Decoherence dynamics of coherent electronic excited states in the photosynthetic purple bacterium Rhodobacter sphaeroides

Decoherence dynamics of coherent electronic excited states in the photosynthetic purple bacterium Rhodobacter sphaeroides

Xian-Ting Liang111Email: xtliang@ustc.edu, Wei-Min Zhang222Email: wzhang@mail.ncku.edu.tw, and Yi-Zhong Zhuo Department of Physics and Institute of Modern Physics, Ningbo University, Ningbo, 315211, China
Department of Physics and Center for Quantum Information Science, National Cheng Kung University, Tainan 70101, Taiwan
National Center for Theoretical Science, Tainan 70101, Taiwan
China Institute of Atomic Energy, P.O. Box 275, Beijing 102413, China
Abstract

In this paper, we present a theoretical description to the quantum coherence and decoherence phenomena of energy transfer in photosynthesis observed in a recent experiment [see Science 316, 1462 (2007)]. As a successive two-color laser pulses with selected frequencies cast on a sample of the photosynthetic purple bacterium Rb. sphaeroides two resonant excitations of electrons in chromophores can be generated. However, this effective two-level subsystem will interact with its protein environment and decoherence is inevitable. We describe this subsystem coupled with its environment as a dynamical spin-boson model. The non-Markovian decoherence dynamics is described using a quasi-adiabatic propagator path integral (QUAPI) approach. With the photon-induced effective time-dependent level splitting energy and level flip coupling coefficient between the two excited states and the environment-induced non-Markovian decoherence dynamics, our theoretical result is in good agreement with the experimental data.

pacs:
67.57.Lm, 03.65.Yz, 31.15.Kb.

I Introduction

In the past decades, increasing attention has been paid to understand the intrinsic mechanisms of the efficient energy transfer in light harvesting complexes. In the previous investigations, the energy transfer was often described by a semiclassical model that invokes ‘hopping’ excited-state populations along discrete energy levels. Explicitly, the electrons in pigment molecules, chromophores, are excited by the incident light. Then the electronic excitation moves downhill from energy level to energy level through the chromophores before being trapped in the reaction center. However, it has not been conceived that the high efficient energy transfers between chromophores is realized through the electronic excited state hopping.

To understand the energy transfer among excited states of each chromophore in the Rhodobacter (Rb.) sphaeroides reaction centers, Fleming’s group proposed recently that the plants and the photosynthetic bacteria may utilize a ‘clever’ quantum algorithm for the energy transfer Science_316_1462 (); Nature_446_2007_782 (). Unlike the semiclassical model, Fleming and co-workers suggested that a successive excitations make a coherence superposition between electronic excited states of the chromophores. The energy transfer is considered to be carried by the coherence of the superposition state through an easiest route analogous to Grover’s algorithm for the fastest possible search of an unsorted information database PhysRevLett79_325_1997 (). However, Mohsehi et al. qu08064725 () argued that the standard Grover’s algorithm may not be applicable to the energy transfer mechanism in photosynthesis. Nevertheless, even if the plants and bacteria work unlike the Grover’s algorithm, the coherent dynamics evolution of the electronic excited states in chromophores could still play an important role in the chromophoric energy transfer NewJPhys10_113019_2008 (); PhysRevLett96_028103_2006 (). In this paper we shall derive a dynamical spin-boson model to describe how long the coherent superposition state can be persisted in the photosynthetic purple bacterium Rb. sphaeroides.

Ii Dynamical Spin-Boson Model

Recent experiments by Fleming group showed that the electronic coherence between two excited states may last for fs or longer Science_316_1462 (); Nature_446_2007_782 (). Instead of investigating the coherence among all excited states of each chromophores in the Rb. sphaeroides reaction centers PhysRevLett_92_2004_218301 (); PhysRevLett77_4675_1996 (), they investigated the coherent superposition state of two electronic excited states and in chromophores created experimentally from two successive laser pulses. The laser pulses (with wavelength nm and nm) derives the system which is initially in the ground state into a coherent superposition state However, the system of the two excited states inevitably interacts with its environment, which results in the decoherence of the coherent superposition state . To obtain the persistent time of coherence, i.e., the decoherence time of , Fleming et al. use the third incident pulse (with wavelength nm) to produce a photon echo. From the echo signals they extract the decoherence time of the coherent state PhysRevLett100_013603_2008 ().

To be specific, in the two-color photon echo experiment on bacterial reaction centers (RC) Science_316_1462 (), the RC from the photosynthetic purple bacterium Rb. sphaeroides includes a bacteriochlorophyll dimer, called the special pair (p), in the center, an accessory bacteriochlorophyll flanking p on each side (BChl), and a bacteriopheophytin (BPhy) next to each BChl. The RC of Rb. sphaeroides has several absorption peaks which are made by the chromophores. In Ref. Science_316_1462 (), the absorption spectrum of the p-oxidized RC at K shows the H band at nm and the B band at nm (where H and B are used to denote excitonic states which are dominatingly produced from monomeric BPhy and accessory BChl in the RC, respectively). At the first step, they used a successive two laser pulses with different colors and tuned for resonant excitation of H transition at nm (at time and the B transition at nm (at time cast on the sample. The two pulses produce a coherent superposition state between the electronic excited states and . Then, in order to measure the decoherence time of the coherent superposition of these two excited states, the third laser pulse is cast on the sample after a time from the second pulse, which generates a photon echo. When the times and are different one can detect the different integrated intensity of the echo signals in the phase matched direction. If the time is fixed (the fixed time fs in Ref. Science_316_1462 () ), the integrated echo signals as a function of represents the decoherence of the coherent superposition between and .

The evolutions of the integrated echo signals are plotted in the Fig. 3 of Ref. Science_316_1462 (). From the experimental data one can see that: (1) The coherence is resonant with different frequencies in the first fs. The first, the second and the third periods are about fs, fs, and fs respectively; (2) The coherence between the excited states and persists for more than fs; (3) The third peak in the evolution of the coherence decay more fast than the first and second peaks. In the following, we shall attempt to understand theoretically the dynamical process of excited electron states in chromophores and to explain the above experimental result. It is interesting to see, as we shall show later, that the problem can be described by a dynamical spin-boson model where the two excited states are time-dependently coupled one another through the laser pulses, as an effect of the photon-induced dynamics. To be explicit, we model the BChl and BPhy molecules by the Hamiltonian in the Condon approximation as Mukamel-book (); JChemPhys107_3876_1997 (); JChemPhys124_234504_2006 ()

(1)

Here, , , and are the energies of the ground state , the two excited states and , and the doubly excited state . is the electronic coupling between the two excited states. is the corresponding electronic dipole, and is the external electronic filed of the two successive laser pulses, namely, where are the decay constants of the laser pulses as they pass though the sample.

For simplicity, we assume that the dipole moments for the H and B states are the same: We can decouple the states from by making the following canonical transformation to Eq. (1):

(2)
(3)

where , , , and . Under the condition , we obtain

(4)

where, , , and . As one can see, the ground state and the doubly excited state are now decoupled from the single excited states and . Thus the decoherence dynamics of the coherent superposition state is fully determined by the effective two-level Hamiltonian, the second curly bracket in Eq. (4) which can be rewritten as

(5)

Here, are the Pauli matrix, , . It shows that the energy splitting of the two excited states and the coupling between them are shifted by the pulse-induced time-dependent dipole-dipole interaction [], as an effect of photon-induced dynamics.

Furthermore, this two-level system, as a part of chromophores, is inevitable to interact with its protein environment through the thermal vibrations. This thermal reservoir can always be modeled with a set of harmonic oscillators. Then the total system of the two-level system coupled to its environment can be written as a dynamical spin-boson model,

(6)

in which the last two terms are the interaction between the two-level system and the bath and the Hamiltonian of the thermal bath itself, respectively. The parameter is the coupling of the system to the bath and ( are the creation (annihilation) operators of the -th thermal mode. The decoherence dynamics of the above two-level system are mainly induced by the back-actions of the thermal bath as well as the decay of the time-dependent coupling induced by laser pulses. The solution of the problem is now completely determined by the parameters and the spectral density of the thermal bathRevModPhys_59_1 ()

(7)

Here is the high-frequency cut-off of the bath modes. Different correspond to the super-Ohmic , the Ohmic , and the sub-Ohmic baths, and is a dimensionless dissipative parameter describing the coupling between the two-level system and the bath.

Iii Numerical Method

The spin-boson model has been investigated by many methods though it has not be exactly solved and some approximation, such as the Markov approximation, must be used Weiss (); RevModPhys_59_1 (). Here, we shall apply the quasiadiabatic propagator path integral (QUAPI) technique ChemPhysLett_221_482 () to explore the decoherence dynamics of this system, where non-Markovian processes are involved. Indeed, as it has been pointed out Science_316_1462 () the evolution of this time-dependent system should be highly non-Markovian. To see how the non-Markovian dynamics may play an important role, it is useful to estimate the correlation time of the thermal bath, which can be obtained from the bath response function

(8)

where with Boltzmann’s constant and the temperature . When the real and imaginary parts of behave as a delta function and its derivative , respectively, the dynamics of the reduced density matrix is Markovian. Otherwise, non-Markovian dynamics occurs. The broader the Re and Im are, the longer the correlation time will be, and the more serious the practical dynamics is distorted by the Markov approximation. Similar to Ref. PhysRevB_72_245328 (), we calculate the correlation times of the bath. The result is shown in Fig. 1. As we can see the correlation time of the bath is about fs which actually depends on the frequency cutoff in the bath.

Figure 1: (Color online) Real and imaginary parts of the response functions () for Ohmic bath. Here, we take cm and K

The decoherence dynamics of the coherent superposition states is characterized by the time evolution of the reduced density matrix obtained after tracing out the bath degrees of freedom, i.e.,

(9)

Following the experiment, the interaction between system and bath is turned on at when the second laser pulse is applied. Thus, the density matrix of the total system before the time is a direct product of the system and bath components, namely, where and are the ”initial” states of the system and the bath at . If we set , the initial resonant two excited state can be written as . After the canonical transformation, the initial state remains almost the same: under the condition which is satisfied for the parameters we taken in the following numerical calculations. We also set the bath initially at the thermal equilibrium, namely, Tr.

The reduced density matrix can be evaluated by using the well established iterative tensor multiplication (ITM) algorithm derived from the QUAPI. This algorithm is numerically exact and successfully tested and adopted in various problems of open quantum systems JChemPhys_102_4600 (); PhysRevE_62_5808 (). For details of the scheme, we refer to previous works ChemPhysLett_221_482 (). The QUAPI asks for the system Hamiltonian splitting into two parts and , where . In order to make the calculations converge we use the time step fs which is shorter than the correlation time of the bath and the characteristic time of the two-level subsystem. In order to include all non-Markovian effect of the bath in the ITM scheme, one should choose so that is not much shorter than the correlation time of the bath. Here, is roughly equal to the number of time steps needed to span the half-width of the response function ChemPhysLett_221_482 (). Then taking should be large enough in our calculations.

Iv Results and discussions

The decoherence of the two exciton states is reflected through the decays of the off-diagonal reduced density matrix element. In Fig. 2a and b we plot the evolution of the off-diagonal reduced density matrix element at temperature K and K, respectively, where the environment is assumed as an Ohmic bath (), and the parameters cm cm cm cm, cm and s. We take the Kondo parameter and the frequency cutoff cm PNAS93_3926_1996 () for the thermal bath. According to Ref. Science_316_1462 (), we take fs, and fs.

Figure 2: (Color online) The evolutions of the off-diagonal coherent terms of the reduced density matrix for the two-level subsystem with the Ohmic bath at temperature (a) K and (b) K.

The black square boxes in Fig. 2 are the experimental data from Science_316_1462 (), the linked blue and red dots are our numerical results. The plots show that our theoretical description is in good agreement with the experimental results. As we see the coherence decay is much faster after the second peak and the oscillation periods of the evolutions increase with the time. The oscillation dephasing behaviors indeed come from the time-dependent level splitting and coupling induced by laser pulses as well as the non-Markovian processes due to the interaction between the two-level system and the thermal bath.

Further calculations show that using the sub-Ohmic bath with and super-Ohmic bath with , we can obtain the similar results, as show in Fig. 3a. However, if we use the same value of the dimensionless dissipative parameter for the Ohmic, sub-Ohmic and super-Ohmic spectral densities, the corresponding decoherence behaviors are completely different. This indicates that the decoherence dynamics is non-Markovian. To show the non-Markovian effect, we also calculate the Markov approximation with the same parameters in the Ohmic case. The detailed numerical results are plotted in Fig. 3b, where the difference between the non-Markovian dynamics and the corresponding Markov approximation is obvious.

Figure 3: (Color online) The evolutions of the off-diagonal coherent terms of the reduced density matrix for the two-level subsystem in sub-Ohmic and super-Ohmic Baths. Here, we set and at K. Other parameters are the same as that in Fig. 2

We should also point out that the bare level splitting is not the experimentally observed values. The experimental values ( cm) of the level splitting contains the pulse-induced time-dependent effects plus the back-action effect from the environment in the non-Markovian regime so that the input value of is different from the splitting of experimental linear absorbance peaks. A practical calculation of the true site energy difference that contains all the the pulse-induced time-dependent effects plus the back-action effect from the environment may be possible Ado062778 () but it is beyond the scope of the present investigation. Here the input value of the bare level splitting is based on how better to fit the experimental data. Our numerical calculations show that the profiles of the evolution curves for the off-diagonal reduced density matrix elements are sensitive to the changes of the bare level splitting , the bare coupling and the parameter but insensitive to the changes of and with cm. In Fig. 4, we plot the time evolution of off-diagonal reduced density matrix element with different . As we can see, the change of the bare level splitting produces a quite different pattern of the decoherence dynamics. A smaller value of will result in a shorter oscillation period of the evolution in time.

Figure 4: (Color online) The evolutions of the off-diagonal coherent terms of the reduced density matrix in Ohmic bath, with different bare level splitting cm at K. Other parameters are the same as that in Fig. 2

Also, the bare electronic coupling between the exciton states and is not the electronic coupling between the BChl and BPhy molecules that used in Science_316_1462 (). Our numerical results suggest that is much smaller ( cm) than the pulse-induced dipole-dipole interaction but is not negligible. Change of leads to very different decoherence behavior as shown in Fig. 5, which is actually also convinced in the supplemental material of Science_316_1462 (). The resulting effective electronic coupling oscillates in time with the maximum amplitude being less than cm

Figure 5: (Color online) The evolutions of the off-diagonal coherent terms of the reduced density matrix for the two-level subsystem in Ohmic bath at K, with different bare electronic coupling , and cm. Other parameters are the same as that in Fig. 2.

As one can see, our numerical result shows that the oscillation of the off-diagonal reduced density matrix element is due to the effective time-dependence of the level splitting and flip coupling between the two excitonic states induced by the laser pulses. This differs from the interpretation given in Science_316_1462 () where it has been pointed out that reproducing the long dephasing time observed would require a value of cm, but a large implies that the BChl and BPhy excitations are almost degenerate, which may not be consistent with the observed spectra. Therefore they argued that the vibrational modes begin to contribute in the energy transfer. Their simulation shows that a vibrational mode (with a frequency cm) coupling to the excitonic states can fit the long dephasing time very well. Here we show that the large effective coupling between the two excited states induced by the laser pulses combining with a very smaller but not negligible bare coupling can reproduce the long dephasing time observed, without including the contribution arisen from the vibrational mode.

On the other hand, the level splitting and flip coupling we derived explicitly depend on the parameter . The dipole moment (debye) where the dipole strength can be estimated by: Kno03497 (). Here is the refractive index, and are the half-width and the peak value at nm and nm for H and B excited states, respectively. Fig. 1 of Science_316_1462 () shows that and . Taking debye (corresponding to debye for 800 nm BChl Sch8621 ()), we have debye. Averaging the dipole strength for BChl and BPhy, we obtain debye C cm. The power intensity used in Fleming’s experiment Science_316_1462 () is J/cm while the pulse duration fs. Therefore the pulse intensity is W/cm which corresponds to a pulse field amplitude V/cm. Thus, the realistic dipole-field coupling strength cm. This is very close to the value of our theoretical best fitting cm in the numerical calculation. We also find that the laser pulse strength controls the decay curves. In Fig. 6, we plot the evolution of the off-diagonal reduced density matrix element to demonstrate the -dependence of the dephasing time. It shows that increasing will decrease the oscillation periods of the evolution in time, and vice versa. This property may be used for further experimental test of whether the pulse-induced time-dependent dipole-dipole interaction or the additional vibrational mode gives rise to the oscillation decay of the coherent excitonic states.

Figure 6: (Color online) The evolutions of the off-diagonal coherent terms of the reduced density matrix for the two-level subsystem with different pulse field strength, and cm, in Ohmic bath at K . Other parameters are the same as that in Fig. 2

In conclusion, we present in this paper a dynamical spin-boson model with the effective time-dependence of the level splitting and flip coupling between the two excited states, induced by laser pulses, to describe the long dephasing time observed recently in a photosynthesis experiment Science_316_1462 (). We use the quasi-adiabatic propagator path integral approach to analyze in detail the non-Markovian decoherence behaviors of the two excitonic states, and . Due to the photon-induced time-dependence of the energy level splitting and flip coupling coefficient between the two excited states and the environment-induced non-Markovian dynamics, our theoretical result is in good agreement with the experimental data.

Acknowledgements.
We would like to thank Prof. Fleming for sending us their experimental data for comparisons. This project was sponsored by National Natural Science Foundation of China (Grant No. 10675066), the National Science Council of ROC under Contract No. NSC-96-2112-M-006-011-MY3, and K.C.Wong Magna Foundation in Ningbo University.

References

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