, S. Haravifard, J. P. Castellan, A. J.
Berlinsky, H. A. Dabkowska, Y. Qiu, and J. R. D. Copley, Phys.
Rev. Lett. 93, 267202 共2004兲.
21 P. Lemmens, M. Grove, M. Fischer, G. Güntherodt, V. N. Kotov,
H. Kageyama, K. Onizuka, and Y. Ueda, Phys. Rev. Lett. 85,2605 共2000兲.
22 K.-Y. Choi, Y. G. Pashkevich, K. V. Lamonova, H. Kageyama, Y.
Ueda, and P. Lemmens, Phys. Rev. B 68, 104418 共2003兲.
23
A. Gozar, B. S. Dennis, H. Kageyama, and G. Blumberg, Phys.
Rev. B 72, 064405 共2005兲.
24 A. Gozar and G. Blumberg, in Frontiers in Magnetic Materials,

125101-11

PHYSICAL REVIEW B 79, 125101 共2009兲

HOMES et al.
edited by A. V. Narlikar 共Spinger-Verlag, Berlin, 2005兲, pp. 735754; this work was originally made available online atarXiv:cond-mat/0509630.
25 T. Rõõm, U. Nagel, E. Lippmaa, H. Kageyama, K. Onizuka, andY. Ueda, Phys. Rev. B 61, 14342 共2000兲.
26
T. Rõõm, D. Hüvonen, U. Nagel, J. Hwang, T. Timusk, and H.
Kageyama, Phys. Rev. B 70, 144417 共2004兲.
27 J. W. Bray, L. V. Iterrante, I. S. Jacobs, and J. C. Bonner, inExtended Linear Chain Compounds, edited by J. S. Miller 共Plenum, New York, 1983兲, pp. 353-415.
28 X. K. Chen, J. C. Irwin, and J. P. Franck, Phys. Rev. B 52,
R13130 共1995兲.
29
C. C. Homes, M. Ziaei, B. P. Clayman, J. C. Irwin, and J. P.
Franck, Phys. Rev. B 51, 3140 共1995兲.
30 A. B. Kuz’menko, D van der Marel, P. J. M. van Bentum, E. A.
Tishchenko, C. Presura, and A. A. Bush, Phys. Rev. B 63,
094303 共2001兲.
31 U. Kuhlmann, C. Thomsen, A. V. Prokofiev, F. Büllesfeld, E.
Uhrig, M. Anton, C. Gross, and W. Assmus, Phys. Status Solidi
A 196, 185 共2003兲.
32 A. B. Sushkov, O. Tchernyshyov, W. Ratcliff, S. W. Cheong, and
H. D. Drew, Phys. Rev. Lett. 94, 137202 共2005兲.
33
G. Caimi, L. Degiorgi, H. Berger, and L. Forró, Europhys. Lett.
75, 496 共2006兲.
34 J. Kim, S. Jung, M. S. Park, S. I. Lee, H. D. Drew, H. Cheong,K. H. Kim, and E. J. Choi, Phys. Rev. B 74, 052406 共2006兲.
35
J. Vermette, S. Jandl, and M. M. Gospodinov, J. Phys.: Condens.
Matter 20, 425219 共2008兲.

36

K. Sparta et al., Eur. Phys. J. B 19, 507 共2001兲.

37 H. Kageyama, K. Onizuka, T. Yamauchi, and Y. Ueda, J. Cryst.

Growth 206, 65 共1999兲.
C. C. Homes, M. Reedyk, D. Crandles, and T. Timusk, Appl.
Opt. 32, 2972 共1993兲.
39 C. C. Homes, J. M. Tranquada, and D. J. Buttrey, Phys. Rev. B
75, 045128 共2007兲.
40
M. Dressel and G. Grüner, Electrodynamics of Solids 共Cambridge University Press, Cambridge, 2001兲.
41 K. Parlinski, Z-. Q. Li, and Y. Kawazoe, Phys. Rev. Lett. 78,
4063 共1997兲.
42
D. J. Singh, Planewaves, Pseudopotentials and the LAPW
Method 共Kluwer Academic, Boston, 1994兲.
43 D. J. Singh, Phys. Rev. B 43, 6388 共1991兲.
44 P. Blaha, K. Schwarz, G. K. H. Madsen, D. Kvasnicka, and J.
Luitz, WIEN2K, an augmented plane wave plus local orbitals program for calculating crystal properties, Techn. Universität Wien,
Austria, 2001.
45 W. Baltensperger, J. Appl. Phys. 41, 1052 共1970兲.
46 C. J. Fennie and K. M. Rabe, Phys. Rev. Lett. 96, 205505
共2006兲.
47
F. D. Murnaghan, Proc. Natl. Acad. Sci. U.S.A. 30, 244 共1944兲.
48 S. V. Dordevic 共private communication兲.
49 K. Parlinksi, software PHONON, 2003.
50 J. F. Scott, Phys. Rev. B 4, 1360 共1971兲.
51
B. D. Gaulin 共private communication兲.
52 A. Gozar 共private communication兲.
38

125101-12