Excitonic linewidth and coherence lifetime in monolayer transition metal dichalcogenides

Excitonic linewidth and coherence lifetime in monolayer transition metal dichalcogenides

Malte Selig    Gunnar Berghäuser    Archana Raja    Philipp Nagler    Christian Schüller    Tony F. Heinz    Tobias Korn    Alexey Chernikov    Ermin Malic    Andreas Knorr Institut für Theoretische Physik, Technische Universität Berlin, 10623 Berlin, Germany Department of Chemistry, Columbia University, New York, New York 10027, USA Department of Applied Physics, Stanford University, Stanford, California 94305, USA Institut für Experimentelle und Angewandte Physik, Universität Regensburg, 93040 Regensburg, Germany SLAC National Accelerator Laboratory, Menlo Park, California 94025, USA Departments of Physics and Electrical Engineering, Columbia University, New York, New York 10027, USA Chalmers University of Technology, Department of Physics, SE-412 96 Gothenburg, Sweden
Abstract

Atomically thin transition metal dichalcogenides (TMDs) are direct-gap semiconductors with strong light-matter and Coulomb interaction. The latter accounts for tightly bound excitons, which dominate the optical properties of these technologically promising materials. Besides the optically accessible bright excitons, these systems exhibit a variety of dark excitonic states. They are not visible in optical spectra, but can strongly influence the coherence lifetime and the linewidth of the emission from bright exciton states. In a recent study, an experimental evidence for the existence of such dark states has been demonstrated, as well as their strong impact on the quantum efficiency of light emission in TMDs. Here, we reveal the microscopic origin of the excitonic coherence lifetime in two representative TMD materials (WS and MoSe) within a joint study combining microscopic theory with optical experiments. We show that the excitonic coherence lifetime is determined by phonon-induced intra- and intervalley scattering into dark excitonic states. Remarkably, and in accordance with the theoretical prediction, we find an efficient exciton relaxation in WS through phonon emission at all temperatures.  
 

As truly two-dimensional materials exhibiting a weak dielectric screening, monolayer transition metal dichalcogenides (TMDs) show a remarkably strong Coulomb interaction giving rise to the formation of tightly bound excitons.He et al. (2014); Chernikov et al. (2014); Berghäuser and Malic (2014); Ramasubramaniam (2012) In addition to the optically accessible bright excitonic states located at the and points at the corners of the hexagonal Brillouin zoneMak et al. (2010); Splendiani et al. (2010); Radisavljevic et al. (2011); Lee et al. (2010), there is also a variety of optically forbidden states including p excitons exhibiting a non-zero angular momentum, intravalley excitons with a non-zero center-of-mass momentum above the light cone as well as intervalley excitons, where a hole is located at the point and the electron either at the or the point,Qiu et al. (2015); Wu et al. (2015); Steinhoff et al. (2015) cf. Fig. 1. In a recent time-resolved and temperature-dependent photoluminescence study, the existence of such dark intervalley excitons has been experimentally demonstrated.Zhang et al. (2015) In particular, it was shown that in tungsten-based TMDs, the intervalley dark exciton lies energetically below the optically accessible exciton resulting in a strong quenching of photoluminescence at low temperatures.Arora et al. (2015); Zhang et al. (2015)

Since excitons dominate the optical response of TMDs, a microscopic understanding of their properties is of crucial importance for their promising technological application in future optoelectronic and photonic devices. The presence of dark states has a strong impact on the coherence lifetime of optically accessible states, since they present a possible scattering channel that can be accessed via emission or absorption of phonons. The coherence lifetime in two-dimensional TMDs is directly reflected by the homogeneous linewidth of excitonic resonances that is experimentally accessible in optical absorption and emission spectra.Kira and Koch (2006) The homogeneous linewidth in monolayer WSe has been recently measured via optical 2D Fourier transform spectroscopy allowing an unambiguous separation from inhomogeneous broadening.Moody et al. (2015) G. Moody et al. find, for temperatures up to 50 , a linear increase of the homogeneous linewidth in the range of 4  to 10 . Further studies show an increase of the linewidth up to 40  in MoTe and 65  in MoS at room temperature. Koirala et al. (2016); Dey et al. (2016) The observed increase is ascribed to scattering with acoustic phonons within the valley. Phonon-induced scattering into dark intervalley exciton states has not been considered. However, a consistent microscopic theory description of these observations is not available so far.

Figure 1: Relaxation channels determining the excitonic lifetime. (a) Minima of the excitonic center of mass motion () dispersion . An exciton at the point can decay via radiative (blue arrow) or non-radiative dephasing . The latter occurs through exciton-phonon scattering within the valley (orange) or to dark excitonic states at the (red) or the valley. For WS, the intervalley and excitons lie energetically below the exciton () allowing efficient scattering via emission of phonons even at very low temperatures.The dashed dispersion curves refer to a situation typical in MoSe, where . (b) An exciton at the (,) point is formed by an hole (red) at the point and an electron (blue) at the (,) point.

Here, we present a joint theory-experiment study aiming at a fundamental understanding of microscopic processes determining the excitonic coherence lifetime in TMDs. In the experiment, we use optical spectroscopy to extract temperature-dependent homogeneous linewidths from the total broadening of the exciton resonances in TMD monolayers. Our theoretical approach is based on the Bloch equation for the microscopic polarization combined with the Wannier equation providing access to eigenvalues and eigenfunctions for bright and dark excitons. The joint study reveals the qualitatively different microscopic channels behind the excitonic coherence lifetime in tungsten- and molybdenum-based TMDs: In MoSe, the coherence lifetime is determined by radiative coupling at low temperatures and by phonon-induced intravalley scattering at room temperature. In contrast, the excitons in WS can be efficiently scattered into the energetically lower-lying intervalley dark excitonic state, cf. Fig. 1. This process is driven by phonon emission that is very efficient even at low temperatures. Note, that we focus on spin-conserving processes, occurring on an ultrashort time scale (tens of femtoseconds) in this study. Intervalley scattering via exchange interaction occurs on a much longer time scale (picosecondsGlazov et al. (2014); Song and Dery (2013)) for supported samples. To describe the coherence lifetime of optically bright excitons, we develop a theoretical model including all relevant relaxation channels on a microscopic footing. Furthermore, to test the theory, we perform experiments on WS and MoSe monolayers using a combination of linear reflectance and photoluminescence spectroscopy. From the obtained total linewidths of the exciton transitions we estimate temperature-dependent homogeneous broadening of the resonances corresponding to the coherence lifetime of the excitons. Our analysis is also consistent with recent reports on total exciton linewidths in MoSeArora et al. (2015), as well as with the behavior of a similar TMD material WSe studied through coherent spectroscopy at low-temperatures Moody et al. (2015) and under resonant excitation conditions Poellmann C. et al. (2015) (Additional details for the experimental procedure and data analysis are given in the Methods section).

The first step of the theoretical evaluation is the solution of the Wannier equation Berghäuser and Malic (2014); Axt and Kuhn (2004); Haug and Koch (); Kira and Koch (2006)

(1)

presenting an eigenvalue equation for excitons in TMDs. It includes the excitonic part of the Coulomb interaction that is treated within the Keldysh formalism for 2D systems.Berghäuser and Malic (2014); Cudazzo et al. (2011) We obtain excitonic eigenenergies and excitonic wavefunctions for optically allowed bright and optically forbidden dark excitons that are denoted by the quantum number . The wavefunctions depend on the momentum describing the relative motion of electrons () and holes () in real space, where and with effective masses for electrons and holes .

The second step is to derive a Bloch equation for the microscopic polarization that determines the optical response of the material. The quantity reads in the excitonic basisThränhardt et al. (2000) with as annihilation (creation) operators for an electron in the state with the band index and being the quantum number of the exciton state. Here, we also have introduced the in-plane momentum denoting the Fourier coordinate of the center-of-mass motion in real space. The electronic dispersion is assumed to be parabolic, which is a good approximation in the vicinity of the point. This results in a quadratic dispersion for the excitons which constitutes the lowest excitonic contributionQiu et al. (2015); Wu et al. (2015) addressed in a coherent optical transmission experiment with fixed polarization. We focus here on the energetically lowest intravalley and intervalley excitons numbered by , i.e. the bound electron and hole are either both located at the point (intravalley), or only the hole is at the point, while the electron is either in the or in the point in the first Brillouin zone, cf. Fig. 1. Since a photon has a negligibly small center-of mass momentum , only excitons with are optically accessible. As a result, all intervalley excitons are dark.

Applying Heisenberg’s equation of motion we can determine the temporal evolution of the microscopic polarization . The Hamilton operator includes (i) an interaction-free part containing the dispersion of electrons and phonons, (ii) the carrier-light interaction determining the optical selection rules, (iii) the carrier-carrier interaction that has already been considered in the Wannier equation, and (iv) the carrier-phonon interaction coupling bright and dark excitons via emission and absorption of phonons. The carrier-light coupling is considered within the semi-classical approach in gauge Malic and Knorr (). The coupling is determined by the optical matrix element projected to the right-handed circular polarized light that is required to excite excitons at the point.Zeng et al. (2012); Cao et al. (2012); Berghäuser and Malic (2014); Xu et al. (2014) The carrier-phonon matrix element is treated within an effective deformation potential approach for acoustic phonons and approximating the Fröhlich interaction for optical phonons.Li et al. (2013); Jin et al. (2014)

Evaluating the commutator in the Heisenberg equation of motion, we obtain in second-order Born-Markov-approximationThränhardt et al. (2000) the Bloch equation for the microscopic polarizations

(2)

While the first term describes the oscillation of the excitonic polarization determined by the excitonic dispersion in , the second term stands for the carrier-light interaction given by the Rabi frequency with the vector potential and the electron charge and mass . The third contribution in equation (2) describes the exciton-phonon-interaction that is given by the function

(3)

Here, is the phonon energy and the phonon occupation in the mode corresponding to the Bose-Einstein distribution. The function contains scattering processes including phonon emission () and absorption (). The exciton-phonon coupling depends on the electron-phonon matrix element and the overlap of the involved exciton wavefunctions in momentum space. The corresponding phonon-induced homogeneous dephasing of the excitonic polarization readsThränhardt et al. (2000)

(4)

giving rise to a non-radiative coherence lifetime for excitons with momentum in the state . Here, we take into account acoustic (LA, TA) and optical phonons (LO, TO),Jin et al. (2014) explicitly considering intravalley scattering between bright () and dark excitonic states () as well as intervalley scattering involving dark and excitons, cf. Fig. 1. To evaluate the exciton-phonon scattering rates, we calculate the rate self-consistently, which corresponds to a self-consistent Born approximation.Schilp et al. (1994); Haug and Jauho (2008)

Besides the exciton-phonon scattering, the coherence lifetime of excitons is also influenced by radiative coupling, i.e. spontaneous emission of light through recombination of electrons and holes. The radiative coupling is obtained by self-consistently solving the Bloch equation for the excitonic polarization and the Maxwell equations in a two dimensional geometry for the vector potential yieldingKnorr et al. (1996)

(5)

Here, is the light velocity in the substrate material and the vacuum permeability.

Figure 2: Homogeneous broadening and coherence lifetime. Absorption spectrum of (a) WS and (b) MoSe focusing on the energetically lowest resonance of the A exciton. All spectra were normalized to their peak maximum. While the blue line only includes the radiative linewidth, the other lines contain also non-radiative contributions due to exciton-phonon scattering at different temperatures. Absolute value of the microscopic polarization for (c) WS and (d) MoSe. The filled curve illustrates a 10  excitation pulse at .

Having solved the Wannier equation, equation (1), and the Bloch equation, equation (2), we have access to the optical response of TMDs and can evaluate the radiative and non-radiative homogeneous linewidth of excitonic resonances reflecting the coherence lifetime of optically allowed excitons. Figure 2 illustrates the absorption spectrum of two dimensional sheets Knorr et al. (1996) of two exemplary monolayer TMDs including tungsten diselenide (WS) and molybdenum diselenide (MoSe). We predict the homogeneous linewidth of the energetically lowest A exciton to be in the range of a few meV corresponding to an excitonic coherence lifetime of a few hundreds of femtoseconds. Depending on the temperature, either the radiative or the non-radiative contribution is the dominant mechanism. We observe a larger radiative broadening in WS (7  vs. 4  for MoSe), while the overall broadening at room temperature is larger for MoSe with 40  vs 24  in WS. Furthermore figure 2 shows the temporal evolution of the excitonic polarization after optical excitation with a 10  pulse. We find that the polarization decays radiatively with a time constant in the range of hundreds of fs. Including exciton-phonon coupling the time constant decreases drastically to some tens of fs at room temperature. Evaluating equations (4) and (5), we can reveal the microscopic origin of the excitonic linewidth. Figure 3 shows the temperature dependence of the linewidth depending on the nature of the coupling mechanism. Further, we show the corresponding exciton coherence lifetime which is connected by , with being the full linewidth. We find an excellent agreement between theory and experiment with respect to qualitative trends as well as quantitative values for the linewidths.

In both investigated TMD materials, we observe a temperature-independent offset originating from radiative recombination. In contrast, the non-radiative coupling via scattering with phonons introduces a strong temperature dependence. Furthermore, we find a remarkably different behavior for MoSe and WS: While for MoSe intravalley exciton-phonon scattering is the crucial mechanism, the excitonic coherence lifetime in WS is dominated by intervalley scattering , coupling the optically allowed exciton with the dark states. The reason lies in the relative energetic position of these excitons. In WS, the exciton is located approximately 70  below the exciton. Hence, exciton relaxation through phonon emission is very efficient even at 0 K resulting in a non-radiative offset in the homogeneous linewidth at low temperatures, cf. Fig. 3(a). The coupling to excitons does not significantly contribute due to the weak electron-phonon coupling element.Jin et al. (2014)

Figure 3: Excitonic linewidth and lifetime. Temperature dependence of the linewidth and lifetime of the A exciton in (a) WS and (b) MoSe in dependence of temperature. The red points with error bars describe the experimental data. The thick red line shows the total linewidth consisting of the single contributions from the radiative decay (blue) and non-radiative decay including intravalley exciton-phonon coupling (orange) as well as intervalley coupling (only shown in the total contribution) and (dashed orange). Note that the latter contribution is very small.

The situation is entirely different in MoSe, where the dark exciton lies approximately 100  above the bright exciton. Thus, only the less efficient absorption of phonons can take place. Since the energy of large-momentum acoustic phonons,required for scattering excitons into states, is only 15  in this material,Jin et al. (2014) the only contribution of intervalley scattering in MoSe stems from the absorption of optical phonons and becomes relevant for temperatures higher than 150K, cf. Fig. 3(b). Our calculations show that the intravalley scattering with acoustic phonons is the crucial mechanism for the excitonic coherence lifetime in MoSe. We observe a linear increase of the linewidth with temperature. Since acoustic phonons have small energies, the Bose-Einstein distribution appearing in equation (3) can be linearized resulting in a dephasing rate exhibiting a linear dependence on the temperature . The slope is given by the exciton mass , the velocity of the acoustic phonons , and the exciton-phonon coupling element at the position , where the delta distribution is fulfilled, cf. equation (3).

The super-linear increase of the linewidth with temperature observed for both MoSe and WS can be ascribed to the scattering with optical or phonons. The overall temperature dependence of the excitonic linewidth can be approximated by For WS, we find a temperature-independent offset of =9.1  consisting of 7  due to radiative decay and 2.1  due to acoustic phonon emission, furthermore the slope describing the linear increase due to acoustic phonons, the rate and the averaged energy of involved acoustic phonons determining the strength of the superlinear increase. We find that optical phonons do not give a contribution to the superlinear increase. The corresponding parameters for MoSe read , , ( due to intravalley optical phonon scattering and due to coupling), and . Our results for the radiative dephasing are in good agreement with recent calculations.Wang et al. (2016)

In conclusion, we have presented a joint theory-experiment study revealing the microscopic origin of the excitonic lifetime in atomically thin 2D materials. We find both in theory and experiment a qualitatively different origin of the coherence lifetime limiting processes in tungsten- and molybdenum-based TMDs. While in MoSe, the coherence lifetime of an optically bright exciton is determined by intravalley scattering with acoustic phonons, in WS scattering into dark excitonic states is crucial. The gained insights shed light into excitonic properties that are crucial for exploiting the technological potential of these atomically thin nanomaterials. In particular, it will allow us to access exciton dynamics on a microscopic level across a large variety of relevant experimental scenarios, including exciton formation, thermalization and relaxation among many others. The presented theoretical approach can be furthermore generalized to quantitatively describe exciton behavior for the whole family of semiconducting 2D materials beyond the representative systems studied here. It provides a theoretical basis to explore fundamental many-body physics of 2D materials, crucial for future applications and allowing for consistent theoretical predictions of the functionality for novel devices on inter-atomic scales.

Acknowledgements

We acknowledge financial support from the Deutsche Forschungsgemeinschaft (DFG) through SFB 951 (A.K.) SFB 787 (M.S.), SFB 689 (T.K. and C.S.), GK 1570 (P.N.), Emmy Noether Program (A.C.) and the EU Graphene Flagship (CNECT-ICT-604391)(E.M.,G.B.). This work was further supported by the U.S. Department of Energy, Office of Science, Office of Basic Energy Sciences, with funding at Columbia University through the Energy Frontier Research Center under grant DE-SC0001085 for optical measurements and at SLAC National Accelerator Laboratory through the AMOS program within the Chemical Sciences, Geosciences, and Biosciences Division for data analysis. A.C. gratefully acknowledges funding from the Keck Foundation.



References

  • He et al. (2014) K. He, N. Kumar, L. Zhao, Z. Wang, K. F. Mak, H. Zhao,  and J. Shan, Phys. Rev. Lett. 113, 026803 (2014).
  • Chernikov et al. (2014) A. Chernikov, T. C. Berkelbach, H. M. Hill, A. Rigosi, Y. Li, O. B. Aslan, D. R. Reichman, M. S. Hybertsen,  and T. F. Heinz, Phys. Rev. Lett. 113, 076802 (2014).
  • Berghäuser and Malic (2014) G. Berghäuser and E. Malic, Phys. Rev. B 89, 125309 (2014).
  • Ramasubramaniam (2012) A. Ramasubramaniam, Phys. Rev. B 86, 115409 (2012).
  • Mak et al. (2010) K. F. Mak, C. Lee, J. Hone, J. Shan,  and T. F. Heinz, Phys. Rev. Lett. 105, 136805 (2010).
  • Splendiani et al. (2010) A. Splendiani, L. Sun, Y. Zhang, T. Li, J. Kim, C.-Y. Chim, G. Galli,  and F. Wang, Nano Letters 10, 1271 (2010).
  • Radisavljevic et al. (2011) B. Radisavljevic, A. Radenovic, J. Brivio, V. Giacometti,  and A. Kis, Nat Nano 6, 147 (2011).
  • Lee et al. (2010) C. Lee, H. Yan, L. E. Brus, T. F. Heinz, J. Hone,  and S. Ryu, ACS Nano 4, 2695 (2010).
  • Qiu et al. (2015) D. Y. Qiu, T. Cao,  and S. G. Louie, Phys. Rev. Lett. 115, 176801 (2015).
  • Wu et al. (2015) F. Wu, F. Qu,  and A. H. MacDonald, Phys. Rev. B 91, 075310 (2015).
  • Steinhoff et al. (2015) A. Steinhoff, J.-H. Kim, F. Jahnke, M. Rösner, D.-S. Kim, C. Lee, G. H. Han, M. S. Jeong, T. O. Wehling,  and C. Gies, Nano Letters 15, 6841 (2015).
  • Zhang et al. (2015) X.-X. Zhang, Y. You, S. Y. F. Zhao,  and T. F. Heinz, Phys. Rev. Lett. 115, 257403 (2015).
  • Arora et al. (2015) A. Arora, M. Koperski, K. Nogajewski, J. Marcus, C. Faugeras,  and M. Potemski, Nanoscale 7, 10421 (2015).
  • Kira and Koch (2006) M. Kira and S. Koch, Progress in Quantum Electronics 30, 155 (2006).
  • Moody et al. (2015) G. Moody, D. C. Kavir, K. Hao, C.-H. Chen, L.-J. Li, A. Singh, K. Tran, G. Clark, X. Xu, G. Berghauser, E. Malic, A. Knorr,  and X. Li, Nat Commun 6 (2015).
  • Koirala et al. (2016) S. Koirala, S. Mouri, Y. Miyauchi,  and K. Matsuda, Phys. Rev. B 93, 075411 (2016).
  • Dey et al. (2016) P. Dey, J. Paul, Z. Wang, C. E. Stevens, C. Liu, A. H. Romero, J. Shan, D. J. Hilton,  and D. Karaiskaj, Phys. Rev. Lett. 116, 127402 (2016).
  • Glazov et al. (2014) M. M. Glazov, T. Amand, X. Marie, D. Lagarde, L. Bouet,  and B. Urbaszek, Phys. Rev. B 89, 201302 (2014).
  • Song and Dery (2013) Y. Song and H. Dery, Phys. Rev. Lett. 111, 026601 (2013).
  • Poellmann C. et al. (2015) Poellmann C., Steinleitner P., Leierseder U., Nagler P., Plechinger G., Porer M., Bratschitsch R., Schuller C., Korn T.,  and Huber R., Nat Mater 14, 889 (2015).
  • Axt and Kuhn (2004) V. M. Axt and T. Kuhn, Reports on Progress in Physics 67, 433 (2004).
  • (22) H. Haug and S. W. Koch, Quantum Theory of the Optical and Electronic Properties of Semiconductors (5th ed. (World Scientific Publishing Co. Pre. Ltd., Singapore, 2004).).
  • Cudazzo et al. (2011) P. Cudazzo, I. V. Tokatly,  and A. Rubio, Phys. Rev. B 84, 085406 (2011).
  • Thränhardt et al. (2000) A. Thränhardt, S. Kuckenburg, A. Knorr, T. Meier,  and S. W. Koch, Phys. Rev. B 62, 2706 (2000).
  • (25) E. Malic and A. Knorr, Graphene and Carbon Nanotubes: Ultrafast Optics and Relaxation Dynamics (1st ed. (Wiley-VCH, Berlin, 2013)).
  • Zeng et al. (2012) H. Zeng, J. Dai, W. Yao, D. Xiao,  and X. Cui, Nat Nano 7, 490 (2012).
  • Cao et al. (2012) T. Cao, G. Wang, W. Han, H. Ye, C. Zhu, J. Shi, Q. Niu, P. Tan, E. Wang, B. Liu,  and J. Feng, Nat Commun 3, 887 (2012).
  • Xu et al. (2014) X. Xu, W. Yao, D. Xiao,  and T. F. Heinz, Nat Phys 10, 343 (2014).
  • Li et al. (2013) X. Li, J. T. Mullen, Z. Jin, K. M. Borysenko, M. Buongiorno Nardelli,  and K. W. Kim, Phys. Rev. B 87, 115418 (2013).
  • Jin et al. (2014) Z. Jin, X. Li, J. T. Mullen,  and K. W. Kim, Phys. Rev. B 90, 045422 (2014).
  • Schilp et al. (1994) J. Schilp, T. Kuhn,  and G. Mahler, Phys. Rev. B 50, 5435 (1994).
  • Haug and Jauho (2008) H. Haug and A.-P. Jauho, Quantum Kinetics in Transport and Optics of Semiconductors, 2nd ed. (Springer-Verlag Berlin Heidelberg, 2008).
  • Knorr et al. (1996) A. Knorr, S. Hughes, T. Stroucken,  and S. Koch, Chemical Physics 210, 27 (1996).
  • Wang et al. (2016) H. Wang, C. Zhang, W. Chan, C. Manolatou, S. Tiwari,  and F. Rana, Phys. Rev. B 93, 045407 (2016).
Comments 0
Request Comment
You are adding the first comment!
How to quickly get a good reply:
  • Give credit where it’s due by listing out the positive aspects of a paper before getting into which changes should be made.
  • Be specific in your critique, and provide supporting evidence with appropriate references to substantiate general statements.
  • Your comment should inspire ideas to flow and help the author improves the paper.

The better we are at sharing our knowledge with each other, the faster we move forward.
""
The feedback must be of minimum 40 characters and the title a minimum of 5 characters
   
Add comment
Cancel
Loading ...
248033
This is a comment super asjknd jkasnjk adsnkj
Upvote
Downvote
""
The feedback must be of minumum 40 characters
The feedback must be of minumum 40 characters
Submit
Cancel

You are asking your first question!
How to quickly get a good answer:
  • Keep your question short and to the point
  • Check for grammar or spelling errors.
  • Phrase it like a question
Test
Test description