# Stimulated Raman Adiabatic Passage in a Dense Medium

Authors: B. D. Fainberg; B. Levinsky
Journal: Advances in Physical Chemistry
 (2010)

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## Abstract

We have considered a coherent population transfer to a higher excited singlet state (S2) of
molecules with anomalous fluorescence in molecular assemblies (e.g., a dense medium). A direct
excitation to S2 requires light in the UV region. Because of this, the transition is conveniently realized by a two-step (two-photon) process: S0→S1→S2, where transitions S0→S1 and S1→S2 correspond to the optical region. We have shown that efficient stimulated Raman adiabatic passage
(STIRAP) in the ladder configuration can be realized in this case, using suitably chirped pulses, to
compensate a change of the two-photon transition frequency in time, induced by the pulses themselves, due to near dipole-dipole interactions. We have provided a reduced state formulation of the
optical control process. Chirping the “pump” pulse that excites transition S0→S1 is nonequivalent to chirping the “Stokes” pulse that excites transition S1→S2, with respect to the population of the intermediate state (S1) in the pulse nonadiabatic regime. We have also shown that with suitably chirped pulses, efficient STIRAP still persists even for a rather large decay of the intermediate state.


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## Body

## 1. Introduction

Population transfer to a higher singlet stateSn (n>1) of complex organic molecules makes no sense, since more often than not Sn (n>1) rapidly relaxes back to the first excited singlet S1 [1–4], though excited-state absorption S1→Sn (n>1) has a profound effect on coherent population transfer S0→S1 with shaped laser pulses [5]. The situation reverses for molecules with anomalous fluorescence like azulene, the molecule known as the textbook exception to Kasha's rule [6], and its derivatives. For such molecules, the first excited singlet state S1 is very short lived (~1 ps) due to a conical intersection [7] and, as a consequence, a strong nonradiative decay of the transition S1→S0. However, a higher excited singlet state S2 is long lived (~1 ns) displaying a strong fluorescence band that corresponds to transition S2→S0 [8–11]. Because of this, there are also reasons to consider a coherent population transfer to higher excited singlet states (S2) of the molecules under discussion. However, a direct excitation to a higher electronic state S0→S2 requires light in the UV region where pulse shaping presents difficulties. Because of this, a coherent population transfer to S2 is conveniently realized by a two-step (two-photon) process, S0→S1→S2 where transitions S0→S1 and S1→S2 correspond to the optical region. Due to the absence of the center of symmetry in azulene (belongs to the Cs point group) and its derivatives, all three transitions S0→S2, S0→S1 and S1→S2 are allowed. In this regard, using stimulated Raman adiabatic passage (STIRAP) [12–16] in the ladder configuration for the population transfer from S0 to S2 seems rather attractive. Indeed, STIRAP is a simple and powerful technique for complete and robust population transfer in three-state quantum systems. Using this technique, the population is transferred adiabatically from an initially populated state |1〉 (S0) to a target state |3〉 (S2), which are coupled via an intermediate state |2〉 (S1) by two pulsed fields. A unique and very useful feature of STIRAP is that the intermediate state, whose presence is crucial for providing two strongly coupled single-photon transitions, never gets populated, not even transiently. The reason is that throughout the adiabatic evolution of the system, the population remains trapped in an adiabatic dark state, which is a superposition of states |1〉 and |3〉 only and does not involve the intermediate state |2〉 that can be a strongly decaying state (S1). Such a dark state is formed by maintaining a two-photon resonance between the target |3〉 and initial |1〉 states during the interaction.Azulene is a molecular multilevel system. In this relation, it is worthy to note the STIRAP application of controlling non-Franck-Condon transitions in Na2 [17] and adiabatic passage by light-induced potentials in polyatomic molecules [18]. The effect of background states on STIRAP was considered by Kurkal and Rice [19] and Cheng et al. [20]. Nakajima et al. [21] discussed population transfer through continuum intermediate states.In this study, we will concentrate on another aspect of STIRAP in molecular systems. The point is that many important molecular systems are made out of assemblies of coupled localized chromophores. Examples are molecular crystals, organic nanostructures, supramolecular structures, and so forth, which are of interest from the point of view of the design of new optical materials with desirable characteristics. Therefore, in this paper, we aim to apply STIRAP rather to the assembly of interacting azulene molecules (or its derivatives) than to noninteracting molecules. In general, calculating optical properties of interacting molecules becomes an intractable many-body problem even for a reduced state formulation of the optical control process in an isolated molecule which is used in this work (see below). The local field approximation (see, e.g., [22]) provides a simple phenomenological way of relating the optical characteristics of isolated molecules to those of molecular assemblies. In the local field approximation the corresponding equations of motion, describing the system evolution, become nonlinear thus displaying the dependence of the transition frequencies on optical excitation [23, 24]. Here, we will consider a dense medium of the molecules with the dependence of the transition frequencies on optical excitation due to near dipole-dipole (DD) interactions [25]. In the following, we show that efficient STIRAP in the ladder configuration can be achieved in a dense collection of molecules exhibiting anomalous fluorescence, but only if a change of the two-photon transition frequency, due to near DD interactions, is taken into account.A two-photon resonance between the initial and final states during the interaction can not be achieved since its frequency depends on the population of these states (many-body effect) (see (13) and (20) below). Our goal is to get an efficient STIRAP in this system. We show that one can use pulses that are suitably chirped (time-dependent carrier frequency) to compensate for a change of frequency of the two-photon transition in time induced by the pulses themselves (a similar idea was proposed in studies of a two-state system in relation to Rabi oscillations in inter-subband transitions in quantum wells [26].)The outline of the paper is as follows. In Section2, we introduce our model and derive a closed set of equations for the expectation values of one-particle variables in the local field approximation. In Section 3, we show that suitably chirped pulses that compensate a change of frequency of the two-photon transition in time induced by the pulses themselves enable us to achieve a “dark” state and, hence, complete population transfer in the interacting media. We provide numerical solutions of the coupled equations for the expectation values of one-particle variables in Section 4. We summarize our results in Section 5.


## 2. Model and Basic Equations

Consider a dense collection of molecules, with densities such that there are many molecules within a cubic molecular resonance wavelength, with three electronic states with energiesE1<E2<E3 under the action of two (phase modulated) pulses E1(t) and E2(t)(1)E(r,t)=∑i=1,2Ei(t)=12∑i=1,2eiEi(t)exp⁡⁡(-iωit+iφi(t))+c.c.
The frequencies of which are close to those of the transitions 1→2 and 1→3, respectively. Here, ℰi(t) and φi(t) describe the change of the pulse amplitude and phase in time, ei are unit polarization vectors, and the instantaneous pulse frequencies are ωi(t)=ωi-dφi(t)/dt. Three states, 1, 2, and 3 correspond to singlet states S0, S1, and S2, of the azulene molecule, respectively (Figure 2). The potential-energy surfaces of polyatomic molecules are multidimensional, and the number of states related to a transition between initial and final states increases with the number of degrees of freedom of a molecule. For that reason, it is desirable to have a reduced space or a reduced state formulation of the optical control process. We will consider azulene in a Shpol'skii matrix for low temperatures; the S2→S1 fluorescence spectrum shows very narrow lines [10] (see Figure 1). We assume that field E2(t) connects states 2 and 3 corresponding to S1, with the excitation of one vibrational quantum of the vibration 1558 cm-1 and the vibrationless state of S2, respectively (see the second intensive line near λ=810 nm in Figure 1). Of course, there is one more (less intensive) line corresponding to the vibration 1756 cm-1 near the line related to 1558 cm-1. However, we will consider only one state 2, representing both vibrationally excited states under discussion in S1.Figure 1
S2→S1 fluorescence of azulene in n-hexane ad 77 K [10].Figure 2
A reduced states formulation of STIRAP in azulene. FieldE2(t) connects states 2 and 3 corresponding to S1 with the excitation of one vibrational quantum, and the vibrationless state of S2, respectively. State 1 represents the vibrationless state of a singlet S0 and field E1(t) excites transition 1→2, so that the sum of frequencies ω1(t)+ω2(t) is close to the frequency of purely electronic transition S0→S2.We assume that state 1 represents the vibrationless state of a singletS0 and field E1(t) excites transition 1→2 (see Figure 2), so that the sum of frequencies ω1(t)+ω2(t) is close to the frequency of purely electronic  transition S0→S2. In the proposed scheme, the frequencies of transitions 1→2 and 2→3 are well separated in order to realize STIRAP (in spite of close energies of purely electronic transitions S0→S1 and S1→S2 [7, 11]), though complete and robust population transfer is also possible when each of the two laser pulses interacts with each of the pair of states [27].The interaction of the dense collection of such systems with electromagnetic fields can be written as(2)Ĥint⁡=-∑nP̂n⋅El,n,
where El,n is the electric field at the location of the nth molecule (local electric field), and P̂n is its optical polarization operator. The local (microscopic) field is related to the Maxwell (macroscopic) field E(r,t), (1), by [22, 25](3)El,n=E(r,t)+4π3∑m≠nPm,
where Pm denotes the expectation value of P̂m. The second term on the right-hand side of (3) represents the electrostatic longitudinal field created by all other particles m (≠n), that is, the instantanous dipole-dipole interactions between the molecules.Let us introduce excitonic operatorsÂn,12≡|n1〉〈n2|, Ân,23≡|n2〉〈n3| and Ân,13≡|n1〉〈n3|, where |nk〉 denotes the k state of molecule n. Then, the optical polarization operator of the nth molecule is given by(4)P̂n=(Dn,12Ân,12++Dn,23Ân,23++Dn,13Ân,13+)+H.c.,
where Dn,kk′ is the transition dipole moment connecting states k and k′ of molecule n, and H.c. denotes Hermitian conjugate. We also introduce operators n̂mk=|mk〉〈mk| describing the population of states |mk〉. It is obvious that(5)n̂m1+n̂m2+n̂m3=I
due to the completeness relation for the 3-level electronic states space of the mth molecule. Here Iis the unit operator. Operators Ân,kk′ obey the following commutation relation: (6)[Âm,kk′,Âm,kk′+]=n̂mk-n̂mk′,
where k=1,2, k′=2,3, and k<k′. Then, the Hamiltonian of the dense collection of three-state systems under consideration can be written as (7)Ĥ=Ĥ0+Ĥint⁡,
where(8)Ĥ0=∑m∑k=1,2,3Emkn̂mk.Emk is the energy of state k of a molecule m.Using the Heisenberg equations of motion, one obtains the equation for the expectation value of any operatorF̂(9)ddt〈F̂〉=iℏ〈[Ĥ0+Ĥint⁡,F̂]〉≡iℏTr⁡([Ĥ0+Ĥint⁡,F̂]ρ),
where ρ is the density matrix. Straightforward operator algebra manipulations, using commutation relations, (6), yield equations for nmk≡〈n̂mk〉 and Am,kk′≡〈Âm,kk′〉 in the rotating wave approximation (RWA). In the derivation of these equations, we kept only single-particle variables, using a factorization into population variables nmk and polarizations Am,kk′ in accordance with the local field approximation [22]. Then, switching to the system that rotates with instantaneous frequency, (10)am,12=Am,12exp⁡[iω1t-iφ1(t)],am,23=Am,23exp⁡[iω2t-iφ2(t)],am,13=Am,13exp⁡[i(ω1+ω2)t-i(φ1(t)+φ2(t))],
we obtain equations for the quantities that vary slowly with time during the period of a light wave. Furthermore, considering a homogeneous excitation of an assembly of identical molecules (Dn,kk′=Dkk′,Emk=Ek,nmk=nk,am,kk′=akk′), we get (11)da12dt=-i{Ω1(t)2[ω21-ω1(t)+p12(n2-n1)]a12+Ω1(t)2×(n2-n1)-Ω2(t)2a13+(p13-p23)a23*a13},(12)da23dt=-i{Ω1(t)2[ω32-ω2(t)+p23(n3-n2)]a23+Ω1(t)2a13+Ω2(t)2(n3-n2)+(p12-p13)a12*a13},(13)da13dt=-i{Ω1(t)2[ω31-ω1(t)-ω2(t)+p13(n3-n1)]a13+Ω1(t)2a23-Ω2(t)2a12+(p12-p23)a23a12},(14)ddt(n1n3)=(-Ω1(t)Im⁡a12Ω2(t)Im⁡a23),(15)n1+n2+n3=1,
where ωkk′=(Ek-Ek′)/ℏ and Ωi(t)=(Di,i+1·ei)ℰi(t)/ℏ is the Rabi frequency corresponding to the ith pulse. The strength of the near DD interaction is given by terms (16)pkk′=4π3ℏ|Dkk′|2N,
where N is the density of molecules [25]. In writing (11)–(14), we have neglected the population-decay time of state 2 (S1). Extending this consideration to a decaying intermediate state is made in Section 4.2.One can easily see from (13) that the two-photon resonance cannot be achieved with the pulses of fixed frequency, at least due to the presence of the “local field” term p13(n3-n1) that depends on the state populations. However, suitably chirped pulses can compensate the “local field” detuning p13(n3-n1), and the first term on the right-hand side of (13) may be zero during the interaction. We will address the question of whether the chirping allows the realisation of a “dark” state and thus allows complete population transfer in the interacting media in the next section.


## 3. “Dark” State in the Interacting Media

The expectation valuesam,kk′ in the system that rotates with instantaneous frequency, (10), can be expressed through the density matrix. Indeed, (17)am,kk′=Tr⁡(âm,kk′ρ)=Tr⁡(|mk〉〈mk′|∑jj′|mj〉ρm,jj′〈mj′|)=ρm,k′k.
In particular, for pure states that are realized in the absence of relaxation, the density matrix can be represented as ρk′k=ck*ck′ where ck are the amplitudes of states, and we consider a homogeneous excitation of an assembly of identical molecules. This enables us to express akk′ by the amplitudes of states ck. Putting akk′=ck*ck′ in equations (11)–(15), we get the following equations for the magnitudes ck:(18)dc1dt=iΩ1(t)2c2,(19)dc2dt=-i[ω21-ω1(t)+p12(|c2|2-|c1|2)+(p13-p23)|c3|2]c2+iΩ1(t)2c1+iΩ2(t)2c3,(20)dc3dt=-i[ω31-ω1(t)-ω2(t)+p13(|c3|2-|c1|2)+(p12-p23)|c2|2]c3+iΩ2(t)2c2,(21)|c1|2+|c2|2+|c3|2=1.Let us assume that pulsesE1(t) and E2(t) are suitably chirped to fulfill the condition of the two-photon resonance during the interaction (the first term on the right-hand side of (20) is equal to zero). Then, one can easily see that under the adiabatic conditions (dck/dt=0), the solutions of (18)–(21) are given by c2=0,c3=-[Ω1(t)/Ω2(t)]c1 and (22)c1=Ω2(t)Ω12(t)+Ω22(t).
This enables us to obtain the adiabatic “dark” state Ψad=c1|1〉+c3|3〉 as a superposition of states |1〉 and |3〉 only, similar to the case of usual noninteracting media without local field effects [12]. Complete population transfer occurs if limt→-∞[Ω1(t)/Ω2(t)]=0 and limt→+∞[Ω2(t)/Ω1(t)]=0, where t→-∞ and t→+∞ correspond to times before and after the interaction with optical pulses, respectively.


## 4. Numerical Calculations

### 4.1. Calculations without Decay

To check these ideas, we provided numerical solutions of coupled equations (11)–(15). For this purpose, it is convenient to switch to equations for the components of the 3-state coherence vector [28](23)vkk′=i(akk′-ak′k),ukk′=akk′+ak′k,w1=n2-n1,w2=-13(n2+n1-2n3),
where k,k′=1,2,3 and k<k′. These components satisfy the following equations:(24)du12dt=-Δ21v12+Ω22v13,du23dt=-Δ32v23-Ω12v13,du13dt=-Δ31v13-Ω12v23+Ω22v12,dv12dt=Δ21u12+Ω1w1-Ω22u13,dv23dt=Δ32u23+Ω12u13+Ω22(3w2-w1),dv13dt=Δ31u13+Ω12u23-Ω22u12,dw1dt=-Ω1v12+Ω22v23,dw2dt=-3Ω2v23,
where detunings with respect to the renormalized optical transitions are given by (25)Δ21=ω21-ω1(t)+p12w1+(p13-p23)(33w2+13),(26)Δ32=ω32-ω2(t)+32w2[p23-13(p12-p13)]-12w1(p23+p12-p13)+13(p12-p13),(27)Δ31=ω31-ω1(t)-ω2(t)+32w2[p13-13(p12-p23)]+12w1(p13+p12-p23)+13(p12-p23).
In deriving equations (24), we have used the relation akk′=ck*ck′ for pure states.We considered the excitation of a dense collection of three-state systems with parameterspkk′, (16), corresponding to those of azulene with two Gaussian pulses of the same duration, ℰi(t)=ℰ0iexp[-(t-ti)2/(2τ2)], and the amplitudes giving the same maximum Rabi frequencies for transitions 1→2 and 2→3, ordered counterintuitively, E2(t) before E1(t). Parameters pkk′, (16), can be evaluated through radiation decay times τrad of transitions Si→Sj by pkk′=ϰkk′N, where ϰkk′≡1/(8π2ωk′k3τrad), and τrad were taken from [8]: τrad(S2→S0)=5·10-9 s, τrad(S1→S0)=8·10-7s and τrad(S2→S1)=2·10-6s. This gives ϰ13=1.06·10-7[cm3/s],p13≡p,p12=0.05p,p23=0.02p. The time delay between the pulses was t1-t2=2τ, and the pulse areas S=∫Ω1,2(t)dt=2πΩmaxτ ranged from 2 to 122. The product of the strength of the near DD interaction, p, and parameter τ characterizing the pulse duration, was equal to pτ=20. This value can be realized, for example, for the density of the active molecules N=3·1019 cm-3 and τ=6.3ps (this value of τ exceeds the decay time of the intermediate state that will be taken into account in Section 4.2). It is worthy to note that N=3·1019cm-3 corresponds to the mean distance between active molecules of 3.2nm justifying the use of the dipole approximation for the near DD interaction.One can see from (20) that the frequency of transition 1→3 shifts to the blue side during the population transfer 1→3, since p13>0 and p13≫p12,p23 for azulene. This denotes that the chirp preserving the two-photon resonance will not bring other levels into play close to the purely electronic transition S0→S2.Figure3 shows the state populations, after the completion of the pulses action as functions of the ratio between the Rabi frequency at the pulse maximum and parameter p for ω21-ω1=0. Dotted lines correspond to the pulses with fixed frequencies when ω31-(ω1+ω2)=0. Other lines describe the population transfer under the two-photon resonance conditions, achieved by chirping the pulse E1(t) (solid lines) and E2(t) (dashed lines). Note that pulse chirping enables us to realize the two-photon resonance during the interaction, giving rise to efficient and robust population transfer by STIRAP in interacting media, in contrast to the excitation with pulses of fixed frequencies. Pronounced oscillations of the populations in the latter case (dotted lines) can be related to bistable (or multistable) behavior of the solution of (24), due to the dependence of the resonance frequency on the population difference [14, 23]. The bistability effect consists of a sudden switching of the population from a low level to a higher level with increasing pump intensity.Populations of the final (a) and intermediate (b) states after the completion of the pulses action as functions ofΩmax/p. Solid lines: chirping the pulse E1(t), dashed: chirping E2(t), dots: pulses with fixed frequencies for ω31-(ω1+ω2)=0.
(a)(b)Chirping the pulseE2(t) gives rise to a much larger population of intermediate state 2 for small values of Ωmax/p, than chirping the pulse E1(t). This can be explained as follows. Let us assume that the chirped pulse is E1(t). To obey the two-photon resonance condition (see (20) and (27)), frequency ω1(t) must be equal to (28)ω1(t)≈ω31-ω2+p(n3-n1)=ω1+p(n3-n1),
since for azulene p13≫p12,p23. Substituting ω1(t) from (28) into (25) for the detuning with respect to the renormalized frequency of transition 2→1 (see also (19)), we get ω21-ω1(t)+pn3=ω21-ω1+pn1=pn1. In other words, detuning of transition 2→1 with respect to ω1(t) comprises pn1 which prevents populating state 2 at the beginning of the process when n1 is close to 1. In contrast, when one chirps the pulse E2(t), detuning of transition 2→1 with respect to ω1 comprises ω21-ω1+pn3=pn3 which can be close to zero at the beginning of the process. Therefore, better conditions for populating state 2 are realized when the chirped pulse is E2(t).Figure4 depicts populations n3 and n2 for the pulses with fixed frequencies when ω31-(ω1+ω2)-p13=0 corresponding to the two-photon resonance condition for the initial populations of states (n1(-∞)=1, see (28)). Note again that only the pulse chirping gives rise to efficient and robust population transfer by STIRAP in interacting media. As to the excitation with pulses of fixed frequencies, pronounced oscillations remain for both populations n2 and n3, though n3 is essentially smaller than that in Figure 3.Populations of the final (a) and intermediate (b) states after the completion of the pulses action as functions ofΩmax/p. Solid lines: chirping the pulse E1(t), dashed: chirping E2(t), dots: pulses with fixed frequencies for ω31-(ω1+ω2)-p13=0.
(a)(b)


### 4.2. Influence of the Decay of Intermediate State

In Section4.1, we have shown that efficient STIRAP for population transfer to higher electronic states in interacting media of molecules with anomalous fluorescence can be realized in the absence of decay, using suitably chirped pulses. However, an intermediate state in this process belongs to the first singlet S1 which decays very fast into S0. In this section, we will extend the above consideration to a decaying intermediate state. We will use (18)–(21) for the magnitudes ck where (19) is replaced by (29)
(29)dc2dt=-12Γc2-i[ω21-ω1(t)+p12(|c2|2-|c1|2)+(p13-p23)|c3|2]c2+iΩ1(t)2c1+iΩ2(t)2c3
taking into account a decaying intermediate state (the first term on the right-hand side of (29)).We provided numerical solutions of coupled equations (18), (20), (21), and (29). Figures 5 and 6 show that with suitably chirped pulses, the efficient STIRAP still persists even for rather large decay τΓ=6 corresponding to τ=6 ps (see Section 4.1) and 1/Γ=1 ps. However, for the excitation with pulses of fixed frequencies, the oscillations of n3 are smoothed at a large decay which may be related to vanishing the bistable (or multistable) behavior for this condition.Figure 5
Populations of the final staten3 with the decaying intermediate state (τΓ=0.6) after the completion of the pulses action as functions of Ωmax/p. Solid line: chirping the pulse E1(t), dashed: chirping E2(t), dots: pulses with fixed frequencies for ω31-(ω1+ω2)=0. Other parameters are identical to those of Figure 3.Figure 6
The same as in Figure5 only for τΓ=6.


## 4.1. Calculations without Decay

To check these ideas, we provided numerical solutions of coupled equations (11)–(15). For this purpose, it is convenient to switch to equations for the components of the 3-state coherence vector [28](23)vkk′=i(akk′-ak′k),ukk′=akk′+ak′k,w1=n2-n1,w2=-13(n2+n1-2n3),
where k,k′=1,2,3 and k<k′. These components satisfy the following equations:(24)du12dt=-Δ21v12+Ω22v13,du23dt=-Δ32v23-Ω12v13,du13dt=-Δ31v13-Ω12v23+Ω22v12,dv12dt=Δ21u12+Ω1w1-Ω22u13,dv23dt=Δ32u23+Ω12u13+Ω22(3w2-w1),dv13dt=Δ31u13+Ω12u23-Ω22u12,dw1dt=-Ω1v12+Ω22v23,dw2dt=-3Ω2v23,
where detunings with respect to the renormalized optical transitions are given by (25)Δ21=ω21-ω1(t)+p12w1+(p13-p23)(33w2+13),(26)Δ32=ω32-ω2(t)+32w2[p23-13(p12-p13)]-12w1(p23+p12-p13)+13(p12-p13),(27)Δ31=ω31-ω1(t)-ω2(t)+32w2[p13-13(p12-p23)]+12w1(p13+p12-p23)+13(p12-p23).
In deriving equations (24), we have used the relation akk′=ck*ck′ for pure states.We considered the excitation of a dense collection of three-state systems with parameterspkk′, (16), corresponding to those of azulene with two Gaussian pulses of the same duration, ℰi(t)=ℰ0iexp[-(t-ti)2/(2τ2)], and the amplitudes giving the same maximum Rabi frequencies for transitions 1→2 and 2→3, ordered counterintuitively, E2(t) before E1(t). Parameters pkk′, (16), can be evaluated through radiation decay times τrad of transitions Si→Sj by pkk′=ϰkk′N, where ϰkk′≡1/(8π2ωk′k3τrad), and τrad were taken from [8]: τrad(S2→S0)=5·10-9 s, τrad(S1→S0)=8·10-7s and τrad(S2→S1)=2·10-6s. This gives ϰ13=1.06·10-7[cm3/s],p13≡p,p12=0.05p,p23=0.02p. The time delay between the pulses was t1-t2=2τ, and the pulse areas S=∫Ω1,2(t)dt=2πΩmaxτ ranged from 2 to 122. The product of the strength of the near DD interaction, p, and parameter τ characterizing the pulse duration, was equal to pτ=20. This value can be realized, for example, for the density of the active molecules N=3·1019 cm-3 and τ=6.3ps (this value of τ exceeds the decay time of the intermediate state that will be taken into account in Section 4.2). It is worthy to note that N=3·1019cm-3 corresponds to the mean distance between active molecules of 3.2nm justifying the use of the dipole approximation for the near DD interaction.One can see from (20) that the frequency of transition 1→3 shifts to the blue side during the population transfer 1→3, since p13>0 and p13≫p12,p23 for azulene. This denotes that the chirp preserving the two-photon resonance will not bring other levels into play close to the purely electronic transition S0→S2.Figure3 shows the state populations, after the completion of the pulses action as functions of the ratio between the Rabi frequency at the pulse maximum and parameter p for ω21-ω1=0. Dotted lines correspond to the pulses with fixed frequencies when ω31-(ω1+ω2)=0. Other lines describe the population transfer under the two-photon resonance conditions, achieved by chirping the pulse E1(t) (solid lines) and E2(t) (dashed lines). Note that pulse chirping enables us to realize the two-photon resonance during the interaction, giving rise to efficient and robust population transfer by STIRAP in interacting media, in contrast to the excitation with pulses of fixed frequencies. Pronounced oscillations of the populations in the latter case (dotted lines) can be related to bistable (or multistable) behavior of the solution of (24), due to the dependence of the resonance frequency on the population difference [14, 23]. The bistability effect consists of a sudden switching of the population from a low level to a higher level with increasing pump intensity.Populations of the final (a) and intermediate (b) states after the completion of the pulses action as functions ofΩmax/p. Solid lines: chirping the pulse E1(t), dashed: chirping E2(t), dots: pulses with fixed frequencies for ω31-(ω1+ω2)=0.
(a)(b)Chirping the pulseE2(t) gives rise to a much larger population of intermediate state 2 for small values of Ωmax/p, than chirping the pulse E1(t). This can be explained as follows. Let us assume that the chirped pulse is E1(t). To obey the two-photon resonance condition (see (20) and (27)), frequency ω1(t) must be equal to (28)ω1(t)≈ω31-ω2+p(n3-n1)=ω1+p(n3-n1),
since for azulene p13≫p12,p23. Substituting ω1(t) from (28) into (25) for the detuning with respect to the renormalized frequency of transition 2→1 (see also (19)), we get ω21-ω1(t)+pn3=ω21-ω1+pn1=pn1. In other words, detuning of transition 2→1 with respect to ω1(t) comprises pn1 which prevents populating state 2 at the beginning of the process when n1 is close to 1. In contrast, when one chirps the pulse E2(t), detuning of transition 2→1 with respect to ω1 comprises ω21-ω1+pn3=pn3 which can be close to zero at the beginning of the process. Therefore, better conditions for populating state 2 are realized when the chirped pulse is E2(t).Figure4 depicts populations n3 and n2 for the pulses with fixed frequencies when ω31-(ω1+ω2)-p13=0 corresponding to the two-photon resonance condition for the initial populations of states (n1(-∞)=1, see (28)). Note again that only the pulse chirping gives rise to efficient and robust population transfer by STIRAP in interacting media. As to the excitation with pulses of fixed frequencies, pronounced oscillations remain for both populations n2 and n3, though n3 is essentially smaller than that in Figure 3.Populations of the final (a) and intermediate (b) states after the completion of the pulses action as functions ofΩmax/p. Solid lines: chirping the pulse E1(t), dashed: chirping E2(t), dots: pulses with fixed frequencies for ω31-(ω1+ω2)-p13=0.
(a)(b)


## 4.2. Influence of the Decay of Intermediate State

In Section4.1, we have shown that efficient STIRAP for population transfer to higher electronic states in interacting media of molecules with anomalous fluorescence can be realized in the absence of decay, using suitably chirped pulses. However, an intermediate state in this process belongs to the first singlet S1 which decays very fast into S0. In this section, we will extend the above consideration to a decaying intermediate state. We will use (18)–(21) for the magnitudes ck where (19) is replaced by (29)
(29)dc2dt=-12Γc2-i[ω21-ω1(t)+p12(|c2|2-|c1|2)+(p13-p23)|c3|2]c2+iΩ1(t)2c1+iΩ2(t)2c3
taking into account a decaying intermediate state (the first term on the right-hand side of (29)).We provided numerical solutions of coupled equations (18), (20), (21), and (29). Figures 5 and 6 show that with suitably chirped pulses, the efficient STIRAP still persists even for rather large decay τΓ=6 corresponding to τ=6 ps (see Section 4.1) and 1/Γ=1 ps. However, for the excitation with pulses of fixed frequencies, the oscillations of n3 are smoothed at a large decay which may be related to vanishing the bistable (or multistable) behavior for this condition.Figure 5
Populations of the final staten3 with the decaying intermediate state (τΓ=0.6) after the completion of the pulses action as functions of Ωmax/p. Solid line: chirping the pulse E1(t), dashed: chirping E2(t), dots: pulses with fixed frequencies for ω31-(ω1+ω2)=0. Other parameters are identical to those of Figure 3.Figure 6
The same as in Figure5 only for τΓ=6.


## 5. Conclusion

In this work, we have considered a coherent population transfer to a higher excited singlet state (S2) in molecular assemblies (e.g., a dense medium) of molecules with anomalous fluorescence. A direct excitation to S2 requires light in the UV region. Because of this, the transition is conveniently realized by a two-step (two-photon) process: S0→S1→S2 where transitions S0→S1 and S1→S2 correspond to the optical region. Since for such molecules, the first excited singlet state S1 is very short living, using STIRAP in the ladder configuration for the population transfer S0→S2 seems rather attractive, since a unique and very useful feature of STIRAP is that the intermediate state (S1) never gets populated, not even transiently. This is provided by maintaining a two-photon resonance between the target (S2) and initial (S0) states during the interaction.The potential energy surfaces of polyatomic molecules are multidimensional, and the number of states related to a transition between initial and final states increases with the number of degrees of freedom of a molecule. We have provided a reduced states formulation of the optical control process, using azulene in a Shpol'skii matrix for low temperatures as an example.Unfortunately, in molecular assemblies (a dense medium of molecules) a change of the frequency of the two-photon transition exists due to near DD interactions. We have shown that in spite of the frequency change, efficient STIRAP can be realized in this case as well, using suitably chirped pulses to compensate a change of the two-photon transition frequency in time induced by the pulses themselves. Chirping the “pump” pulse that excites transitionS0→S1 and the “Stokes” pulse that excites transition S1→S2 are nonequivalent with respect to the population of the intermediate state (S1) in the pulse nonadiabatic regime. We have also shown that with suitably chirped pulses, the efficient STIRAP still persists, even for a rather large decay of the intermediate state.It is worthy to note that the method for the compensation of two-photon detuning, proposed in our work, can be used not only in the case of violating the two-photon resonance due to near DD interactions, but also due to the off-resonant Stark shift [29]. In general, the pulse chirp must compensate the two-photon detuning stemming from both cases.



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*Source: 798419-2010-12-22.xml*