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Transcript of tic Mv # o ? m 3 3 n ISEDD %a&A 010015523-3 - OSTI.GOV
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(ottxm, mm)
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Ao ; OPTICAL DENSITY
044 LBS : SP1822, A =620nm)
a(1);b(2);c(3);d, e(5@)
ENERGY! j/cm2)045
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400 600 800Repetition Number
El 47 SP1822<D"f/ff
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100 200 300 400 500 600 700 800 900 1000Repetition Number
048 (it 1. 0x 10~5M)
A/Ao 0.5
Repetition Number
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WAVELENGTH(nm)
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- 126-
(618, a)(650. B )
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Wavelength(nm)@352 a > yS , A a . A 0 0^#
20 40ENERGY(mJ/cm2)
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p H B
2. i. 7 m
1) mmfo#, Am, 969(1989).
2) mam#, B$<k#A#56#%##9%#, 725(1988).
3) mem#, 363(1988).
4) K. Sakoda, K. Kominami and M. Iwamoto, Jpn. J. Appl. Phys., 27(7),
11304(1988).
5) K. Sakoda, K. Kominami and M. Iwamoto, Jpn. J. Appl. Phys., 28, Suppl.
28-3, 229(1989).
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Phys. Rev., Ml , 3185(1990).
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pp853 (1963).
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13) RB#l62#m6%m#^#o
14) Hig-i-vf- >J TJl, 3J35H^t, pll (1990) .
15) K. Kobayashi, H. Sumitomo and Y. Ina, Polym. J., 15, 667(1983).
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Japan,33 (2), 1310(1984).
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983(1990).
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LI 144 (1990).
19) BB%635^J:%mm#5#o
- 157-
20)
21) W. Koehler and J. Friedrich, Phys. Rev. Lett., 59(19), 2199(1987).
22) W.Koehler, J. Zol If rank and J.Friedrich, Phys. Rev. B39(8), 5414(1989)
- 158-
x
X TSPP(Na) : o-*TCPP(Na) : —^ ^-CO]Na
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Ether
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20 40 60 80 100T(K)
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01
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3: 57.1kV/cm
17124 17127
Wavenumbers (cm1)
17124 17127
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1. W. E.Moerner, ed., Persistent Spectral Hole Burning: Science and
Applications (Springer-Verlag, Berlin, 1988).
2. W. E. Moerner, J. Mol. Elect. L_ 55-71 (1985).
3. M.Maier, App 1. Phys. B 41, 73-90(1986).
4. A. J.Meixner et a 1., J. Phys. Chem. 90, 6777-6785(1986).
5. G. C. Bjork 1 und, Opt. Lett. 5^15-17(1980).
6. M. Romagno 1 i et a 1. , J. Opt. Soc. Am. B 1, 571-585(1984).
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YAG Laser
ms. 9
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wavelength ( nm)
0 3.10 ZnTPPOiiRx^^ h/V
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600 700wavelength(nm)
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SY0:901217057.SPC DET: 8IA SOURC: QH1 B/S: QU1 SP: 7 SM: 1RES : 0.100 DATE:21-OEC—90 TIME: 17:34:11 BC: 1 PC: 3COADD: 16 LP: 4 HP: 2
7.1 K DEG,, 420SEC0NDS EXPOSURE, 852.853 mm
APER: 7 EV: E APOD: HAMMING FILTER: FIS
6
X 1.0E+041.87
1. 10-
0.72-
0.33-
-0.0515950. CM—1 .62696 UM
15450..64725
15260..85789
15760.:63694
14950..66890
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SY0:901217057.SPC DET: SIA SOURC: OH1 B/S: QU1 SP: 7 SM: 1RES : 0.100 0ATE:21-DEC-90 TIME: 17:34:11 BC: 1 PC: 3COADD: 16 LP: 4 HP: 2
7.1 K DEC., 420SECOND8 EXPOSURE, 652. 853 mm
APER: 7 EV: E APOD: HAMMING FILTER: FIS
6
X 1.0E+035.000
3.898-
2.796-
0.592-1
-0.51015340.0 CM—1 .651890 UM
15330.0 .852316
15320.0.652741
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Polymer Formu1 a Peak frequency ( cm ”1)
1 polystyrene (CH2CHC6H5) n 14± 12 po1y(methy1 methacrylate) (CH2CCH3CO2CH3) n 133 poly (ethyl methacrylate) (CH2CCH3CQ2C2H3)n 134 poly (butyl methacrylate) (CH2CCH3CO2C4H9). 165 poly(auryl methacrylate) (CH2 CCH 3 CO 2 C12 H 25)n 166 poly (vinyl acetate) (CH2 CHO2 CCH3) n 127 poly(2-hydroxyethyl methacrylate) (CH2CCH3CO2C2H4OH). 238 poly (vinyl alchohol) (CH2CHOH) „ 259 poly (acryl ic acid) (CH2CHCOOH) „ 25
10 urea formaldehyde resin b) 2311 dextran (C 6 H 1 0O5) n c> 30
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[ i ] swiftraa = 37, 388 (1988)
[2] S.Saikan, A.Fujiwara, T.Kushida and Y.Kato,
Jpn. J. Appl. Phys. 26, 1941 (1987)
[3] S.Saikan, H.Miyamoto, Y.Tosaki and A.Fujiwara,
Phys.Rev. B36 5074 (1987)
[4] 37, 79 (1987)
[5] S.Saikan, Phys. Rev. A38 4669 (1988)
[6] S.Saikan, T. Nakabayashi, Y. Kanematsu and N. Tato,
Phys.Rev. B38 5074 (1988)
-316-
[7] S. Saikan, Ultrafast phenomena VI, Spr inger-Ver lag, p 349
[8] S. Saikan, A. Imaoka, Y. Kanematsu and T. Kishida,
Chem, Phys. Lett. 162, 217 (1989)
[9] S. Saikan, A. Imaoka, Y. Kanematsu, K. Sakoda,
K. Kominami and M. Iwamoto, Phys. Rev. B41, 3185 (1990)
[10] S. Saikan, T. Kishida, Y. Kanematsu, H. Aota,
A. Harada and M. Kamachi, Chem. Phys. Lett. 166, 358 (1990)
-317-
mmzmz# ^pii
1.
a = tt d (nL—nR ) /A (radian)
RIR®^: um#^#GT &o £< m\,' Z>tl2>(D&± h u R A © D
m (589nm) ------
:
[ a ] = a / c d
c =mm g/mU d = -t? A/ JE (dm= -r y y — h ;V)
:
Em’ ] = ( 3 Zn 2 +2) (MW/100 ) [a]
n =9Z%m#T$, MW = ^f i
2.
Drude
Em’ ] = a A o 2Z (A 2 - A 02)
A o - # iR 0 c# ,i:\ # #
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(0£J& £ # ft © > Kron ig-Kramers Relation)
WORD)XfCD)
Figure 1.6. Optical rotatory dispersion (ORD) and circular dichroism (CD)
curves for a pair of coupled oscillators.
3. me?®*##®##!#
1) Z> C t tc J: -o T Se g <D
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2 ) h V y ^ t #
aimgiitzm&t Zo —
3 ) ^t£7 t h ? a i y ?
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[ a ) d = - 42° (trans)
~ 0 ° (cis)
319-
ffl. 2 fcfxr > h V
4. 7 * b ? u i y t
i) T'/Ky ') k
459 (1980) Figure 2. Circular dichroism spectra associated
with the amide n- n * transition bef ore( —) and
after (----) photoirradiation in the mixed
solvents of various DCE/HFIP compositions.
- 320-
fH fo 7 -i Jl A 1+1
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CH3
x=2.4(%),y=26,z=15
mm
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0
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CHz 2, £OOCHz^N=N@ £OOCHz®
CHiKl-CHzCHzNI+fCOCHNH^------------------- (COCHNHfeHLU
220 230 260 250
Wave Length ( nm )
Figure. CD Spectra of the
membrane; (—)after Vis.
irradiation, (---•) after UV
irradiation.
b-ti-AvK^iJ VO-t? >{8m£&o V v
# V f K
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$
Aib TypeCH3
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9°0 '^NCHz
Y
= p[ Lys (Z)m-azoAla] rh=1,2,3 = p[Lys(Z)m'-azoAla-Ai b] m' = (0), 1.2
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Delta Epei1 on/Azobenzene Unit
coCOCO
Delta EpeI Ion/Azobenzene Unit
6% ( C D ) X < ?
h h 7 > X
: ------ . y %
Table I. Optical Rotation at 589 nm for Polypeptides and
Model Peptides. Solvent=TMP, 5 cm cell.
Polypeptide [a ] D (trans) [ a ] D (cis) concentration(M)
1-1" <30°I-2b 270° 180° 8. 6x IQ'S1-3" <10°
11-1 2.2° -19° 3. 2x 10-*11-2 -206° -110° 1. 95x 10~311-3 -18°
OO 3.58x10-'
Ac-azoAla-OMe <5° 116° 3. 96x 10-'Ac-(azoAla)2-OMe -13° -19° 4.12x 10-'
"Due to a limited solubility of the I-m polypeptides, accurate [a] d
values could not be measured.
Photo isomeric State
- 323-
-bJln-xmmfc m*. AE £> Chem. Left., 1986, 983.
OCONIIR
,OCONIIR
\
R-2
6 -* X
[a] d =+94° (trans)> -41° (cis)
( T H F 40 200 300 400 500 600Havelength/nm
Fig. 1 Absorption (A) and CD
(B) aspectra in the trans-cis
isomerization of CPAPC in
THF <8> . (trans content: a,
lOOg; b, 70g; c, 40; d, lOg).
— 324 —
5. +7/1/7 h v v ^
1) □ l/Xf 'J 7
nl/Xf'J7 ^ %^#$2C D (C L C I C D)
Circular Dichroism Indiced by Cholesteric Liquid Crystals (CLCICD)
Hj_L M//L ------—-
For LII-CLC with XQb < *refM // l: gab < 0 H x L: 9ab > 0
2(Al - A„>
E. Sackmann and J. Voss,Chem. Phys. Lett. , 14, 528 (1972).
CPL
h - np
RCPL : Reflected
LCPL: Transmitted
Glass Plate
CLC(RH Helix)
>lO/i
Selective Reflection by CLC
9Cz -2/2N-2 (50/50)k -0.5
X (nm)
•Lb TRANSITION MOLECULAR AXISMOMENT
'Lb TRANSITION MOLECULAR AXISMOMENT
— 325 —
PALGII^OS P 0
S£* b, Polym. Bull., 17, 285 (1987)
PALG: (NH-CH-C0)n-(CH2)2
CO0
H,rig. 1 Reversible change In optical rotatory power of PALG thin films
containing the splropyran of 1 molt (-Q-) and 4 molt ( -O- I In alternative illumination with uv(------ ) and visible light (-------- ) for20 sec.
Open and full marks represent colorless and photo-merocyanlne form, respectively.
Preparation condltltlons of the films t Method B, casting concentration “4.5 wtt, solvent • dloxane. Film thickness I about 4 tin.
6 6 Repetition times
2)
2ti2JI(l& rr ^ U -7- J CMC ( 1988)
Ky 'jfr-L - $)\>9 y - p <b K f y/i/- L - y - P
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—("CO —CH — NP0r-I 7
CM*ICl 12ICOCHCHz^H
4
m i.2o (cd) b -]300 150 200
p;i/o a wcco
3 > 3 i/ xt- v v ftz 'jti'Dfy ?m n
- (Nil-CH-CO) - (NH-CH-CO)-
u 200
E 100
Havelength (nm)
--------I P8LG membrane1C12-Azo(2.505E-2M)/C0/230-530nm
4)
Havelength (nm)
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t£lii b> BCSJ, 57, 3253 (1984)
CH3 0 CH,
Cg-L-Ala-Azo-CmN
50-70*
Wavelength Z nm
Fig. 2. Temperature dependence of absorption (a) and CD (b) spectra. C,-L-Ala-Azo-C10N+, 5x 10~* M, heating cycle.
- 327-
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(1) m#^m, 68(12), 1333-1341(1985)
(2) &##&- :7t^'yUX^yf> / 6###^###, F^###
#, p -206 (AS, 1988)
(3) ^fflfarfjb : l, be^ u, no.452, 131-157(1988)
(4) -la^Hf : yt° 54(10), 1019-1030(1985)
(5) Mil : r%ta###J , P183-207 (A#, 1988)
(6) : B4L#56###^Xm, #1102, (1988)
(7) Y. Wang, et. a 1., Chem. Phys. Lett., 148 (2,3), 136(1988)
(8) mmmn, b
142#m^#46[g^im#%^%#, P22-27(1989. 11)
(9) BBBS3A 5> : *Sm&-7 9 □ ->7^ PMMAI, Polymer Preprints,
38(8), 2639-2691(1989)
00) S. Matsumoto, et. a 1., Mol. Crys. & Liq. Crys., in print (1990)
01) D. Narayana, et. a 1., Appl. Phys. Lett., 48(18), 1187-1189(1986)
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condtors, p155-162(Springer, 1988)
04) , pon-622
( BfiJXS, 1989)
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- 336-
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- 337-
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338-
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- 339-
PHONON STRUCTURES IN THE SPECTRA OF SOLIDS
Y.TOYOZAWA
Institute for Solid State Physics, University of Tokyo,
Roppongi, Minato-ku, Tokyo, Japan
Recent studies on phonon structures in the optical spectra of (A) localized
electrons and (B) intrinsic excitons are surveyed from a unified view-point.
The coupling function, the basic quantity governing the multiphonon structures,
is subject to various effects of local perturbation of lattice, and is sensitive
to spacial extension of electronic orbitals. Remarkable difference in phonon
structures between (A) and (B) can be related with the motional reduction of
coupling strength in case (B). Exciton motion in a deformable lattice is
classified into three types, which are closely correlated with features of
exciton emission spectra.
1. I nt rodut i on
Dynamic aspects of the motion of electrons in a deformable lattice manifest
themselves most clearly in the line shapes of absorption and emmission spectra
associated with the electronic transitions. The electron-phonon interaction
causes phonon structures, line widths and shifts, removal of electronic
degeneracies and many other effects in the optical spectra; careful analysis of
the line shapes sometimes provides us with insight into the details of
interacting electron-phonon system. The purpose of the present paper is to give
a comprehensive, rather than exhaustive, survey on recent developments in
theoretical studies of phonon structures*1).
* As a review article on the phonon structures in the optical spectra of localized electrons, see, for instance ref.1).
— 340 —
Both (A) localized electronic excitation (and de-excitation) associated with
lattice imperfection (sec. 2 and 3) and (B) intrinsic exciton movable through
the lattice (sec. 4 and 5) will be considered from a unified viewpoint. By so
doing, we will obtain better understanding of the common mechanism underlying
the phonon structures of various types, and deeper insight into the effect of
energy transfer in case (B). Although excitons in organic molecular crystals
as well as those in inorganic crystals are included in case (B), the optical
spectra of the former behave more or less like the case (A), since the exciton
transfer energy in molecular crystal is usually far smaller than that in
inorganic crystal.
Unless otherwise stated, we shall confine ourselves to the case of absolute
zero of temperature where the phonon structures, if any, should be discernible
most clearly.
2. Difference in equilibrium lattice configuration
We start from the Hamiltonian for the electron-phonon system H+ Hl= He +
H6l + Hl which is the sum of the electronic energy H in the deformable
lattice and the lattice vibrational energy Hl. We expand H in powers of
lattice displacement coordinate q whose origin will be chosen in a way
suitable for the individual problems concerned; the zeroth order term will
be denoted by He and will hereafter be called simply the electronic energy,
while the linear and higher order terms, denoted by H„l as a whole, will be
called the electron-lattice interaction. The linear term can be written as
= I I'(r)q,. (1)
qi’s are normal coordinates with which Hl is written in diagonal form: Hl=
£ i(pi + co iqi)/2. The A -1h eigenvalue of He for the localized electrons will
be denoted by EA. The first order perturbation of HjT (to which we shall
-341-
confine ourselves in this section) contributes linear term £ i IU x q 4 to
the adiabatic potential and hence to the relative displacement A i between the
equilibrium configurations for the ground (A=g) and excited (A=e) states:
A i = (I i g — Ii e) / 0) i . (2)
We begin with one dimensional configuration coordinate model to see the effect
of A on the multiphonon structures in the absorption spectra for the
electronic transition g e. As is seen from fig. 1, A is related with
lattice relaxation energy
£=w»AV2, (3)
absorptionA—-
Fig. 1. Adiabatic potentials (center) and absorption spectra (right) with one
dimensional configuration coordinate model for localized excitation.
For intrinsic excitation, the exciton band may be formed (left).
which would be released if the system were excited vertically following the
classical Franck-Condon principle. It corresponds to the number S of released
phonons which is given by
S= s /ha> = (jl> A 2/2h. (4)
In fact, the normalized intensity distribution of the optical transitions from
the lowest vibrational level (n=0) of g to various vibrational levels n of e
- 342-
is given by a Poisson distribution
W„ — exp(- S) • S”/n!, (5)
the most probable number of phonons emitted being n« S. The Debye-Waller
factor e~* is related with the overlap integrate-s/2 between the lowest
vibrational states of g and e1). S is an important parameter characterizing
the multiphonon structures, and will be called the coupling strength.
Generalization to more realistic multidimensional configuration coordinate
model is straightforward. The contribution to (4) comes from various
frequencies:
S — S D (tv ) d to , (6)
D(w) = Z (w i A ?/2M) a (w - w ,). (7)
D(<y) will be called the coupling function. While the zero-phonon line is still
a sharp line with fractional intensity e~8 as before, the line shape of one
phonon sideband is now given by e-sD(co), that of the two phonon sideband by
the convolution: (e~‘/2!) / D(w — co ’ )D(<w ’ )Au>' and so on. (Note that the
energy h oj is measured from the zero-phonon line.) A single function D (co)
determines the line shapes of the multiphonon sidebands of all orders.
The zero-phonon line and multiphonon sidebands would be discernible only if
ScS 5, otherwise the former would be too weak to be observable, while the higher
order sidebands with increasing diffuseness would overlap with each other,
forming a single broad band as a whole.
The above argument applies also to the emission spectra of localized electrons,
if the energy is measured in the opposite direction from the zero-phonon line.
In fact, the absorptiun and emmission spectra should be the mirror image of each
other around the common zero-phonon line, according to the approximation of the
present section.
D((o) contains information on lattice vibrations around the imperfection as
- 343-
seen from the electron as a probe. In the first place, it should reflect the
phonon spectrum of the host lattice, and is therefore expected to show the Van
Hove singularities. However, the selection rule predicts suppression of
singularities at certain important symmetry points in the Brillouin zone when
the imperfection has inversion symmetry. For imperfections with lower symmetry,
it is expected that most of the Van Hove singularities are active in D().
Moreover, the local perturbation of dynamical matrix should give rise to the
metamorphism2) (see fig. 2) of active Van Hove singularities in the one phonon
Fig. 2. Metamorphism of Van Hove singularities Mo, Mi, M2 and M3 into various
shapes, caused by local perturbation of the lattice.
sideband D(<y) as in the case of impurity induced infrared absorption by
lattice vibrations. The phase of the metamorphism shown in fig. 2 is closely
related to the phase shift of scattering of phonons by the imperfection3).
Such singular structures are in fact observed in the phonon sidebands of the
absorption spectra of F-aggregate centers1,4) in alkali halides. The sideband
for a dipole forbidden transition in MgO:V2+ may be another example5). Further
developments in high resolution spectroscopy combined with neutron diffraction
data will enable unambigous assignments of singularities, and may shed a light
on the phonon-imperfection scattering mechanism.
In the second place, the local perturbation sometimes gives rise to localized
mode or resonance mode which appear as a line or a diffuse peak in D ( <m ) as was
344-
observed and analysed for rare earth ions in ionic crystals6).
The third problem concerns the manner in which D(<w) rises as w increases
from zero. The main contribution to low co comes from acoustic mode phonons
of long wavelength; if we take for qi the normal modes of perfect lattice and
use the deformation potential for the electron-phonon interaction (1), D(cu)
rises as co 5 due to the near cancellation of (2) for long wave-length phonons.
If the local perturbation is taken into account, it can be shown7, 3) that D(<y)
rises as co , a result which is in better agreement with observations.
The power becomes larger for dipole forbidden transitions, in agreement with
the observation of MgO:V2+.
Finally, it should be noted that S varies over a wide range depending on the
spacial extension of the electrons. Approximating qi by acoustic and optical
modes in perfect lattice of typical ionic crystal, and assuming for the ground
and excited states the Is and 2p orbitals with radii r. and rP (> r,),
respectively, one can estimate the contribution to S of the two modes as
functions of orbital radii; the state with a radius closer to the lattice
constant makes a predominant contribution; the result is shown schematically in
fig. 32). It can be seen that the zero-phonon line and multiphonon structures
Fig. 3. Coupling strength S for acoustic and optical modes estimated for typical
ionic crystal, as functions of the orbital radius of localized electron,
d is the lattice constant.
— 345 —
are discernible only for (i) large (compared to lattice constant) radius
electrons or (ii) small radius electrons in the inner shell of the impurity
atom. As is seen from fig. 3. the longitudinal optical (LO) phonon predominates
in the multiphonon structures in case (i) since S0P > S,c. The well known
edge emissions in 11-VI compounds belong to this case. In case (ii) both the
modes make comparable contributions; the sideband in MgO:V2+ belongs to this
case. When (iii) the electron radius is comparable to the lattice constant,
S is as large as several tens, and one can expect a single broad absorption band
without phonon structures. There are many examples which belong to this case,
including the simple color centers in alkali halides. If the ground and excited
states have comparable radii, S can be small enough for the phonon structures
to be discernible even if each radius is comparable to lattice constant, because
appreciable cancellation takes place in (2). This situation seems to apply to
F-aggregate centers in alkali halides.
3. Difference in frequencies
We now examine the effect of Hel on the quadratic terms of the adiabatic
potentials. The contribution comes from the second order perturbation of the
1 inear interact ion (1):
I ‘A A ’ I A ’ AjS £ -------------------- q i q j - (8)
*■ 1 A ‘ ( * A ) E A - E A ’
and from the first order perturbation of quadratic interaction: (He<2>) A A.
They make additonal contribution to the local perturbation of dynamical matrix
mentioned in sec. 2. We can then transform to new q/ s such that for the
ground electronic state they are the normal coordinates for the corrected
potential, with their origins at the equilibrium configuration. The l -dependet
linear and quadratic terms caused by Hel remain for other electronic states.
— 346 —
Different electronic states have not only different equilibrium positions and
different frequencies, but also different principal axes of vibrations. It may
happen that localized or resonance mode appears only in the excited (or ground)
state. One can expect a general trend that (8) makes large negative
contribution to the lowest excited state which is closely followed by a host
of higher excited states. This may be the most reasonable explanation for the
empirical rule that vibrational frequency is usually smaller for excited states.
A modification of this situation will be mentioned in sec. 5.
Multiphonon structures are rather complicated. Confining ourselves to the one
phonon sideband, we have to use D. (w ) for the absorption spectra (co > 0)
and D, ( I co I ) for the emission spectra (co < 0), where D„ (a>) and D, (o>)
are related to the phonon spectra in the excited and ground states, respectively,
and are now different from each other. Not only the mirror image relation
between absorption and emission spectra breaks down, but also the relative
intensities of multiphonon components within each spectra deviate from the
Poisson distribution8).
The width of the zero-phonon line at finite temperature is caused by an
infinite number of infinitesimal differences in the vibrational frequencies
for the two electronic states. This is an adiabatic version of the so-called
Raman term9) for the width, as is easily confirmed.
4. Exciton motion in deformable lattice
In order to extend our study to the excitation of the host crystal, we must
include in H„ all the valence electrons so that any atom (or molecule) of the
crystal lattice can be excited on an equal footing. Moreover, H„ has
interatomic transfer energies, through which the excitation can propagate
through the crystal, forming an exciton band of total width 2b«2zv (z is the
number of nearest neighbors and v is the nearest neighbor transfer energy).
- 347-
Namely, the excitation can take advantage of propagating through the lattice
to lower its energy by b (see fig. 1).
Alternatively, the excited atom can distort the surrounding lattice without
propagating to neighboring atoms, lowering thereby the energy of the system by
e as was mentioned in sec. 2 (see fig. 1). Once this lattice relaxation takes
place, the resonance condition breaks down and the exciton will be localized
there. The exciton will prefer the band state without lattice distortion or
the self-trapped state with lattice distortion according as b^ e .
Of course, the self-trapped exciton should propagate from atom to atom
accompanied by the lattice distortion, because of the translational symmetry
of the whole electron lattice system. However, the transfer is now ve~*
(S is defined by (4) with average phonon energy hco). In order that the
center of lattice distortion is transferred from one atom to its neighbor, the
distortion A around the first atom should disappear while the same amount of
distortion must build up around the second atom. Each process contributes an
overlap integral e~,/2 as was mentioned in sec. 2. When S>1, the energy
lowering be-* due to propagation is negligible, and the exciton is practical ly
localized.
One may well ask if it is not possible to find a compromise between the two
ways of lowering energy, namely to find an optimum lattice distortion
xA (0< x< 1) such that the sum 5 E of the energy change caused by lattice
distortion and that caused by propagation is minimized. The answer is negative
since
<5 E = - b • exp(- Sx2) - ex2 (9)
is convex upward as a function of x2. Either the running exciton (x=0) or
the self-trapped exciton (x=l) is the stable state according as S is below
or above the boundary (solid line) in fig. 4. When b/h <y > 1, abrupt and
drastic increase of exciton effective mass by a factor of exp(b/hw)« exp(S)
takes place across this boundary10). At high temperatures, the self-trapped
- 348-
exciton will make hopping motion from atom to atom with an activation energy
of the order of e /2.
When b/M w and S are not large compared to unity, however, one can make no
clearcut distinction between the two types of states mentioned above, since in
this situation the lattice distortion A is not large compared to the amplitude
of zero-point vibration (h/<v)1/2. Detailed study for this case has been made
for the one-dimensional lattice11). Exciton motion in this situation may be
called “the intermediate type”, in contrast to the band type and the hopping
type which have clearcut distinction when S or b/fiw is large compared to unity.
self - trapped
intermediate
Fig. 4. Three types of exciton motion in deformable lattice which depend upon
the two parameters: S= e /ha> and b/ha>.
The above classification of exciton motion is closely related with the nature
of the emission spectra of exciton. In inorganic crystals, b/hro is usually
much larger than unity, and in fact one can classify the crystals distinctly
into two types, according as the relaxed state of exciton is the band state or
the self-trapped state. In the former case, the emission spectra consist of
a sharp resonance line and the optical phonon sidebands each of which replicates
the Maxwellian distribution of free excitons in the initial state. In the
349-
latter case, the emission spectra are similar to those of localized electrons
with large S (structureless broad band, with large Stokes shift), although the
absorption spectra may reflect the nature of free exciton except for the low
energy tail.
In organic molecular crystals, the situation b/hco<5 1 takes place very often,
and it is expected that the nature of exciton extends continuously from the
intermediate type to the self-trapping type (as is exemplified by the excimer).
Much remains to be done in this fertile area.
5. Phonon structures in exciton spectra
Most of the published studies on the line shape of exciton spectra start from
the band model of exciton, and then take into account the effect of phonons.
We will take here a different approach to the same problem, namely, we start
from localized excitation interacting with phonons, and then consider the effect
of energy transfer. This will enable us to relate the present problem with
that of localized excitation described in sec. 3 and 4. Another merit of this
approach is that it may be useful for the study of those molecular crystals in
which excitation transfer energy is as small as acoustic phonon energies.
Let us note that the multiphonon structures described in sec. 2 can also be
derived by higher order perturbation theory for the optical process in which
localized electron and phonons are excited simultaneously. In this approach,
the phonon energy to i( which appeared in the denominator of (2) comes in as
energy denominator for the intermediate state. If the excitation can transfer
from atom to atom, forming an exciton band with effective mass M and with its
bottom at k = 0, the exciton created optically with simultaneous emission of
a phonon with wave vector k should have recoil wave vector - k and kinetic
energy h2k2/2M. (Note that we use here the normal modes in perfect lattice
since there is no lattice imperfection in the ground electronic state of the
- 350-
crystal.) Then, the energy denominator for the intermediate state should be
taken as
h« k+ (ft2k2/2M) = hQ k (10)
instead of the phonon energy hco k alone. Then the coupling function (7) can be
written, for the exciton, as follows:
1 I 15.- 15. I 2fHco) = Z------------------------------------- <5 (co — Q k). (11)
k 2hw k Q k
— 15 g and I\ e represent the ho 1 e-phonon and electron-phonon interaction in
the non-transferable exciton state which has relative motion only. By changing
variable from Qk to <» k = <y * (Q k) through the relation (10), we get
£)( <y ) = D [ co * (co ) ] dco * {co) / dco [co*(co)/co] 2. (12)
Here 0(co) is the coupling function in the limit of v -► 0 (M -»• °°) which
corresponds to the localized excitation described in sec. 2. The functional
relationship between Qk and co k = co * (Q k) is shown schematically in fig. 5
for acoustic and optical modes.
As is easily seen from (12), the coupling strength defined by (6) would be
equal for the localized excitation and the transferable exciton but for the
factor [ ] 2 This factor has an effect of weakening the coupling strength,
more drastically for the acoustic mode than for the optical mode as is seen from
fig. 5. While the second moment / co 2£K(o)dco is equal to that of localized
excitation, the first moment / coDCco) dco is (co*(co)/co} times smaller than
that of localized excitation. This is a kind of motional narrowing.
The frequency shift co k in the one phonon process is modulated from time to time
with much higher frequency Q k, since the excitation transfers to a neighboring
atom with frequency Qk before the lattice vibrates one cycle
-351-
0 k
Fig. 5. Energies of (exciton)+ (one phonon) state as functions of k.
with frequency co k. The narrowing factor in such a situation is given by
co k/Q k as is well known.
For the acoustic branch, we insert co k = sk (s is the sound velocity) in (10)
and get co k = co * (Q k) = 2 (1 + i/1+(Q k/co ,)2) 1 Q k with
hco . = %Ms2.
0. c (CO) given by (12) is shown schematically in fig. 6, in comparison with
the corresponding D, c (co ) for localized excitation. While D, c (co ) rises
linearly with co , D, c reaches its maximum quite soon, at hco ss hco ,12). This
separation between the acoustic phonon side peak and the zero-phonon line is on
the order of 10-4 eV (one hundredth of the value for localized excitation) for
typical inorganic crystal. The ratio Sac/Sac is on the order of (4co ,/co m)2
[ In (co m/4co ,) - 2] where co m is the maximum point of D. c (co ). It is usually
less than 10~2.
On the other hand, the strength of the two phonon sideband is not given by
14S,c because the system is not harmonic due to the exc i ton recoil energy.
352-
In fact, it is much larger, even than S,c itself, being on the order of
(4<y ,/<y m)S,c. Assuming that the radius of the heavier particle (hole, in most
cases) in the exciton internal motion is on the order of interatomic distance,
we can read S,c« 20 in fig. 3, and therefore, we expect that the two phonon
Coupling function D(a)) for exc i ton (solid line) are compared
schematically with the corresponding coupling function D() for
localized excitation (dotted line). For shallow excitons, the exciton-
phonon bound state may be squeezed out from the optical branch of D(oj)
(broken line).
sideband of exciton spectra has intensity comparable to the zero-phonon line.
In this way, the multiphonon structures in exciton spectra are completely
different from those of localized excitation as far as acoustic branch is
concerned, except for those molecular crystals with transfer energy as small as
average acoustic phonon energy. (Exciton spectra of such crystals may retain,
to some extent, the features of the acoustic phonon structures described in sec.
2.) Except at very low temperature, the acoustic phonon structures are not
important in exciton spectra, and in most cases, the overall line shapes have
been analysed without decomposing them into multiphonon structures.
- 353-
The difference between the multiphonon structures of localized excitation
and those of intrinsic exciton is less drastic for the optical branch as was
mentioned above. In fact, the optical spectra calculated for the one dimensional
lattice show clearly the structures due to optical phonons13). Assuming small
electron-hole effective mass ratio, we can estimate from (10) and (12) that
where rh is the orbital radius of the hole in the
exciton and h<y 0 is the L0 phonon energy (k-dependence is neglected). The ratio
is on the order of one tenth, being much larger than in the case of acoustic
branch.
The L0 phonon sideband in exciton spectra has been observed in a number of
ionic crystals. In all cases, the intensity ratio of the sideband to the zero-
phonon line is in fact an order of magnitude smaller than the value (for
localized excitation) read from fig. 3, in agreement with the above estimation.
According to (11) and fig. 5, the L0 phonon s i deband £> 0 p () should start at
a) — a> o, extending towards the higher energy side as is shown schematically in
fig. 6. This is the case for alkali halides which have deep excitons. However,
in a number of ionic crystals with shallow exciton, the L0 phonon sideband has
been observed at energy lower than the threshold, namely at (1 - A) <w „ where A
is on the order of ten per cent. These sidebands have been ascribed to the
bound14) or quasi-bound state15) of an exciton and an L0 phonon (EPBS or EPQBS).
Note that (10) represents the energy of a non-interacting pair of an LO phonon
and an exciton (measured from the energy of k= 0 exc i ton) which have been
created simultaneously by an incident photon. However, there should be final
state interaction between them which, if large enough, may give rise to a bound
state below the continuum hQk of relative motion, with binding energy
corresponding to the oberved hcu „ A (see fig. 6). The situation is similar to
the exciton spectrum itself, which has branched off from the continuum of a free
pair of an electron and a hole as the result of Coulomb attraction.
In the present case, the attractive force is ascribed to the phonon-induced
- 354-
virtual transitions among internal states of the exciton. This corresponds to
the second order effect described in sec. 3 (see (8)). Since we are concerned
with the relative motion of the LO phonon and the exciton, the discrete mode
squeezed out below o)„ by the second order effect should be localized not to
the fixed lattice but to the moving exciton. It should be noted that the second
order effect should be larger for shallower excitons because of the energy
denominator. This is consistent with the fact that the bound state appears
only for shallow excitons.
That the final state interaction is essential for the phonon energy shift is
also consistent with the observations that the LO phonon energy shows no shift
in the emission spectra of exciton. Multiphonon sidebands replicate the
Maxwellian distribution of excitons in the initial state, but the lower energy
threshold of each sideband is at an integral multiple of LO phonon energy
(measured downward) from the resonance emission line, and the line shape is in
good agreement with perturbation calculation*.
In the case of molecular crystals, the (optical) phonon energy difference
between the absorption and emission spectra is straight-forwardly related with
the difference in the intramolecular vibrational frequencies of excited and
ground states, while the concept of exciton-phonon bound state may be somewhat
redundant. However, the underlying mechanism is essentially the same for
organic and inorganic crystals.
* See ref.16) where the references to experimental works on 11-VI compounds are also found. As for cuprous halides, see ref.17).
- 355-
References
1) D.B. Fitchen, Physics of color Centers (Academic, New York and London, 1968)
p.293.
2) Y. Toyozawa, Dynamical Processes in Solid State Optics (Syokabo, Tokyo and
W. A. Benjamin, New York, 1967) p. 90.
3) H. Sumi, to be published.
4) G. Baumann, F. Lanzl, W. Von der Osten and W. Waidelich, J. de Phys.
supplement 28 (1967) C4-72.
5) G. F. Imbusch, W. M. Yen, A. L. Shawlaw, D. E. McCumber and M. D. Sturge, Phys.
Rev. 133 (1964) A1029.
6) M. Wagner and W. E. Bron, Phys. Rev. 139 (1965) A223.
7) A.A. Maradudin, Solid State Physics 18 (Academic, New York and London, 1966)
p. 273.
8) T. Miyakawa and S. Oyama, Phys. Letters 28A (1968) 206.
9) D. E. McCumber and M. D. Sturge, J. App 1. Phys. 34 (1963) 1682.
10) Y. Toyozawa, Polarons and Excitons (Oliver and Boyd, Edinburgh and London,
1962) p.211.
11) R. E. Merrif ield, J. Chem. Phys. 40 (1964) 445.
12) K. K. Rebane, V. G. Fedoseyev and V. V. Hizhnyakov, in Proc. of the 9-th Int.
Conf. on Semiconductors (Nauka, Leningrad, 1968) p.430.
13) A. Suna, Phys. Rev. 135 (1964) Alll.
14) Y. Toyozawa and J. Hermanson, Phys. Rev. Letters 21 (1968) 1637.
15) Y. Toyozawa, to be published in Proc. of the Third Int. Conf. on
Photoconductivity: a supplement to Int. J. Phys. Chem. Solids.
16) B. Sega 11 and G. D. Mahan, Phys. Rev. 171 (1968) 935.
17) T. Goto, T. Takahashi and M. Ueta, J. Phys. Soc. Japan, 24 (1968) 314.
- 356-
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- 363-
Spectrally Programmed Stimulated Photon Echo
Masahaur Mitsunaga, Ryrzi Yano, and Naoshi Uesugi
NTT Basic Research Laboratories, Musashino-shi, Tokyo 180, Japan
ABSTRACT : A stimulated photon echo has been observed from the artificially
modulated inhomogeneous distribution of a medium. A cryogenic Eu3+:YA103 sample
with a quasipersistent hole lifetime is exposed to a frequency-scanned and
intensity-modulated cw laser for multiple holeburning. A coherent burst
equivalent to the stimulated photon echo is obtained by triggering this sample
by a pulsed laser. We further demonstrate that any desired transient pu1seshape
can, in principle, be obtained by appropriate frequency-domain programming,
opening the way to a novel type of optical memory.
-364
The stimulated, or three-pulse, photon echo (SPE),1-3 although it has been
known for a long time, is the object of renewed attention mainly because of its
potential use as time-domain optical memory. 4-6 To review the phenomenon, a pair
of optical pulses, the first pulse and the second pulse, separated by time r
creates a periodically modulated inhomogeneous distribution of period 1/r by
temporal interference of the two pulses. This modified frequency distribution of
radiators persists for a time T,tor.,„ until the medium reaches back to its
thermal equilibrium. This storage time T,tor»«e ranges from ms to hours for
typical rare-earth-ion-doped crystals and is often determined by the hyperfine
sublevel lifetime of the ground state. If a third pulse, or read pulse, excites
the whole spectrum of radiators within T,t„r.«SPE is observed as a coherent
burst of emission at z after the read pulse. This emission can be regarded as
a temporal interference of radiators.
Although this process is well understood and is taken as a matter of course,
the above explanation itself indicates that the first pulse and the second pulse
are not absolutely necessary for observation of an SPE: the only essential
requirement is a sinusoidally-modulated frequency distribution of radiators. We
report here for the first time on SPEs without applying the first and the second
pulses, instead by preparing the sample in an equivalent situation to that of
the conventional SPE by periodic hole-burning using a single frequency laser.
We call this a spectrally programmed stimulated photon echo (SPSPE). Furthermore,
we demonstrate that in principle any arbitrary temporal pulseshape can be
obtained after the read pulse by appropriate preparation of the sample in the
frequency domain.
The SPSPE is also important from the viewpoint of applied optics. So far there
are two basic kinds of frequency-selective optical memory. One method is hole
burning memory7 (persistent or non-persistent), where information is stored and
recalled in the frequency domain. The other is the stimulated photon echo
memory4-6, where time-domain optical data is stored and recalled. In the latter
- 365-
case information is stored in the frequency domain as the Fourier transform of
the input temporal data. Although these two techniques stem from the same
mechanism and have lots of advantages and disadvantages in common, they have
been developed rather independently. This SPSPE bridges tha gap between the two
and offers a new type of memory, i. e., with frequency-domain data storage ari
time-domain data retrieval. 8
Here we present a simple theoretical approach. For simplicity we neglect the
saturation effect so that hole-depth is proportional to burn-laser intensity.
If the burn-laser is frequency-scanned and intensity-modulated within a time
much shorter than T,tor.,e, the intensity spectrum I (co B) of the burn-laser
represents the input data applied to the medium. In tnis case the population
difference co at frequency co of the medium is given by the superposition of
all the hole-burning spectra:
co ( oo ) dcoBl(coB)h(co, co b) . (1)
where h(co, oo B) is the population spectrum caused by the burn-laser at oo B and
is a Lorentzian for a simple tow-level system. If the system has some hyperfine
structures, h (co, oo B) becomes very complicated as shown later and may be
obtained experimentally. If a pulse is applied at t=0 after this frequency-
domain preparation, this population distribution is connverted to the dipole
distribution and the dipoles start to precess freely. The signal amplitude S(t)
is then given by averaging the dipoles over the original inhomogeneous
distribution G(co) of the medium:
S(t) = dcodcoBl(coB)G(co)h(co, oo B) exp (i co t — t/T2). (2)
where T2 is the homogeneous dephasing time. This will give the transient
response for arbitrary frequency-domain programming. The simplest case is easily
-366
deduced for the hole spectrum expressed by a delta function (h(co, u> B) = 6 (co
- <y b)), the long dephasing time (T2 and the broad inhomogeneous
broadening (G( w) =1). In this ideal case Eq. (2) is reduced to the exact
Fourier transform of the input data I (to B). Specifically, a SPE emission can
expected when I (to B) is sinusoidally modulated.
The most appropriate sample to this end presently seems to be Eu3+ ions doped
in crystals. This sample shows a quasi-permanent hole-recovery time
(~ hours)9, 10 that allows enough working time for frequency-domain programming.
It also exhibits a ultranarrow homogeneous line-width (—kHz)11 • 12, or u1tralong
T2, that enables real-time measurement of coherent transients in the nano-to-
microsecond region. We examined the 7F0-5Do transition (581.68nm) of 0.1-at.X
Eu3+:YAlOs at liquid He temperature. In Fig. 1 the experimental setup for
ovserving SPSPE is illustrated. The experiment is divided into two stages ; a
writing (burning) period in the frequency domain, and a reading period in the
time and frequency domain. During the writing period, the path A in Fig. 1 is
open while B, C, and D are blocked. To realize periodic hole-burning, a single
frequency cw ring dye laser of about 20 mW is frequency-scanned around the
absorption line peak while its intensity is modulated by an acousto-optic
modulator (AOM). Thereafter, the hole spectrum can be obtained by scanning the
attenuated and unmodulated cw dye laser and monitoring the transmitted laser
intensity by unblocking C. To observe a transient response of the medium, A and
C are blocked with B and D unblocked. The same spot is hit in a col 1 inear
configuration by a 10-Hz-repetit ion pulsed dye laser of 5-ns pulse width and
6-GHz spectral width with the same wavelength as the cw laser. That signal
transmits through an AOM shutter that opens after the excitation pulse and it is
detected by a photomultiplier. The temporal signal is thus fed into a digitizing
osci1 loscape and finally stored in a computer.
In a preliminary experiment, a single hole was burned and its transient
response investigated.13 With the cw laser frequency fixed, the burn time was
- 367-
0.5 second. The hole apectrum shown in the inset of Fig. 2, with the sharp main
hole at the center and several side-holes and anti-holes symmetrically in both
sides reflecting the hyperfine level structures, is characteristic of the Eu
ion14. The transient signal after the read pulse is shown by the lower trace of
Fig. 2. The upper trace is a numerical Fourier transform of the hole spectrum.
The effect of the finite read-pulse-width has been taken into account when
calculating the upper trace. The tow traces give a satisfactory agreement
indicating that the transient response is indeed a Fourier transform of the
structure impressed in the frequency domain. The reason why the numerical curve
decays faster than the experimental curve can be understood as follows: the hole
spectrum given in the inset is considered as a convolution of real hole
structure and the finite spectral width of the probe laser. Therefore, the real
hole-width should be narrower than the one in the inset and should give a slower
transient decay. It should be noted that the intrinsic hole-width is several kHz.
This means that, with decreasing laser linewidth, the transient response should
last much longer.
Next, we scanned the cw laser frequency while modulating its intensity. The
frequency scan width is given as A f and the scan time as T,c.n. Laser
intensity was synchronously modulated with a frequency fmod. This prepared a
periodic holeburning structure of fmodT.cn periods in the frequency range of
Af, providing the frequency period f „ e r = A f/(fmodT,c.n). With this
preparation, SPE should be expected at a time 1/f P.r after the read pulse.
Typical values were: A f~300 MHz, T.c.n~l second, and fmOd~30 Hz, giving
fPer =10 MHz. In Fig. 3 the hole-burning spectrum (inset) and the transient
signal for this case are shown. After the read pulse, a sharp SPE emission is
observed at time~100 ns, which is equal to the inverse of fPer. This signal was
very stable fom shot to shot and the signal size was even bigger than ordinary
SPEs we had seen in the same sample. The signal sround t =190 ns is the higer-
order component of this frequency grating and is due to the imperfect (non-
- 368-
sinusoidal) modulation. In fact, in later experiments we noticed that by
increasing A f and fmod with fP„r fixed, a nicer single pulse without the
harmonics component could be obtained (Fig.4).
Finally, we investigated the SPSPE of multiple-bit data by overwriting several
periodic patterns in the inhomogeneous spectrum and afterwards applying a read
pulse. Fig. 4 shows the transient waveform from the medium representing an 8-bit
ASCII coded character N(01001110). The experimental conditions were: A f = 1
GHz, T,can = 280 ms, and each bit was stored successively by changing the
modulation frequency fmod as 240, 480, 560 and 640 Hz. It should be noted that
the number of bits that can be stored is currently limited by our poor laser-
spectral-width. If it becomes comparable to the homogeneous line-width, finer
holebruning sructure should be expected. The ultimate storage density is given
in principle by the inhomogeneous-to-homogeneous 1inewidth ratio, which should
amount to ~ 105 for this sample.
This Letter proposes and demonstrates a novel type of optical memory, or
optical pulse generation. The desired pu 1 seshape can be obtained by first
burning, in the inhomogeneous line of a medium, a hole whose shape is the
Fourier transform of the output data and then by triggering it with a pulsed
laser. This may be regarded as an all-optical function generator working in the
nano-to-microsecond region with less than 100 zz m spot size. Finally we emphasize
that in this way the phase of the pulsed signal is well under control. For
example, erasuure of an SPSPE can be easily achieved by overwriting the
frequency grating with the same period and amplitude but phase-shifted by 180
degrees.
- 369-
REFERENCES
1. See, for example, R. M. Macfar lane and R. M. Shelby, in Spectroscopy of Solids
Containing Rare Earth Ions, edited by A. A. Kaplyanskii and R.M. Macfarlane
(North-Ho11 and, Amsterdam, 1987).
2. Y. C. Chen, K. Chiang, and S. R. Hartmann, Opt. Common. 29, 181 (1979).
3. J. B. Mors ink and D. A. Wiersma, Chem. Phys. Lett. 65, 105 (1979).
4. T. W. Mossberg, Opt, Lett. 7, 77 (1982); N. W. Carlson, Y. S. Bai, W. R. Babbitt,
and T. W. Mossberg, Phys. Rev. A30, 1572 (1984).; W. R. Babbitt, Y. S. Bai, an
T.W. Mossberg, Proc. Soc. Photo-Opt. Instrum, Engr. 639 , 240 (1986).
5. P. Saari, R. Kaarli, and A. Rebane, J. Opt. Soc. Am. B3, 527 (1986);
A. Rebane, J. Aaviksoo, and J. Kuhl, Appl. Phys. Lett. 54, 93 (1989).
6. M. Mitsunage, K. Kubodera, and H. Kanbe, Opt. Lett. 1 1, 339 (1986);
M. Mitsunaga, M. K. Kim, E. Xu, and R. Kachru, Phys. Rev. Lett. 63, 754 (1989).
7. Persistent Spectral Hole-Burning: Science and Applications, Topics in
Current Physics 44, Editor W. E. Moerner, Springer Verlag. 1988.
8. Frequency-domain retrieval of time-domain data (pulse train) was reported:
A. Rebane, R. Kaarli, P. Saari, A. Anijalg, and K. Timpmann, Opt. Common.
47, 173 (1983): A. K. Rebane, R. K. Kaarli, and P. M. Saar i, JETP Lett.
38, 383 (1983).
9. M. K. Kim and R. Kachru, Opt. Lett. 14, 423 (1989).
10. M. Mi tsunaga and N. Uesugi, Opt. Lett. 15, 195 (1990).
11. R. M. Shelby and R. M. Macfar lane, Phys. Rev. Lett. 45, 1098 (1980).
12. R. M. Macfar lane and R. M. Shelby, Opt. Common. 39, 169 (1981).
13. The transient response from an optical hole was reported in Ruby:
S. Nakanishi, 0. Tamura, T. Muramoto, and T. Hashi, Opt. Common.
31, 344 (1979); T. Muramoto, S. Nakanishi, and T. Hashi, Opt. Common.
24, 316 (1978).
14. R. M. Shelby and R. M. Macfar lane, Phys. Rev. Lett. 47, 1172 (1981).
- 370-
FIGURE CAPTIONS
Fig. 1. Schematic of the experiment. Key: AOM, acousto-optic modulator; PMT,
photomultiplier tube.
Fig. 2. Single hole-burning spectrum for the 7F0-5D0 transition of Eu3+:YA103
(inset) and its transient response signal after the read pulse (lower
trace). The upper trace is the numerical Fourier transform of the hole
spectrum.
Fig. 3. Periodic hole-burning spectrum (inset) and its transient response signal
after the read pulse, mimicking the stimulated photon echo.
Fig. 4. Transient response signal following the read pulse when the sample was
spectrally programmed beforehand in such a way to show the ACSII-coded
time-domain optical data “N” (01001110).
371-
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- 373-
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Lehrstuhl fur Experimentalphysik IV Universitat Bayreuth,
Postfach 101251, D-8580 Bayreuth, FRG
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Prof. J. Friedrich
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Institute of Quantum Electronics, Nonlinear Optics
Laboratory, ETH-Honggerberg
Prof. P. Gunter
ETH-Zentrum IfrPnJ
Laboratoriurn fur Physikal ische Chemie Universitatsstrasse
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* Multiphoton Processes In Atoms And Molecules And their Applications.
V. S. Letokhov
Institute of Spectroscopy, USSR Academy Science
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9 . 21 (A) Dr. Bernhard Dick
Max-Planck-Institut fur Biophysikalische Chemie
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Am Fassberg, D3400 Gottingen-Nikolausborg, FRG
Phone 0551-1-216 Fax 0551-2-1468
9. 24 (>9 ) Prof. Dr. D. Haarer
Lahrstuhl fur EXperimentalphysik IV
Universitat bayreuth, Postfach 101251, D-8580 Bayreuth
Federal Republic of Germany
Phone 0921-55-3240 (Seer. 3241) Fax 0921-55-3250
380
9. 25 (*) Prof. Dr. J. Friedrich
Institut fur Physika1ische Chemie, Universitat Mainz,
Welder Weg 11, D6500 Mainz, Federal Republic of Germany
Phone 06131-39-4212 Fax 06131-39-3768
9 . 27 (^) Prof. Dr. P. Gunter
Institute of Quantum Electronics, Nonlinear Optics
Laboratory, ETH-Honggerberg, HPF,
CH-8093 Zurich, Switzerland
Phone 01-377-2290, 4411 Fax 01-371-5989
9 . 28 (A) Prof. Dr. Urs P. Wild
Laboratorium fur Physika1 ische Chemie,
Universitatsstrasse 22, ETH-Zentrum, CH-8092 Zurich
Switzerland
Phone 01-256-4381 Fax 01-251-3402
10. 1 ) Prof. Dr. S. Volker
Rijksuniversiteit te Leiden, Faculteit der Wiskunde en
Natuurwetenschappen, Huygens Laboratoriurn,
Neils Bohrweg 2, 2333 CA Leiden, The Netherlands
Phone 71-275907, (Seer. 275910) Fax 71-275819
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FIG. 2. Permanent broadening of a spectral hole after application of a high electric field and subsequent narrowing by a moderate field of opposite sign. The hole was burnt at a wavelength of629.3 nm; the irradiated laser intensity and light dose (energy per unit area) were 27 /zW/cm2 and 13 mJ/cm2, respectively, (a) Initial hole spectrum before applying a polarizing field;(b) after applying + 171 kV/cm for about 5 min and subsequent shorting of the electrodes; (c) during application of — 8.6 kV/cm; (d) after recording trace (c) and reconnecting the electrodes again. The traces (a), (b),(c) , and (d) correspond to the scans 1,2,5, and 6, respectively, as depicted in Fig. 3; scans 3 and 4 are not shown.
average exptt. error
♦171 4-171
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FIG. 3. Histogram giving an overview of the various measured hole widths as a functiop of the various field conditions. Full squares: scans taken immediately after applying + 171 kV/cm (scan 20: — 171 kV/cm) for about 5 min and shorting the electrodes (plus repetitive runs). Full triangles: scans taken during the application of a moderate field of opposite sign. The numbers denote the field strengths in kV/cm. Empty circles: scans taken after application of a “depolarizing" field in opposite direction and after shorting the electrodes (plus repetitive runs).
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T[K]FIG. 5. Extrapolated hole width as a function of temperature. The fit is a superposition of two exponentials according to y= yn +ate~m,/kr + a2e~mi-/kr with parameters fifl, = 27 cm'1, AO, = 300 cm'1, o, = 2.85, a2 = 3000. Note, that the extrapolated hole width is twice the homogeneous linewidth.
FIG. 6. Schematic representation of scattering of acoustic (trace 2) and optical phonons (traces 3 and 4) off the K = 0 state of a linear exciton [dispersion curve: E(k) = E„ — 2(3 cos ka, see trace 1 J. /? is the coupling matrix element between monomers, a is the repetition unit of the aggregate chain.
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ETH (Honngerberg) Tr x Institute of Quantum Electronics^ afrfnl L tz0
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Fig. I. (a) Self-induced photorefractive ring resonator; Ml, M2, M3, and M4 are mirrors; BS is a beam splitter to couple out the oscillating beam from the cavity ; the amplification is provided by two-wave mixing in the photorefractive crystal, (b) Self-induced photorefractive linear resonator; Ml and M2 are two parallel mirrors; the amplification is provided by two-wave mixing in the photorefractive crystal: only the light traveling toward the left-hand side of the drawing is amplified.
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2- (l, 2-dimethyl-3-indolyl) etheno (l)fc =k CM, 2-dicyano-l-(benzo(b) thiophen-
3- yl) -2-(l,2-dimethy-3-indolyl) ethene (2)^^5%L/:o
8% 7K K ID =k (9 ##7.k#^ 2-C2, 3, 5-trimethyl-3-thienyl)-3-(l,2-dimethyl-3-
indolyl) maleic anhydride (3)&«fc C52-(benzo(b)-thiophen-3-yl)-3-(l, 2-dimethyl
-3-indolyl) maleic anhydride(4)~^#Lf:o (3)©^M#l:«k5BiRx/<^ h7l/^
- 403-
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5. 3t to
1) S. Kawauchi, H.Yoshida, N. Yamashina, M.Ohira, S. Saeda. M. Irie
A new photochromic spiro (3H-1, 4-oxazine)
Bull. Chem. Sec., Jpn, 63, 267 (1990)
2) K.Uchida, Y. Nakayama, M. Irie
Thermally irreversible photochromic systems. Reversible photocyc 1 i zat ion
of 1,2-bit (benzo(b)thiophen-3-y1)ethene derivatives
Bull. Chem. Soc., Jpn. 63, 1311 (1990)
3) Y. Nakayama, K. Hayashi, M. Irie
- 406-
Thermally irreversible photochromic systems. Reversible photocyclization
of 1, 2-diselenenylethene and 1,2-diindolylehene derivatives
J. Org. Chem., 55, 2592 (1990)
4) Y. Nakayama, K. Hayashi, M. Irie
Thermally irreversible photochromic systems. Photoreaction of diary-
lethene derivatives with imidazo(1, 2-a) pyridine rings.
Bull. Chem. Soc., Jpn, 64, 202 (1991)
5) Y. Nakayama, K. Hayashi, M. Irie
hermally irreversible photochromic systems. Reversible photocyclization
of non-symmetric diarylethen derivatives.
Bull. Chem. Soc., Jpn, 64, 789 (1991)
407-
1 C NliAi: «k ? h Jl&it
x y z w
Calculated Experimental
max / nm.,(Oscillator Strength) A max/nm
1b CN H II II 369(0.74), 313(0.00), 305(0.02,, 486
205(0.01 ), 272(0.17)
2b II CN II II 376(0.75), 308(0.04), 303(0.02), 508
203(0.27), 269(0.59)
3b II II CN H 305(0.92), 307(0.10), 300(0.03) , 530
291(0.25), 273(6.34)
4b II II II CN 374(0.75), 310(0.*05), 305(0.005), 505
202(0.14), 266(0.45), 251(0.24),
247(0.13)
5b II II II II 374(0.72), 301(0.12), 296(0.02), 507
204(0.23), 268(0.40)
^ 2 2, 3 —Di (2,4, 5- trimethy1-3-thiemrl) maleic anhydr ide® ® JR x A ^ KfG
AP4X#, ^ h 71/>
A max(nm)Solvent 1a 1b
Quantum Yield3, ^ 1a1 a-^ 1 b 1b—x 1 a X max (nm) ^ ^
Hexane 331 552 0.13 0.16 488 1 .0Benzene 340 564 0.07 0.12 541 0.35THF 335 560 0.04 0.11 560 0.088ch3cn 336 563 0.003 0.10 — <0.01
a) 1 a~* 1b:Irradiation with 405nm-light.1b-A1a:Irradiation with 546nm-light.
b) Fluorescence maxima, excitation wavelength:405nm.c) Relative fluorescence quantum yield, excitation wavelength:405nm.
- 408-
m 3 i?T V
CompelRepeatable Cyo1o Number
d_ n a_ d_ rr under vacuum
Me Me
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12 0
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3 - *7 3C
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1 O
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0 1 2-(2, 3, 5-1rime thy 1-3-thienyl)-3-(l,2-dime thy 1-3-indolyl) ethene
CD 7 * h ? a ; v ^ KfG
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— 446 —
2
Delay Time T]2 (psec)IE 1 Echo decay curve of HITC:PVA excited by the diode laser at 10K.
The excitation wavelength is 786nm.
ziCD
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Delay Time T12 (psec)
IE 2 Echo decay curve of DDC-4:PVAc at 6K excited by the SLD.
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m 3
(a)Diode
LaserFPI }----- ( PD3
Sample
AOMDriver
Func. PulserGene.
Computer
(a) AOMdiff. eff.
BurnProbe
(b) injectioncurrent
(c) wavelength
(a) Schematic diagram of the experiment. AOM is an acousto-optic modulator and FPI is a Fabry-Perot interferometer. (b) Timing charts of bum and probe, (a), (b) and (c) in (b) show diffraction efficiency of the AOM, injection current of the laser diode and wavelength of the diode laser, respectively.
^ 4
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0.4 -c
° Hole Depth • Hole Width
Burn Duration (sec)
Hole-depth and hole-width dependences on the bum duration.
- 449-
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£^ 0.2x
10~8 10“2 10_1 10° 101 102 103 Time Separation (sec)
Hole width dependence on the time separation between burn and probe,
circles were obtained by current sweep of a diode laser, and the open
obtained by nanosecond pulse incoherent light photon echoes.
«• 1 I.
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Time Separation (sec)
Hole depth dependence on the time separation between burn and probe.
L
104
The closed
circle was
— 450 —
rhom
(cm™
1)0 7
• HOLE BURNING
O PHOTON ECHO (CW )
X PHOTON ECHO (PULSE)
0.052 5 10 20 50
Temperature (K)
Log-log plotted temperature dependence of the homogeneous width horn of HITCtPVA.
The solid line represents T 1.3 temperature dependence.
-451-
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Wave Number (cm~1)
Multiple probing of a single hole by current sweep of a diode laser.
0 0 L10
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Erasing Time (sec)
L40
Hole-depth dependence on the erasing time by the irradiation of a light emitting diode.
-452
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6. 3t E
1) R. Yano, S. Uemtira, H. Nakatsuka, and M. Okada, “Superluminescent Diode
Excitation of Femtosecond Accumulated Photon Echoes” to be published in
JOSA B,
2) H. Nakatsuka, K. Inouye, S. Uemura, and R. Yano, “Observation of the Time
Evolution of Persistent Holes in an Organic Amorphous System using a
Diode Laser” Chem. Phys. Lett., 171 (1990) 245.
3) S. Sadao, H. Nakatsuka, K. M. Abed in, and M. Okada, “Dynamics of Persistent
Hole Burning in Organic Glasses and its Fractal Interpretation” to be
pub 1 i shed.
4) H.Nakatsuka, D.Masuoka, and T.Yamamoto, “Optical Phase Conjugation in
Cooled Dye Film” Opt. Commun., 80 (1990) 215.
5) H. Nakatsuka, D. Masuoka, T. Yamamoto, S. Uemura, and R. Yano, “Optical Phase
Conjugation using a Diode Laser in a Cooled Organic Dye Film” to be pub 1
ished in Nool. Opt.
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1) Optical Ramsey fringes in photochemical hole burning.
S. Saikan, A. Imaoka and T. Kishida : Phys. Rev. B39 (1989) 11207.
2) Improved time resolution in an accumulated photon echo by using a
repetitively frequency scanned dye laser.
S. Saikan, T. Kishida and A. Imaoka : J. Opt. Soc. Am. B6 (1989) 1579.
3) Linear electron-phonon interaction in dye-doped polymers.
S. Saikan, A. Imaoka, Y. Kanematsu and T. Kishida
Chem. Phys. Lett. 162 (1989) 217.
4) Time dependence of hole spectrum due to dispersive burning kinetics in
dye-doped polymers.
Y.Kanematsu, R.Shiraishi, S.Saikan and T.Kushida
J. Chem. Phys, 91 (19.89) 6579.
5) Optical memory based on heterodyne detected accumulated photon echo.
S. Saikan, K. Uchidawa and H. Ohsawa : Opt. Lett. 14 (1989) 841.
6) Femtosecond optical memory with an incoherent light source.
K. Uchikawa, H. Ohsawa and S. Saikan : Jpn. J. App 1. Phys. 28 (1989) 841.
7) Polymer dependence of boson peak frequency studied by hole burning and
Raman spectroscopies.
S. Saikan, T. Kishida, Y. Kanematsu, H. Aota, A.Harada and M. Kamachi.
Chem. Phys. Lett. 166 (1990) 358.
8) Temperature dependence of Debye-Waller factor in dye-doped polymers.
S. Saikan, A. Imaoka, Y. Kanematsu, K. Sakoda, K. Kominami and M. Iwamoto.
Phys. Rev. b41 (1990) 3185.
9) Fluorescence detection of femtosecond accumelated photon echo.
K. Uchikawa, H. Ohsawa, T. Suga, A. Furusawa and S. Saikan.
Ultrafast phenomena VR p.145.
10) Linear electron-phonon interaction in dye-doped polymers studied by
- 468-
femtosecond accumulated photon echo.
S.Saikan : Ultrafast phenomena VE p.453.
11) Phase modulation technique for accumelated photon echo.
S. Saikan, K. Uchikawa and H. Ohsawa : Opt. Lett. 16 (1991) 10.
12) Fluorescence detection of femtosecond accumulated photon echo.
K. U chikawa, H. Ohsawa, T. Suga and S. Saikan.
Opt. Lett. 16 (1991) 13.
13) Extremely weak linear electron-phonon coupling in protonated
chromoproteins studied by phase modulated photon echo.
J.W-I.Lin, T.Tada, S. Saikan and T. Tani : submitted to Phys. Rev. B.
— 469 —
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