Energetics. In bacterial photosynthetic systems having carotenoids (Cars) with n = 9–13 conjugated double bonds in the all-trans configuration, shorter-chain Cars (n = 9 and 10) are selectively bound to LH2 antenna complexes for the light-harvesting function, which includes the absorption of light energy followed by singlet-energy transfer to bacteriochlorophyll (BChl) [1]. The all-trans conjugated chain having C_2h symmetry gives rise to low-lying singlet states, including the optically-allowed 1B_u⁺ and the optically-forbidden 2A_g⁻, 1B_u⁻ and 3A_g⁻ states, concerning transitions from/to the ground 1A_g⁻ state [2,3]. The 1B_u⁻ and 3A_g⁻ states of Cars were first identified by the measurement of resonance-Raman excitation profiles (RREP) [1].

As shown in Figure 1, the observed slopes of the linear relations for the 2A_g⁻, 1B_u⁻ and 3A_g⁻ states, as functions of 1/(2n + 1), were in the ratio of 2:3.1:3.8, which is in excellent agreement with those theoretically predicted for shorter polyenes (n = 5–8) in the ratio of 2:3.1:3.7 [4]. This is actually the basis for the assignment of these forbidden electronic-excited states. Because of the set of linear relations, the next low-lying singlet state below the 1B_u⁺ state is the 1B_u⁻ state for the shorter-chain Cars (n = 9 and 10), whereas the 3A_g⁻ state, for the longer-chain Cars (n = 11–13). Figure 2 shows the chemical structures of the relevant Cars (n = 9–13).

Dynamics. The singlet internal-conversion processes of 1B_u⁺ → 1B_u⁻ → 2A_g⁻ → 1A_g⁻ and the singlet-to-triplet fission followed by the triplet internal-conversion process of 1B_u⁻ → T₂ (A_g) → T₁ (B_u) have been identified in the set of Cars (n = 9–13) in solution by pump-probe time-resolved spectroscopy using ∼100 fs pulses. The singlet internal conversion including the 3A_g⁻ state, i.e., 1B_u⁺ → 3A_g⁻ → 1B_u⁻ → 2A_g⁻ → 1A_g⁻, has been identified in Cars (n = 11–13) by pump-probe spectroscopy using <5 fs pulses, and in Cars (n = 10 and 11) by subpicosecond time-resolved Raman spectroscopy using ∼100 fs pulses [1,5,6].

The low-lying singlet states of all-trans Cars have been found to give rise to plural channels of Car-to-BChl singlet-energy transfer during the processes of internal conversion in the order, 1B_u⁺, 1B_u⁻ and then 2A_g⁻. This is the reason for the natural selection of the shorter-chain Cars in the all-trans configuration by antenna complexes. By transferring the rates of internal conversion within the Car and BChl a molecules in solution to those bound to the LH2 antenna complexes, the efficiencies of Car-to-BChl singlet-energy transfer through the 1B_u⁺-to-Q_x, 1B_u⁻-to-Q_x and 2A_g⁻-to-Q_y channels as well as the efficiencies of the 1B_u⁻-to-T₁ singlet-to-triplet fission reactions were determined [1,7,8]. The sums of efficiencies through the three channels for Cars (n = 9, 10, 11 and 11) were evaluated to be 88, 84, 51 and 54%, respectively, which nicely correlates to those determined by comparison of the electronic-absorption and fluorescence spectra, i.e., 92, 89, 53 and 55%. The sudden decrease in the Car-to-BChl singlet energy-transfer efficiency, on going from n = 10 to n = 11, was explained by the closing of the latter two channels due to the lowering of the 1B_u⁻ and 2A_g⁻ energies shown in Figure 1. Thus, the important roles of the 1B_u⁻ state in the singlet-to-triplet transformation and the Car-to-BChl singlet-energy transfer have been determined. However, the roles of the 3A_g⁻ state in the light-harvesting function are left to be determined.

Energetics. Because of the unique linear relations among the 1B_u⁺(0), 1B_u⁻(0) and 3A_g⁻(0) vibrational origins as shown in Figure 1, the 1B_u⁻(0) level, for example, completely or approximately overlaps with the 1B_u⁻(1) and 1B_u⁻(2) levels in the shorter-chain Cars (n = 9 and 10), whereas with the 3A_g⁻(1), 3A_g⁻(2) and 3A_g⁻(3) levels in the longer-chain Cars (n = 11, 12 and 13, respectively) as shown in Figure 3.

We will call the pair of overlapped levels ‘diabatic vibronic levels’ or ‘diabatic pair’, because a diabatic basis set, instead of an adiabatic basis set, becomes necessary to theoretically describe their excited-state properties [10] (see Section 1.3). Thus, the shorter-chain Cars can form the 1B_u⁺ + 1B_u⁻ diabatic pairs, whereas the longer-chain Cars, the 1B_u⁺ + 3A_g⁻ diabatic pairs. It is to be noted that the energy gap between the diabatic pair is the largest in Car (n = 11) and negligible in Car (n = 10) (Figure 3), if we assume the interval of vibronic levels to be ∼1,400 cm⁻¹, inclusively taking into account the C=C (ν₁) and C–C (ν₂) stretching modes.

The definition of the diabatic pair includes not only that the pair of vibronic levels is overlapped with each other, but also that the overlapped vibronic levels are located close to the conical intersection (see Figure 4). Concerning the set of potential functions, the shifts of the 1B_u⁺, 1B_u⁻ and 2A_g⁻ potential minima, in reference to the ground 1A_g⁻ potential minimum, were determined by the Franck-Condon simulations of stationary-state fluorescence spectra from Cars (n =9–13) [9]. The 3A_g⁻ potential has been determined by pump-probe stimulated-emission spectroscopy of Cars (n = 11–13) after coherent excitation using 30 fs pulses [11], the details of which will be described in Section 3.1 of this article. Figure 4 clearly shows that the above-mentioned diabatic pairs, i.e., 1B_u⁺(0) + 1B_u⁻(1) and 1B_u⁺(0) + 1B_u⁻(2) in Cars (n = 9 and 10) as well as 1B_u⁺(0) + 3A_g⁻(1), 1B_u⁺(0) + 3A_g⁻(2) and 1B_u⁺(0) + 3A_g⁻(3) in Cars (n = 11, 12 and 13), are located close enough to the conical intersection, and satisfies the above condition of the diabatic pair. Another set of five pairs, which are located one vibrational-quantum higher, also fits this definition.

Dynamics. The all-trans conjugated chain of Cars has approximate C_2h symmetry in the ground state and, as a result, the singlet electronic states can be classified by symmetry into kA_g⁻, lB_u⁻, mB_u⁺ and nA_g⁺, where the + and – signs are called Pariser’s labels [2] and k, l, m and n indicate the ordering of the electronic states having the same symmetry (from the lowest to the higher energies). As shown in Figure 1, the low-lying singlet-excited states are in the order, 2A_g⁻, 1B_u⁻, 3A_g⁻ and 1B_u⁺. Concerning Pariser’s labels, optical transitions are allowed (forbidden) between electronic states with different signs (the same sign), whereas internal conversion is allowed (forbidden) between electronic states with the same sign (different signs).

As will be described in the next section, both the optically-allowed 1B_u⁺ counterpart and the optically-forbidden 1B_u⁻ or 3A_g⁻ counterpart keep their own symmetry properties, and behave as if they were totally independent symmetry-wise even after forming the diabatic pair.

The unique characteristics of the low-lying singlet-excited states of Cars in the all-trans configuration can be summarized as follows: (a) Singlet-excited states having different symmetries, energetically in the order of 1B_u⁺, 3A_g⁻, 1B_u⁻ and 2A_g⁻, are closely located within a small energy difference in the region of 1–3 vibrational quanta (see Figure 1). (b) The minima of the 3A_g⁻, 1B_u⁻, 1B_u⁺ and 2A_g⁻ potentials are located, in this order, in a small region of mass-adjusted normal coordinate of q = 0–2 (see Figure 4). (c) A pair of excited-state potentials with different symmetries can cross at the conical intersection keeping their own symmetry characteristics, the details of which are described below.

In the vicinity of a conical intersection, the Born-Oppenheimer approximation - on which the adiabatic description is based - breaks down. The reason for this is as follows: (1) The derivative coupling can be expressed as the vibronic coupling divided by the potential-energy difference like (1) 〈 φ i A | ∂ ∂ Q a | φ j A 〉   =   〈 φ i A | ∂ H ∂ Q a | φ j A 〉 / { V i i ( Q ) − V j   j ( Q ) }

In the complete all-trans planar configuration in the ground state having the C_2h symmetry, the vibronic-coupling term between a pair of electronic states (φ_i and φ_j) having different Pariser’s ± labels vanishes. However, when the Car molecule is excited to the 1B_u⁺ state, for example, there is a good chance for the conjugated chain to take a twisted conformation (degrading the C_2h symmetry) and to give rise to a certain value of the vibronic coupling. Then, in the vicinity of conical intersection where V_ii(Q) – V_jj(Q) approaches to 0, the derivative coupling diverges. (2) The time-dependent perturbation theory shows that the rate of change in any of the MO and CI coefficients is proportional to the value of V_ii(Q) – V_jj(Q) and, therefore, the reorganization of electronic wavefunction practically cannot take place in the vicinity of the conical intersection.

Therefore, it becomes absolutely necessary to use diabatic expression, instead, setting the derivative coupling to be zero, i.e., (2) 〈 φ i D | ∂ ∂ Q a | φ j D 〉 = 0and fix the MO and CI coefficients by the use of the orthogonal floating atomic orbitals. As a result, a pair of electronic wavefunctions, expressed by such a diabatic basis set, keeps the symmetry of each electronic state at any nuclear coordinate (Q), which makes the pair of nuclear potentials having different symmetries cross each other at the conical intersection, as shown in Figure 4.

The above consideration has rationalized the apparently unique characteristics of the diabatic pair of electronic states: At the first glance, it looked strange and accidental that the symmetry properties of singlet-excited states conserve, as if they were totally independent from each other. However, it has turned out to be quite logical after we carefully consider the characteristics of the diabatic pair.

Working on the set of Cars (n = 9–13) has been very fortunate, because the shorter-chain Cars (n = 9 and 10) and the longer-chain Cars (n = 11–13) form completely different diabatic pairs in symmetries, i.e., 1B_u⁺ + 1B_u⁻ and 1B_u⁺ + 3A_g⁻, respectively. This situation has enabled us to make a comparison between the two different combinations of symmetries in these diabatic pairs, and to establish the symmetry notation of the relevant singlet-excited states we have proposed.

In the electronic mixing of the diabatic pair (‘diabatic electronic mixing’) as well as in the internal conversion from a diabatic pair (‘diabatic internal conversion’), we have found a common symmetry selection rule, i.e., ‘1B_u⁺-to-1B_u⁻ is allowed but 1B_u⁺-to-3A_g⁻ is forbidden’. When a 1B_u⁺ + 1B_u⁻ diabatic pair vibrationally relaxes down to the bottom of the 1B_u⁺ potential, for example, the 1B_u⁺(0) optically-allowed counterpart relaxes through radiative transition to the 2A_g⁻ or 1A_g⁻ state, whereas the 1B_u⁻ optically-forbidden counterpart relaxes through internal conversion to the iso-energetic 2A_g⁻ vibronic level followed by vibrational relaxation in the particular manifold.

The above experimental results (to be described in detail in Section 2.2) evidence that the symmetry of each electronic state is totally conserved during the formation of the diabatic pair as well as in the splitting of the diabatic pair into the optically-allowed and the optically-forbidden counterparts.

Pump-probe stimulated-emission and electronic-absorption spectroscopy. We used both ∼100 fs and ∼30 fs pulses for pump-probe stimulated-emission and electronic-absorption spectroscopy. Correlation between the time-duration and the spectral-width of these pulses is presented in Figure 5, showing the intensity profiles and the numerical values of FWHM.

In comparison to the energy gap between the diabatic pair of Car (n = 11) (∼300 cm⁻¹) shown in Figure 3, for example, the ∼100 fs pulses with the FWHM_σ of ∼200 cm⁻¹ still tend to selectively excite one of the counterparts of the diabatic pair, whereas the ∼30 fs pulses with the FWHM_σ of ∼700 cm⁻¹ can excite the optically-allowed and optically-forbidden diabatic counterparts simultaneously and coherently. Therefore, we call excitation with ∼100 fs pulses ‘selective excitation’, whereas excitation with ∼30 fs pulses ‘coherent excitation’.

Visible-pump and near infrared-probe spectroscopy mainly probes transient-absorption spectra with some contribution of stimulated emission, while visible-pump and visible-probe spectroscopy probes the strong 1B_u⁺ stimulated emission as the optically-allowed counterpart. The latter spectroscopy is useful to identify stimulated emission from the optically-forbidden 1B_u⁻ or 3A_g⁻ counterpart of the diabatic pair, if any, and to conclude the presence or absence of the diabatic electronic mixing.

Kerr-gate fluorescence spectroscopy. We used this technique to probe fluorescence (mainly spontaneous emission) from the optically-forbidden vibronic levels of the Car molecules when they are being vibronically excited. This spectroscopic technique directly determines the energies of the emitting vibronic levels. Further, the excited-state molecules are free from disturbance by the probing radiation.

After the Introduction (Section 1), we are going to correlate the unique excited-state properties of the diabatic vibronic levels that we have found most recently. Those findings are classified into different categories in terms of the spectroscopic techniques used:

Section 2: We used ∼100 fs pulses for selective excitation: First, we excited to the 1B_u⁺(0) level of a set of all-trans Cars (n = 9–13) in nonpolar solvent, and mainly probed transient absorptions by the use of near-infrared (NIR) white continuum to determine the 1B_u⁺, 1B_u⁻ and 3A_g⁻ lifetimes (Section 2.1). Then, we excited the same set of Cars to the 1B_u⁺(0) level and examined the presence or absence of stimulated emission from the optically-forbidden counterpart by the use of visible (VIS) white continuum. As a result, we found a symmetry selection rule in the diabatic mixing and diabatic internal conversion (Section 2.2). We also examined all-trans- and 15-cis-β-carotenes in nonpolar and polar solvents, and tried to find the effects of cis–trans configurations and those of the polarization of the conjugated chain by polar solvents on the initial stimulated emission patterns. The effect of aggregation was also found (Section 2.3).

Section 3: We used ∼30 fs pulses for coherent excitation of Cars (n = 11–13) in polar solvent, THF. Here, we observed stimulated emission followed by transient absorption from the 3A_g⁻ counterpart, exhibiting a single peak with the 3A_g⁻(0) energy. The results lead us to conclude that the shift of the 3A_g⁻ potential, with respect to the ground 1A_g⁻ potential, is negligible (Section 3.1). The stimulated emission after coherent excitation of Cars (n = 9 and 10) actually consisted of three components; one from the long-lived 1B_u⁺ + 1B_u⁻ diabatic pair, and the other two from the short-lived 1B_u⁺ and 1B_u⁻ counterparts. On the other hand, the stimulated emission after coherent excitation of Car (n = 11–13) consisted of one, from the long-lived 1B_u⁺ + 3A_g⁻ diabatic pair and the other two, from the short-lived 1B_u⁺ and 3A_g⁻ counterparts. The set of three components was explained by the mechanisms of quantum beat (Section 3.2). The same type of stimulated emission consisting of three components was observed after coherent excitation of Cars (n = 9–11) bound to the LH2 antenna complexes, which accompanied the shift of the 1B_u⁻(0) and 3A_g⁻(0) levels to the lower energies and efficient triplet generation (Section 3.3).

Section 4: We used ∼100 fs pulses to excite Cars (n = 9–12) to the 1B_u⁺(3) or 1B_u⁺(4) level and probed fluorescence, by Kerr-gate fluorescence spectroscopy, to examine the slowest two steps of vibrational relaxation, i.e., 1B_u⁺(2) → 1B_u⁺(1) → 1B_u⁺(0). We found the breakdown of the above-mentioned symmetry selection rule in the diabatic electronic mixing and diabatic internal conversion, due to the degradation of molecular symmetry, while the Car molecules were being excited (Section 4.1).

Section 5: We will summarize the results obtained (Section 2–Section 4) and discuss the future trend of the present line of research.

After Section 6: Conclusion, we will introduce Section 7: Relevant work done by other investigators.

As shown in Figure 1, the next low-lying singlet state below the 1B_u⁺ state is the 1B_u⁻ state in Cars (n = 9 and 10), whereas it is the 3A_g⁻ state in Cars (n = 11–13); further, in Cars (n = 10), the 1B_u⁺ state is overlapped with the 3A_g⁻ state. Since the set of Cars is dissolved in nonpolar solvent (n-hexane or a mixture of n-hexane and benzene), the conjugated chains are expected to keep the C_2h symmetry in the ground state, before selective excitation with ∼100 fs pulses (the same symmetry should be conserved immediately after excitation).

Figure 6 exhibits the pump-probe time-resolved spectra of Cars (n = 9–13), and Figure 7 shows the species-associated difference spectra (SADS, top) and time-dependent changes in population (bottom) that have been obtained by singular-value decomposition (SVD) followed by global fitting of the spectral-data matrices by the use of a two-component sequential model. The first component, appearing immediately after excitation, is ascribable to the optically-allowed 1B_u⁺ state to which all the Car molecules were excited by the absorption of photons; each SADS consists of transient absorption and stimulated emission. The second component, appearing around 0.2 ps after excitation, is ascribable to the 1B_u⁻ state in the shorter-chain Cars (n = 9 and 10), whereas to the 3A_g⁻ state in the longer-chain Cars (n = 11–13), according to the energy diagram (Figure 1). The contribution of the 3A_g⁻ transient absorption is also seen in the second component of Car (n = 10) as expected.

The decay time constants listed in Table 1 show that the 1B_u⁺ lifetimes of Cars (n = 9 and 10) are on the order of 0.1 ps, which is much longer than those of Cars (n = 11–13) on the order of 0.01 ps. On the other hand, the 1B_u⁻ lifetimes are around 0.25 ps, whereas the 3A_g⁻ lifetimes are around 0.10 ps.

Figure 8 shows the pump-probe time-resolved spectra of Cars (n = 9–13) in nonpolar solvent after selective excitation with ∼100 fs pulses to the 1B_u⁺(0) level (called ‘0 ← 0 excitation’). Here, we can see the singlet-state internal-conversion processes of 1B_u⁺ → 1B_u⁻ → 2A_g⁻ → 1A_g⁻ (ground). In this subsection, we focus on the initial stimulated emission patterns that are useful in examining the presence or absence of diabatic electronic mixing between the optically-allowed 1B_u⁺(0) and the iso-energetic optically-forbidden 1B_u⁻ or 3A_g⁻ vibronic levels. In this relation, we notice that the intensity of the strongest stimulated emission peak relative to the second-strongest one is much higher in the shorter-chain Cars (n = 9 and 10) than in the longer-chain Cars (n = 11–13). The higher intensity in the former has turned out to be due to additional contribution of the 1B_u⁻ stimulated emission (vide infra).

Figure 9 shows the pump-probe time-resolved spectra when Cars (n = 9–13) were excited to the 1B_u⁺(1) level (called ‘1 ← 0 excitation’) in terms of the 1B_u⁺ counterpart. Here, we need to remember the presence of the iso-energetic 1B_u⁻ or 3A_g⁻ diabatic counterpart; these diabatic pairs are shown on the top of Figure 3. We notice that the relative intensity of the strongest two stimulated-emission peaks changes with time, not in Car (n = 12) but in Car (n = 10), for example, the latter of which actually reflects vibrational relaxation (vide infra).

Figure 10 exhibits the initial stimulated-emission patterns that have been extracted from the time-resolved spectra as SADS by means of the SVD and global-fitting analysis. In Cars (n = 9 and 10), we succeeded in time-resolving the initial two components reflecting vibrational relaxation. We tried to simulate those negative signals in terms of the following components: the 1B_u⁺ stimulated emission (in red), the 1B_u⁻ stimulated emission (blue) and the bleaching of ground-state absorption (black) shown in broken or dotted line. Their sums (black dotted-broken line) are compared with the observed stimulated-emission patterns as SADS (black solid line).

The results of simulation can be summarized as follows: (a) Shorter-chain Cars (n = 9 and 10): After the 0 ← 0 excitation, the observed stimulated emission can be explained by simultaneous stimulated emission from the diabatic pairs, i.e., 1B_u⁺(0) + 1B_u⁻(1) and 1B_u⁺(0) + 1B_u⁻(2), respectively. After the 1 ← 0 excitation, the vibrational relaxation of 1B_u⁺(1) + 1B_u⁻(2) → 1B_u⁺(0) + 1B_u⁻(1) and 1B_u⁺(1) + 1B_u⁻(3) → 1B_u⁺(0) + 1B_u⁻(2), respectively, take place. (b) Longer-chain Cars (n = 11–13): After the 0 ← 0 excitation, only the 1B_u⁺(0) stimulated emission is observed, whereas after the 1 ← 0 excitation, only the 1B_u⁺(1) stimulated emission, instead. Neither the contribution of the 3A_g⁻ counterpart nor the vibrational relaxation of 1B_u⁺(1) → 1B_u⁺(0) is observed at all in the set of SADS.

Figure 11 summarizes the relaxation dynamics starting from the diabatic pair for all the set of Cars (n = 9–13): The shadowed envelopes show simultaneous stimulated emission from the 1B_u⁺ + 1B_u⁻ diabatic pair, and the bent and short arrows, internal conversion and vibrational relaxation, respectively. (a) Shorter-chain Cars (n = 9 and 10): As revealed by the simulation described above, the simultaneous stimulated emission from the 1B_u⁺ and 1B_u⁻ diabatic pair and the vibrational relaxation of the diabatic pair, i.e., υ = 1 → υ = 0 in terms of the 1B_u⁺ counterpart, are seen. (b) Longer-chain Cars (n = 11–13): Neither the stimulated emission from the 3A_g⁻ optically-forbidden counterpart nor the vibrational relaxation in the 1B_u⁺ manifold is seen in Cars (n = 11–13). This is because the 1B_u⁺ + 3A_g⁻ diabatic electronic mixing never takes place, and the 1B_u⁺ → 1B_u⁻ diabatic internal conversion, instead, takes place very efficiently.

As shown in the pump-probe time-resolved spectra and the simulation of the initial stimulated emission, the 1B_u⁺ + 1B_u⁻ stimulated emission transforms into the 1B_u⁻ transient absorption while taking vibrational relaxation in Cars (n = 9 and 10), whereas the 1B_u⁺ stimulated emission directly transforms into the 1B_u⁻ transient absorption in Cars (n = 11–13). Although the resultant 1B_u⁻ transient absorption is the same, the mechanisms of its generation are different between the shorter-chain and the longer-chain Cars. It is continuous vibrational relaxation in the 1B_u⁻ manifold in the former, while it is the 1B_u⁺ to 1B_u⁻ internal conversion followed by vibrational relaxation in the 1B_u⁻ manifold in the latter (Figure 11).

In the latter case, we saw efficient 1B_u⁺ → 1B_u⁻ → 2A_g⁻ internal conversion in the time-resolved spectra and in the results of SVD and global-fitting analysis of the spectral-data matrices (see Figure S3 in Supporting Information of Ref. [13]). Thus, the reason for the absence of the 3A_g⁻ signal in the pump-probe time-resolved spectra of Cars (n = 11–13) (Figures 8 and 9) has been explained.

The above set of results lead us to the following symmetry selection rule, concerning the diabatic electronic mixing and diabatic internal conversion: ‘1B_u⁺-to-1B_u⁻ is allowed but 1B_u⁺-to-3A_g⁻ is forbidden’. This selection rule has been theoretically explained [10].

Figure 12 presents (a) the molecular structures of all-trans- and 15-cis-β-carotenes having C_i and C_2v symmetries and (b) an energy diagram for β-carotenes with the effective conjugation length of n = 10.6 (evaluated from the crossing point between the 3A_g⁻(0) energy of 18,700 cm⁻¹ in β-carotenes and the 3A_g⁻(0) regression line reproduced from Figure 1). Here, a consecutive vibrational ladder with a spacing of 1,300 cm⁻¹ including the 2A_g⁻(0), 1B_u⁻(0), 3A_g⁻(0) and 1B_u⁺(0) origins can be formed, a unique property of this particular Car.

Figure 13 shows a set of pump-probe time-resolved spectra after selective excitation with ∼100 fs pulses to the 1B_u⁺(1) level (the absorption maximum) of all-trans- and 15-cis-β-carotenes in nonpolar (n-hexane) and polar (DMF and DMF + IL) solvents; here, DMF indicates dimethylformamide and IL, an ionic liquid, i.e., methyl-3-octylimidazoluim tetrahydrofluoroborate.

Figure 14 presents the stimulated-emission patterns (black solid line) that have been obtained as the first SADS components in the SVD and global-fitting analysis of the time-resolved data matrices, parts of which are presented in Figure 13. We tried to simulate each stimulated-emission pattern by the use of the Franck-Condon profiles for the 1B_u⁺ → 1A_g⁻ stimulated emission (red broken line) and the bleaching of the 1B_u⁺ ← 1A_g⁻ absorption (black dotted line) as well as the Gaussian profiles from the 1B_u⁻(1) (blue broken line) and 3A_g⁻(0), 3A_g⁻(1), 3A_g⁻(2) and 3A_g⁻(3) (green broken line) vibronic levels. In the calculation of the Frank-Condon simulation, we analyzed the fluorescence data of β-carotene [15] again to determine the 1B_u⁻ potential treating collectively the C=C and C–C stretching modes. Here, the Gaussian profiles of the 1B_u⁻(1) level is an approximation (actually it has a pair of wings on both sides; see Figure 10). Most importantly, the Gaussian peaks of the 3A_g⁻(0) – 3A_g⁻(3) levels must originate from the negligible shift of the 3A_g⁻ potential in reference to the 1A_g⁻ potential (to be proven in Section 3.1).

The stimulated-emission profiles of all-trans- and 15-cis-β-carotenes can be characterized as follows (see Figure 14): (a) Comparison between the two isomers: In n-hexane, all-trans-β-carotene exhibits a simplified stimulated-emission profile consisting of two main peaks, i.e., 3A_g⁻(0) and 3A_g⁻(1), whereas 15-cis-β-carotene exhibits a progression consisting of five peaks, i.e., 1B_u⁻(1), 3A_g⁻(0), 3A_g⁻(1), 3A_g⁻(2) and 3A_g⁻(3), both in addition to a weak Franck-Condon profile from the 1B_u⁺(1) level. This spectral change, on going from all-trans- to 15-cis-β-carotene, reflects the lowering of the symmetry of the conjugated chain from C_i to C_2v. (b) Comparison among three solvents: In all-trans-β-carotene, the stimulated-emission peaks increase in number on going from n-hexane to DMF or DMF + IL. Some peaks are further enhanced in the latter polar solvent. In 15-cis-β-carotene, no changes in the number of peaks are observed on going from n-hexane to DMF or DMF + IL, although changes in the relative intensities are observed; 15-cis-β-carotene in DMF + IL gives rise to the clearest set of Gaussian peaks. We added IL to enhance the polarization of the conjugated chain; actually, some 3A_g⁻ Gaussian peaks seem to be enhanced after addition of IL.

Figure 15 exhibits vibronic levels giving rise to the relevant peaks appearing as a sum of the 1B_u⁺ → 1A_g⁻ stimulated emission (Franck-Condon) components and the 3A_g⁻ → 1A_g⁻ plus 1B_u⁻ → 1A_g⁻ stimulated emission (Gaussian) components. The overlapped 1B_u⁺ + 3A_g⁻ vibronic levels as well as the isolated 3A_g⁻(0) and 1B_u⁻(1) levels can give rise to a progression of peaks due to the multiple 1B_u⁺(m) ↔ 3A_g⁻(n) or 1B_u⁻(1) radiative resonance transitions to facilitate the mutual transfer of phonons (vibrational energy) between a pair of molecules in aggregates.

We have been determining the 1B_u⁺, 2A_g⁻ and 1B_u⁻ potentials of Cars by fluorescence spectroscopy: The shift of potential minimum, in reference to the ground-state 1A_g⁻ potential, was the largest in the 2A_g⁻ state, a middle in the 1B_u⁺ state, and the smallest in the 1B_u⁻ state [9], the 3A_g⁻ potential being left to be determined. However, we saw a progression of the Gaussian-type 3A_g⁻ stimulated emission in isomeric β-carotenes (see Section 2.3), each of which strongly suggested the negligible shift of the 3A_g⁻ potential; here, the progression was ascribed to resonance transfer of phonons between a pair of Car molecules in aggregates as mentioned in Section 2.3.

Figure 16 shows a set of pump-probe time-resolved stimulated-emission and transient-absorption spectra after coherent excitation with ∼30 fs pulses to the 1B_u⁺(0) + 3A_g⁻ (υ = 1–3) diabatic levels of Car (n = 11–13) in THF solution. Following the initial 1B_u⁺(0) stimulated emission, a set of peaks assignable to the 3A_g⁻ stimulated emission appears. The stimulated emission peak systematically shifts to the lower energy with n, and exactly fits the regression line of the 3A_g⁻(0) energy obtained by the measurement of resonance-Raman excitation profiles (Figure 1) as shown in Figure 17. Subsequently, a set of peaks ascribable to the 3A_g⁻ transient absorption with the same energy appears as shown in the time-resolved spectra.

The time-dependent changes in the fluorescence and absorption patterns can be characterized as follows: (1) The 3A_g⁻ stimulated emission appears first as a single peak having the 3A_g⁻(0) energy; no vibrational structures ascribable to the Franck-Condon factors are seen at all. (2) The 3A_g⁻ transient absorption appears next also as a single peak having the 3A_g⁻(0) energy. No vibrational structures are seen in the 3A_g⁻ transient absorption either. (3) The 3A_g⁻ transient absorption is longer-lived and gets stronger in intensity than the 3A_g⁻ stimulated emission at later delay times, the former becomes overlapped with the 1B_u⁻ transient absorption having a vibrational structure and less clear.

Figure 18 shows a mechanism proposed to explain the above time-dependent changes in the stimulated-emission and transient-absorption patterns in Car (n = 12), for example. The key issue here is the negligible shift of the 3A_g⁻ potential in reference to the 1A_g⁻ potential. Under this condition, all the vibrational wavefunctions in both the upper 3A_g⁻ and the lower 1A_g⁻ states become orthogonal, and only the iso-energetic 3A_g⁻(2) ↔ 1A_g⁻(2), 3A_g⁻(1) ↔ 1A_g⁻(1) and 3A_g⁻(0) ↔ 1A_g⁻(0) emissive or absorptive transitions become allowed. Then, all the above characteristics (i), (ii) and (iii) can be explained as follows:

(a) The Car (n = 12) molecules are coherently excited by absorption of photons to the 1B_u⁺(0) + 3A_g⁻(2) diabatic pair (see Section 3.2 for the details of this state). Following the processes of vibrational relaxation in the 3A_g⁻ manifold, the 3A_g⁻(2) → 1A_g⁻(2), 3A_g⁻(1) → 1A_g⁻(1) and 3A_g⁻(0) → 1A_g⁻(0) stimulated emission, having exactly the same energy as that of the 3A_g⁻(0) ← 1A_g⁻(0) transition (Figure 3), should take place in this sequence. (b) A substantial amount of light energy deposited on the 3A_g⁻(2) level should be accumulated as thermal energy on the 1A_g⁻ vibronic levels after a while, when its dissipation is slow. This gives rise to the 3A_g⁻(0) ← 1A_g⁻(0), 3A_g⁻(1) ← 1A_g⁻(1) and 3A_g⁻(2) ← 1A_g⁻(2) absorptive transitions with the same transition energy as mentioned above.

Thus, the negligible shift of the 3A_g⁻ potential, in reference to the 1A_g⁻ potential, has been established by coherent excitation of the set of Cars (n = 11–13).

The unique excited-state dynamics after coherent excitation with ∼30 fs pulses to the diabatic pair of Cars (n = 9–13) in THF solution stems from the following experimental conditions: (a) The interaction between the optically-allowed 1B_u⁺(0) and the optically-forbidden iso-energetic 1B_u⁻ or 3A_g⁻ levels should become stronger in polar solvent than in nonpolar solvent due to the polarization of the conjugated chain and the resultant symmetry degradation from C_2h to C_s. (b) The spectrally-broad ∼30 fs pulses enable the simultaneous coherent excitation of the diabatic pair as mentioned above. (c) The photon density (the number of photons per unit time) should be much higher in ∼30 fs pulses than in ∼100 fs pulses; therefore, there is a good chance that the diabatic pair becomes densely populated. These conditions gave rise to unique spectral patterns (Figure 19) that are completely different from those obtained by selective excitation with ∼100 fs pulses in nonpolar solvent (Figure 8). Here, the Franck-Condon simulation of the stimulated emission is impossible.

To facilitate the spectral comparison, the initial stimulated-emission patterns that have been presented in Figure 8 are reproduced for Cars (n = 9–11) in Figure 20, in the spectral regions corresponding to those of Figure 19 are presented. The vertical broken lines indicate the positions of the predominant stimulated-emission peaks in Figure 19 (note the difference in solvent polarity between n-hexane and THF).

The pump-probe time-resolved spectra of Cars (n = 9–11) presented in Figure 19, that have been recorded under the above-mentioned experimental conditions (a), (b) and (c), can be characterized as follows: (i) An initial short-lived stimulated-emission peak from the 1B_u⁺(0) level. Immediately after excitation, a weak and sharp peak ascribable to the pure 1B_u⁺(0) stimulated emission appears. (ii) A persistent stimulated emission peak from the 1B_u⁺(0) + X⁻(υ) diabatic pair. (Here, X⁻(υ) indicates the 1B_u⁻(1), 1B_u⁻(2), 3A_g⁻(1), 3A_g⁻(2) and 3A_g⁻(3) levels for Cars (n = 9, 10, 11, 12 and 13, respectively).) Subsequently, a much stronger, broad and long-lived stimulated-emission peak ascribable to the 1B_u⁺ + X⁻(υ) diabatic pair appears. This particular peak even tends to split into two in Car (n = 10) in the 0.15–0.30 ps time region. Eventually, the stimulated emission from the diabatic pair disappears and the bleaching of the ground-state 1B_u⁺(0) ← 1A_g⁻(0) absorption and the 2A_g⁻ transient-absorption remain. (iii) The 1B_u⁻(0), 3A_g⁻(0) and 1B_u⁺(0) stimulated emission peaks. Around 0.06–0.10 ps, a peak systematically shifting to the lower energy with n, which is ascribable to the 1B_u⁻(0) stimulated emission, appears in Cars (n = 9 and 10). As shown in Figure 17, the energies of these stimulated emission peaks agree with those determined by RREP measurement. In the shorter-chain Cars (n = 9 and 10), another 1B_u⁺(0) stimulated emission ascribable to the 1B_u⁺(0) → 1A_g⁻(1) transition appears, while stimulated emission from the 1B_u⁺(0) + X⁻(υ) diabatic pair predominates. Later, both the 1B_u⁺(0) and 1B_u⁻(0) stimulated emission peaks are replaced by the 1B_u⁻ transient absorption peaks.

The above spectral characteristics can be explained in terms of the mechanism of quantum beat (see Figure 21 referring to Figure 19). To be consistent to what will be described in Section 3.3, we will take the case of Car (n = 10) as the first example: (i) The stimulated emission from the 1B_u⁺(0) + 1B_u⁻(2) diabatic pair, which follows the initial weak stimulated emission from the pure 1B_u⁺(0) level, can be attributed to the coherent cross term. In phenomenological expression, the 1B_u⁺(0) lifetime becomes substantially lengthened by back-and-forth exchanges between the optically-allowed 1B_u⁺ and optically-forbidden 1B_u⁻ states; for the rigorous theoretical description of this quantum beat mechanism, see Eq. 48 in Ref. [10]. (ii) The 1B_u⁻(0) level that is responsible for stimulated emission is the result of vibrational relaxation from the 1B_u⁻(2) optically-forbidden counterpart of the diabatic pair; this is attributed to one of the incoherent terms. (iii) The 1B_u⁺(0) level exhibits strong 1B_u⁺(0) → 1A_g⁻(1) stimulated emission in this particular Car; this is ascribable to the other incoherent term.

Next, we proceed to the case of Car (n = 11), which can be explained in a similar way, where 1B_u⁻(2) is replaced by 3A_g⁻(1) as shown in Figure 21: (i) The stimulated emission from the 1B_u⁺(0) + 3A_g⁻(1) pair (which follows the initial weak stimulated emission from the pure 1B_u⁺(0) level) exhibits a strong, broad and long-lived peak. (ii) The 3A_g⁻(0) stimulated emission is weakly observed. (iii) The pure 1B_u⁺(0) → 1A_g⁻(0) stimulated emission is probably hidden in the diabatic 1B_u⁺(0) + 3A_g⁻(1) profile. The stimulated emission due to the 1B_u⁺(0) → 1A_g⁻(1) transition is not clearly seen at all, most probably it is overlapped with the 3A_g⁻(0) → 1A_g⁻(0) stimulated emission.

Thus, in terms of the quantum beat formalism, the 1B_u⁺(0) + X⁻(υ) stimulated emission is ascribable to the coherent cross term, while the 1B_u⁺(0) and the X⁻(0) stimulated emission, to the pair of split incoherent terms.

Finally, the key question is whether we can actually observe the real quantum beat: Figure 3 shows that the energy gap between the 1B_u⁺(0) and 3A_g⁻(1) pair of Car (n = 11) is around 300 cm⁻¹, whereas that between the 1B_u⁺(0) and 1B_u⁻(2) levels of Car (n = 10) is almost zero. Therefore, there is a good chance of observing the real quantum beat not in Car (n = 10) but in Car (n = 11). Figure 22 shows the time-dependent changes in the integrated intensity of stimulated emission from the 1B_u⁺(0) + 3A_g⁻(1) diabatic pair in Car (n = 11). After the subtraction of the background time profile, we can actually see the oscillatory changes in the fluorescence intensity. This result strongly supports our explanation of the observed spectral characteristics in terms of the quantum-beat mechanism.

As shown in Section 3.2, the coherent excitation of Cars (n = 9–13) in a polar solvent, THF, exhibited not only the long-lived stimulated emission from the 1B_u⁺(0) + X⁻(υ) diabatic pair but also the short-lived stimulated emission from the split 1B_u⁺(0) and X⁻(0) levels, which have been explained in terms of the quantum-beat mechanism. Therefore, we have tried to find whether the excited-state dynamics, after the coherent excitation of Cars (n = 9–11) that are bound to LH2 antenna complexes, is similar to, or different from, the excited-state dynamics free in THF solution.

Excited-state dynamics as revealed by time-resolved spectra and by the results of SVD and global-fitting analysis. Figure 23 shows the pump-probe time-resolved stimulated-emission and transient-absorption spectra of Cars (n = 9–11) bound to LH2 complexes from Rba. sphaeroides G1C, Rba. sphaeroides 2.4.1 and Rsp. molischianum. The time-resolved spectra can be characterized as follows:

(a) Cars (n = 9 and 10). Following the weak 1B_u⁺(0) stimulated emission, strong stimulated emission from the 1B_u⁺(0) + X⁻(υ) diabatic pair appears, giving rise to a broad peak or even clearly-split two peaks. Simultaneously, the 1B_u⁺(0) → 1A_g⁻(1) and the 1B_u⁻(0) → 1A_g⁻(0) weak stimulated emission peaks emerge. The set of stimulated emission components can be explained in terms of the quantum beat mechanism, as in the case of these Cars in THF solution. The latter pair of stimulated emission is replaced by the 1B_u⁻ transient absorption, and then by the combination of the mB_u⁺ ← 2A_g⁻ and T_n ← T₁ transient absorption peaks.

The above sequence of events can be proven by the SVD and global-fitting analysis of bound Car (n = 10), for example; the SADS and time-dependent changes in population are presented in Figure 24 (left-hand-side). The sequential transformation of Component 1 → Component 2 → Component 3 is ascribable to spectral transformation, i.e., a set of the 1B_u⁺ + 1B_u⁻, 1B_u⁺ and 1B_u⁻ stimulated emission → the 1B_u⁻ transient absorption → the 2A_g⁻ and T₁ transient absorption. The transformation is schematically presented in Figure 25 (in the middle).

(b) Car (n = 11). As shown in Figure 23, after the initial 1B_u⁺ emission (whose structure is not clear), the strong and extremely-broad pair of stimulated-emission signals ascribable to the 1B_u⁺(0) + 3A_g⁻(1) and 1B_u⁺(1) + 3A_g⁻(2) diabatic pairs appear. Simultaneously, a weak stimulated emission signal ascribable to the 3A_g⁻(0) → 1A_g⁻(0) transition appears and becomes replaced by the positive 1B_u⁻ transient-absorption signal. Eventually, it transforms into the 2A_g⁻ and T₁ transient-absorption signals.

The above sequence of events has been proven by the SVD and global-fitting analysis of the spectral data matrix, the results of which are shown in Figure 24 (right-hand-side): The sequential transformation of Component 1 → Component 2 → Component 3 is ascribable to spectral transformation i.e., the pair of the 1B_u⁺ + 3A_g⁻ and 3A_g⁻ stimulated emission → the 1B_u⁻ transient absorption → the 2A_g⁻ and T₁ transient absorption. The transformation is schematically presented in Figure 25 (on the right end).

The singlet-state energies of Cars (n = 9–11) when bound to the LH2 antenna complexes. Figure 26 compares the 1B_u⁺(0), 1B_u⁻(0) and 3A_g⁻(0) energies of Cars (n = 9–11) bound to the LH2 antenna complexes (crossed symbols) to those free in THF solution (open symbols). Surprisingly, the low-energy shift upon binding of the Cars is even larger in the covalent 1B_u⁻(0) and 3A_g⁻(0) levels than in the ionic 1B_u⁺(0) level. The results strongly suggest the polarization of the conjugated chain, which must enhance the electronic mixing of the diabatic pair.

Unique excited-state dynamics of Cars bound to LH2 complexes. The excited-state dynamics of the bound Cars (n = 9–11) can be characterized as follows: (a) The substantially-higher intensity of stimulated emission from the optically-forbidden 1B_u⁻(0) and 3A_g⁻(0) levels as well as the much broader stimulated emission from the 1B_u⁺(0) + X⁻(υ) diabatic pair strongly support the idea of enhanced polarization of the Car conjugated chain and the resultant stronger diabatic interaction. (b) The much faster decay of the initial stimulated emission after the coherent excitation of the diabatic pair obviously reflects the branching pathway to the Car-to-BChl singlet-energy transfer in addition to internal conversion within Car. This pathway of Car-to-BChl singlet-energy transfer has been established as introduced in Section 1.1. (c) The most conspicuous change, upon the binding of Cars, is the efficient triplet generation. We have already shown that the triplet generation is due to singlet heterofission from the 1B_u⁻ state [1]. The high efficiency of triplet generation suggests a substantial twisting around the C=C bonds in the Car conjugated chain when bound to the apo-peptides and BChls.

Our preliminary Kerr-gate fluorescence spectroscopy was found contradictory in our series of attempts to determine the 1B_u⁻ lifetime of neurosporene, Car (n = 9), for example: As described in Section 2.1, we obtained a value of 240 fs (Table 1) and a similar value of 265 fs [18] by excitation of this Car to the 1B_u⁺(0) level and probing by the use of the NIR white continuum. By subpicosecond time-resolved Raman spectroscopy, we obtained a value of 250 fs [19], whereas by fluorescence upconversion spectroscopy, a value of 270 fs, as the 1B_u⁻ lifetime after excitation to the 1B_u⁺(0) level [20]. Thus, the 1B_u⁻ lifetime has been consistently determined to be in the range of 240–270 fs.

In the previous Kerr-gate fluorescence spectroscopy, after excitation to the 1B_u⁺ (3) level, however, we obtained the 1B_u⁺(0) lifetime of 260 fs, the value of which agreed with the 1B_u⁻ lifetime [21]. This result confused us. Therefore, we have decided to examine a set of Cars (n = 9–12) after excitation at 12,500 cm⁻¹, which is just below and above the 1B_u⁺(3) level in Car (n = 9 and 10) and around the 1B_u⁺(4) level in Cars (n = 11 and 12). The results actually provided us with deeper insight into the unique excited-state properties of the diabatic pairs, which has turned out to be the reason for the apparent contradiction.

Figure 27 shows the time-resolved fluorescence spectra of Cars (n = 9–12). The spectra of the longer-chain Cars (n = 11 and 12) can be contrasted to those of the shorter-chain Cars (n = 9 and 10) as follows: (a) Fluorescence decays faster in the longer-chain Cars than in the shorter-chain Cars. (b) The spectral profile is more stretched and the relative intensity in the higher-energy region is enhanced in the longer-chain Cars than in the shorter-chain Cars. (c) In each Car, the fluorescence maximum shifts to the higher energies with time, but this trend is less pronounced in the longer-chain Cars than in the shorter-chain Cars. The time-dependent high-energy shift is ascribable to the Franck-Condon factors and reflects the vibrational relaxation in the 1B_u⁺ manifold (vide infra). Since the rate of vibrational relaxation from υ = ℓ to υ = ℓ–1 is proportional to the quantum number of the starting vibrational level, ℓ [22], hopefully, we would be able to time-resolve the last two steps of the slowest vibrational relaxations.

Figure 28 shows the results of the SVD and global-fitting analysis of spectral-data matrices by the use of a 3-component sequential model: The species-associated fluorescence spectra (SAFS) with reasonable S/N ratios (shown in the upper panels) nicely reflect the time-dependent changes in the fluorescence spectra (Figure 27). The decay time constants indicated on the time-dependent changes in population for the I, II and III components (shown in the lower panels) can be characterized as follows: (a) The lifetimes of components I and II are approximately in the ratio of 1:2, supporting their assignment to the 1B_u⁺(2) and 1B_u⁺(1) starting levels of vibrational relaxation in terms of the optically-allowed 1B_u⁺ counterpart. (b) The lifetimes of component III are 250 and 240 fs in Cars (n = 9 and 10), whereas 91 and 100 fs in Cars (n = 11 and 12); the values approximately agree with the 1B_u⁻ and 3A_g⁻ lifetimes of the corresponding the shorter-chain and the longer-chain Cars listed in Table 1. In the comparison of those values, we need to take into account the fact that the present result is just on the edge of our spectroscopic and analytical techniques.

Figure 29 shows the results of simulation for the fluorescence patterns obtained as a set of SAFS, which can be characterized as follows: (a) In Cars (n = 9 and 10), fluorescence patterns I and II can be simulated in terms of the Franck-Condon factors for the downward transitions from each of the 1B_u⁺ and 1B_u⁻ diabatic pairs (shown in red and blue lines), but fluorescence pattern III is dominated by transition from the 1B_u⁺(0) level. In the fluorescence pattern II of Car (n = 10), the contribution of the 3A_g⁻ transitions is also seen as expected from the energy diagram (Figure 1). (b) In Cars (n = 11 and 12), the broad fluorescence profiles, I, II and III, could be simulated by the Franck-Condon factors for transitions from the 1B_u⁺(2), 1B_u⁺(1) and 1B_u⁺(0) counterparts (shown in red) and by a pair of the 3A_g⁻ progressions designated as 3A_g⁻(l) and 3A_g⁻(m) (shown in green). As described in Section 2.3, we saw a single 3A_g⁻ progression in all-trans-β-carotene in polar solvent as well as 15-cis-β-carotene in polar and nonpolar solvents (Figure 14). Here, we temporarily ascribe the pair of progressions to the crystalfield splitting due to the intermolecular interaction of a pair of Car molecules in aggregates; note that we used a concentration as high as ∼10⁻⁴ M (facilitating aggregate formation) to record very weak fluorescence. Here, the contribution of the 3A_g⁻ fluorescence predominates not only in fluorescence profiles I and II, but also in fluorescence profile III.

Thus, the fluorescence patterns can be clearly classified into two groups: one, in the shorter-chain Cars (n = 9 and 10) and the other, in the longer-chain Cars (n = 11 and 12). Most importantly, we have obtained not only the 1B_u⁺-to-1B_u⁻ diabatic electronic mixing in the shorter-chain Cars but also the 1B_u⁺-to-3A_g⁻ diabatic electronic mixing in the longer-chain Cars (11 and 12). The results indicate that symmetry degradation takes place while the Car molecules are being vibronically excited, presumably due to the twisting of the conjugated chain around the C=C bond(s). Then, the symmetry selection rule concerning the diabatic electronic mixing (see Section 2.2) breaks down, and the 1B_u⁺-to-3A_g⁻ diabatic electronic mixing becomes allowed.

Now, we will try to explain why the lifetime of ‘the apparent 1B_u⁺(0) level’ agrees with the 1B_u⁻ lifetime in Cars (n = 9 and 10), whereas with the 3A_g⁻ lifetime in Cars (n = 11 and 12): Figure 30 presents the mechanisms: Here, each of the mixed diabatic pair is shown by a shadowed envelope, where the density of inclined lines is set proportional to the contribution of the optically-forbidden 1B_u⁻ or 3A_g⁻ counterpart. In considering the relaxation processes, we need to consider the selection rule in relation to the Pariser’s ± labels (see Section 1.2).

(a) In the shorter-chain Car (n = 9), for example, the vibrational relaxation, 1B_u⁺(2) + 1B_u⁻(3) → 1B_u⁺(1) + 1B_u⁻(2) → 1B_u⁺(0) + 1B_u⁻(1), takes place first. When the diabatic pair has reached to the bottom of the 1B_u⁺(0) potential, the allowed relaxation for the 1B_u⁺(0) counterpart is the instantaneous 1B_u⁺(0) emission, whereas the allowed relaxation for the 1B_u⁻(1) counterpart is the 1B_u⁻(1) → 2A_g⁻(4) internal conversion. Therefore, it is quite natural that the time constant of the latter process corresponds to the 1B_u⁻ lifetime. Actually, the allowed 1B_u⁻-to-2A_g⁻ internal conversion is taking place so efficiently from the upper 1B_u⁻ vibronic levels that the 1B_u⁻ population has been almost exhausted before the diabatic pair reaches to the bottom of the 1B_u⁺(0) potential.

(b) In the longer-chain Car (n = 11), for example, after the vibrational relaxation in the sequence of 1B_u⁺(2) + 3A_g⁻(3) → 1B_u⁺(1) + 3A_g⁻(2) → 1B_u⁺(0) + 3A_g⁻(1), the 1B_u⁺(0) stimulated emission and the 3A_g⁻(1) → 2A_g⁻(4) internal conversion are to take place; the former must take place instantaneously, while the latter, with the 3A_g⁻ lifetime. Here, the 3A_g⁻(1) level is still highly populated when the diabatic pair reaches to the bottom of the 1B_u⁺ potential.

This pair of observations reflects the unique excited-state properties of the diabatic pair consisting of the optically-allowed 1B_u⁺ counterpart and the optically-forbidden 1B_u⁻ or 3A_g⁻ counterpart. When the diabatic pair relaxes down to the bottom of the 1B_u⁺ potential, the 1B_u⁺ counterpart relaxes through emission, whereas the 1B_u⁻ or 3A_g⁻ counterpart relaxes through internal conversion. This is actually the splitting processes of the diabatic pair. The relative contribution of the optically-allowed and the optically-forbidden counterparts seems to vary in the processes of vibrational relaxation.

In this theoretical paper, multi-reference Møller-Plesset perturbation theory with complete active-space configurational interaction (CASCI-MRMP) was applied to calculate the energies of the vertical π → π* transitions of all-trans polyenes (n = 3–14), focusing on the nature of the four lowest-lying singlet-excited states and their ordering: It has been determined that the ionic 1B_u⁺ state is the lowest optically-allowed excited state, while the covalent 2A_g⁻, 1B_u⁻ and 3A_g⁻ states are the optically-forbidden states increasing in energy in this order. The calculations predict that the 1B_u⁻ state becomes lower than the 1B_u⁺ state at n ≥ 7, while the 3A_g⁻ state becomes lower than the 1B_u⁺ state at n ≥ 11.

It was a challenge for the theoreticians to carry out highly accurate ab initio calculations of the longer polyenes to realize the state ordering determined by the use of resonance-Raman excitation profiles. Before starting the calculations, the authors had demonstrated (in other molecular systems) that CASCI-MRMP was more efficient than, and comparable in accuracy to MRMP based on CASSCF reference functions.

To calculate the vertical excitation energies from the ground state to the relevant singlet states, the ground-state equilibrium geometries were optimized at the MP2 level. A reference CASCI wave function was obtained by partitioning the SCF orbitals, and optimizing the expansion coefficients of all configurations that were generated by all the possible arrangement of the active electrons among the active orbitals. The 10 valence π electrons were treated as active electrons. The effect of σ electrons was included through the perturbation calculation performed with MRMP, which was applied to each individual excited state.

In the present case of alternant hydrocarbons, the pairing properties are satisfied at the CASSCF and even the CAS-CI level. The 1A_g⁻, 1B_u⁺, 2A_g⁻, 1B_u⁻ and 3A_g⁻ states could be characterized by the use of it.

The calculated vertical-excitation energies did not exhibit a simple linear dependence on 1/(2n + 1) but fit to an exponential function, for fixed n₀, E n = E ∞ + ( E n 0 − E ∞ )   exp   [ − a   ( n − n 0 ) ]

Figure 31 shows an energy diagram for n = 9–13; approximate linear regression lines, as functions of 1/(2n + 1), are drawn for comparison to those in Figure 1. The state ordering of the four lowest-lying singlet states, i.e., 1B_u⁺, 2A_g⁻, 1B_u⁻ and 3A_g⁻, determined by the measurement of resonance-Raman excitation profiles (Figure 1) is in general agreement with that predicted by the highly accurate ab initio calculations including the σ- and π-electrons (Figure 31). The absolute values of the state energies and their dependence on n are still in poor agreement. When agreement between the observed and calculated state ordering becomes closer in the future, the results of calculations must provide us with a most reliable clue to confirm the symmetry notation of each singlet-excited state. It is much more straightforward to determine the symmetry of each excited state theoretically rather than spectroscopically, although the latter is ideal.

Following a preliminary report on β-carotene [33], Alfred Holzwarth and his coworkers have most recently reported the intensity fluctuation of transient absorption immediately after the excitation of lutein, i.e., Car (n = 10), to the 1B_u⁺ state and ascribed it to quantum beat due to coherence coupling between the 1B_u⁺ and 1B_u⁻ vibronic levels [34]. Oscillatory intensity changes were most pronounced in the 600–700 nm region as shown in Figure 32a. The oscillatory changes in the electronic absorption were simulated by a scheme consisting of five components, whose time-dependent changes in population are shown in Figure 32b. The results of simulation are overlaid on the time profiles in Figure 32a. Interestingly, the profile and magnitude of intensity changes were strongly dependent on the solvent, which probably reflect the shift of the 1B_u⁺ counterpart in energy. Also, they are strongly dependent on the wavelengths of excitation and detection.

To prove that the counterpart of the 1B_u⁺ state is the 1B_u⁻ state in the coherence coupling, the fluorescence pattern that does not exhibit the mirror image with respect to the electronic-absorption pattern (as shown in Figure 33a) was theoretically analyzed in lutein and β-carotene. The 1B_u⁺ and 1B_u⁻ energies and potentials have been theoretically determined as shown in Figure 33b. Most importantly, the pair of the 1B_u⁺ and 1B_u⁻ energy levels is almost iso-energetic and located close to the conical intersection, showing the reliability of their theoretical calculations.

The above results of analysis and interpretation in the case of β-carotene and lutein seem to be closely correlated to our case of bacterial Cars. In our terminology, it may be called ‘coherent excitation of the 1B_u⁺ + 1B_u⁻ diabatic pair’ in lutein.

It is also encouraging, that these authors proved the presence of the 1B_u⁻ state, which is coherently coupled with the 1B_u⁺ state. Detailed discussion on the nature of the 1B_u⁻ state and the mechanism of quantum beat based on their sophisticated theoretical calculations are described in their original literature. Such theoretical analysis combined with spectroscopic studies will reveal the more detailed mechanisms of diabatic electronic mixing and quantum beat.