## Abstract

The ultrafast saturable absorption in graphene is experimentally and theoretically investigated in the femtosecond (fs) time regime. This phenomenon is well-modeled with valence band depletion, conduction band filling and ultrafast intraband carrier thermalization. The latter is dominated by intraband carrier-carrier scattering with a scattering time of 8 ( ± 3) fs, which is far beyond the time resolution of other ultrafast techniques with hundred fs laser pulses. Our results strongly suggest that graphene is an excellent atomic layer saturable absorber.

© 2010 OSA

## 1. Introduction

Graphene is new class of single atom thick materials which possesses a unique smooth-sided conical band structure that converges to a single Dirac point [1–4]. In the recent years, graphene has been subjected to extensive studies [1–19]. Among these studies, there are several reports on the effects of weak light interaction with graphene. Within the model of the non-interacting, massless Dirac fermions [1,2], the weak light absorption is calculated to be independent of frequency and to have a universal opacity, *π*·*α* = 2.3% (where *α* is the fine structure constant) [5–7]. This theoretical prediction has been confirmed by recent infrared to visible reflectivity and transmission measurements [8–11]. However, studies on the coupling between photons and fermions in graphene under high intensity, ultrashort laser pulse excitation are limited [12–17]. In particular, the relationship between the nonlinear optical properties of graphene and the basic fine structure constant has never been investigated.

Here, we experimentally characterized and theoretically modeled the ultrafast saturable absorption in graphene, which was epitaxially grown on a transparent wide bandgap semiconductor SiC substrate. Our findings revealed that graphene possesses excellent saturable absorption properties with low saturation intensity; controllable saturation depth; ultrafast recovery time; near symmetric spatio-temporal narrowing and high damage threshold. Its ultrafast saturation absorption properties are well-described by the effects of valence band depletion, conduction band filling and ultrafast intraband carrier relaxation. The latter is dominated by intraband carrier-carrier (c-c) scattering with a scattering time of 8 ( ± 3) femtoseconds (fs), which is far beyond the time resolution of other ultrafast techniques with hundred fs laser pulses. Graphene presents us with a unique system to model these non-linear effects with fundamental physics. Key to the development of practical graphene-based optoelectronic devices is through a clear understanding of its intrinsic optical properties.

## 2. Graphene characterization

In our experiments, bi-layer graphene with rotational stacking faults (30.0 or ± 2.20°) was epitaxially grown on both sides of a 0.4 mm thick n-type C-terminated 6H-SiC (0001) substrate. The thickness of graphene was measured by monitoring the attenuation of the bulk SiC component in the Si 2p photoemission spectroscopy signal and confirmed with the Raman spectrum [18–21]. Due to the different stacking structure compared to hexagonal Bernal graphite, the layers are effectively decoupled [22]. Raman spectroscopy was performed to determine the quality of the epitaxial graphene as well as to confirm the number of layers. The measurements were carried out with a WITEC CRM200 Raman system with 488 nm (2.54 eV) excitation and a spot size of diameter ~500 nm with a 100 × microscope objective (NA = 0.95).

In Fig. 1
, the in-plane vibrational G peak at ~1577 cm^{−1} and the two-phonon 2D peak at ~2717 cm^{−1} are clearly identifiable. The smaller peaks at ~1520 cm^{−1} and ~1713 cm^{−1} originate from the 4H-SiC substrate. The former is the overtone of the SiC TO(X) phonon at 761 cm^{−1} while the latter is a combination of the optical phonons with wave vectors near the M point at the zone edge of the SiC substrate [19,20]. The relatively small defect-induced D band (~1360 cm^{−1}) suggests good crystallinity in the graphene samples. The comparable Raman intensity of the G band and the 2D band as well as the broad 2D band (at 100 cm^{−1}) confirms the primarily two-layer nature of the graphene sample [19]. A Raman image obtained using the intensity of the G-band is shown in the inset of Fig. 1. The G-band intensity is known to increase almost linearly with the number of graphene layers [21]. The relative uniformity of the graphene layers is also evident from the large area uniformity of the G-band intensity shown in Fig. 1 inset.

## 3. Ultrafast saturable absorption investigation

Z-scan technique was used to investigate the pump intensity dependent transmittance [23]. The 1 kHz, 200fs wide laser pulses, centered at 800 nm, were generated from a Coherent Legend^{TM} regenerative amplifier that was seeded by a Coherent Mira^{TM} oscillator. The full-width-at-half-maximum of the photon energy dispersion was 0.04 eV. The laser pulse was focused perpendicular on the sample with a lens of focal length 30 cm. The beam waist at the focus was 31 ± 2 μm and was confirmed with a standard two-photon absorption experiment on a 0.5 mm thick ZnSe bulk crystal. In our experiments, as the graphene sample was translated through the focal point along the laser propagation axis, the transmittances at different *z* positions were recorded. The effects of the ultrafast saturable absorption and the spatio-temporal reshaping of the transmitted 800nm fs pulses in graphene were analyzed. The response from a bare SiC substrate was also measured under the same conditions and at the same pump intensities (≤ 120 GW/cm^{2}) where negligible nonlinear absorption has been found. The nonlinear absorption from SiC substrate will be obvious at 200 GW/cm^{2}, where, graphene still shows saturable absorption.

In graphene, the excitation process near the Dirac point can be described by the Dirac Hamiltonian with linear wavevector dependent energy dispersion (*ε = ћν _{F}|k|*, where

*ν*= 10

_{F}^{6}

*m/s*is the Fermi velocity) as shown in Fig. 2(a) . For epitaxially grown graphene layers on SiC substrate, the first layer is highly doped and the Fermi level is located at approximately 0.35 eV in conduction band [13]. However, this doping will not affect the photon absorption at 1.55 eV [Fig. 1(a)]. After photoexcitation by 1.55 eV (800 nm) fs laser pulses, a non-equilibrium population of electrons in the conduction band (

*ε = ћω/2*) and holes in valence band (

*ε*= -

*ћω*/2) is created with momentum conservation. Here, the effects of triangular warping and other nonlinear effects have been found to be negligible even at visible wavelengths (i.e. up to 3.1 eV) [7,10]. From Fermi’s golden rule, the instantaneous absorbed power is:

*ћω*is the photon energy,

*D( ± ћω/2) = ћω/(πћ*are the density of states at

^{2}ν_{F}^{2})*ε = ± ћω/2*and ƒ

_{t}(ε) is the electron occupation probability at time

*t*. The Dirac fermion transition matrix

*M*

_{t}from initial state $|m\u3009$ to final state $|n\u3009$ under the perturbation of incident electromagnetic field at time

*t*is [10]:

Under low optical excitation where the carriers undergo fast interband decay in graphene [12–15], it is reasonable to use the following approximations: ƒ_{t}(-*ћω*/2) ≈1 and ƒ_{t}(*ћω*/2) ≈0. With the incident power ${W}_{t}^{i}=(c/4\pi ){I}_{t}$, the linear optical transmittance can be calculated as:

It is dependent on the fine structure constant *α* but independent of the excitation wavelength and the material parameter *ν _{F}*.

In contrast, high intensity excitation creates large temporal populations of carriers in the valence band (VB) and the conduction band (CB). Further absorption of incoming photons at the same energy (within the pulse duration) will be reduced, giving rise to a bleaching effect seen in Fig. 2(c) as increased transmittance. Concurrently, the nonequilibrium carrier distributions in the CB and VB will undergo ultrafast intraband relaxation through non-dissipative c-c scattering and to a slower extent by carrier-optical phonon (c-op) coupling. Free carrier absorption in graphene is unlikely as such process require the assistance of phonons for momentum conservation. Thermalization is quickly achieved leaving ultra high temperature Fermi-Dirac distributions in the VB and CB [Fig. 2(b)]. Subsequently, optical and acoustic phonon processes take place on a longer timescale to cool the carrier distributions along with electron-hole recombination [12–15]. For a Gaussian temporal pump pulse with uniform spatial component, *I _{t}* can be expressed as

*I*exp(

_{0}*-t*). The dynamics for VB and CB electron occupation probabilities $f\left(\mp \epsilon \right)$can then be described by:

^{2}/τ^{2}*τ*is half-width at 1/

*e*of the maximum of laser pulse and

*τ*is the ultrafast carrier relaxation time which is dominated by intraband c-c scattering. The first and second terms on the right hand side (RHS) of Eqs. (4) and (5) represent the photon-absorption-induced electron occupation probability balance between the valence band and conduction band. The third term on the RHS of Eq. (4) (or Eq. (5)) is derived from hole (or electron) relaxation increasing (or decreasing) in the valence (or conduction) band respectively. The initial conditions prior to laser excitation are:

_{1}Equations (4), (5) and (6) can be solved together to give the result as:

*Erf*[

*x*] is the Gaussian error function.

The absorbed energy per unit area for one pulse can be written as:

For a real focused Gaussian laser pulse, both the temporal and spatial profiles follow a Gaussian distribution, then

*w*is the minimum beam waist,

_{0}*λ*is the pump laser wavelength,

*z*is on-axis relative position to the focal point,

*r*is radial coordinate and

*I*

_{00}is the on-axis peak irradiance at the focal point.

Integrating Eq. (9) over the cross-section at *z*, the absorbed energy per pulse is:

Using Eq. (11), a good fit of the experimental data in Fig. 2(c) (solid line) is obtained with *τ*
_{1} as the only fitting parameter. Our fitted value *τ*
_{1} (7 ± 3 fs) agrees well with the 13±3 fs intraband carrier equilibration time reported by Breusing *et al*. for 20 – 30 nm thick graphite that was probed using transient absorption spectroscopy with 7 fs laser pulses [15]. *τ*
_{1} comprises contributions from both the intraband c-c scattering and the dissipative c-op coupling, i.e. *τ _{1} = τ_{c-c} τ_{c-op}/(τ_{c-c} + τ_{c-op})*, where

*τ*and

_{c-c}*τ*

_{c-op}refer to the lifetimes for c-c scattering and c-op coupling respectively. It is usual that

*τ*

_{c-op}»

*τ*so that

_{c-c}*τ*

_{1}≈

*τ*. A typical value of

_{c-c}*τ*is ~100 fs [15]. From this approximation, the ultrafast intraband c-c scattering time,

_{c-op}*τ*is calculated to be 8 ± 3 fs. Such ultrafast dynamics in graphene is far beyond the temporal resolution of typical pump-probe experiments conducted with hundred fs pulses [12,14].

_{c-c}Next, we consider the ultrafast intraband carrier thermalization (dominated by the intraband c-c scattering) in the absence of energy dissipation. Transient Fermi-Dirac distributions can be established at ultra high temperatures *T*
_{0} with different chemical potentials (*μ*
_{e} and *μ*
_{h}) according to the following conditions of particle number and energy conservation:

When exciting a single layer of graphene with *ћω* = 1.55 eV photons, the dependence of the electron temperature (*T*
_{e}) and corresponding chemical potential (*μ*
_{e}) on the electron density (*N*
_{e}) are shown in Fig. 3
. The thermalized *T*
_{e} mono decreases while the corresponding *μ*
_{e} mono increases as *N*
_{e} increases. For *N*
_{e} = 1.9 × 10^{5}/um^{2}, a thermalized *T*
_{e} = 4000 K will be obtained. At the threshold electron density, *N*
_{th} = 1.5 × 10^{5}/um^{2}, the thermalized temperature is equal to the Fermi temperature of *N*
_{th}. This corresponds to *μ*
_{e}(*N*
_{th}) = 0. For electron density *N*
_{e} < *N*
_{th} (in the limit of low laser pump intensity), the established temperature will be greater than the Fermi temperature of *N*
_{e}. At this electron density, more of the fermions are in the higher excited states within the CB. This results in *μ*
_{e}(*N*
_{e}) < 0. One possibility is that at high temperatures, the fermion gas approaches the classical ideal gas. In addition, the threshold electron density *N*
_{th} is dependent on the pump photon energy (*ћω*). With *μ*
_{e} = 0 and the conditions of Eq. (12), the following relationship can be deduced: ${N}_{th}=8.9\times {10}^{-5}{\pi}^{5}{(\hslash \omega )}^{2}/{(\hslash {v}_{F})}^{2}$. In the absence of optical phonon coupling, under 1.55 eV photon excitation, the highest electron density that can be populated in graphene is around 5.8 × 10^{5}/um^{2}. Beyond this upper limit, 100% transmittance for the subsequent incoming photons will be observed.

The effects of sudden photon absorption and subsequent c-c scattering on the intrinsic ultrafast saturable absorption of monolayer graphene can be demonstrated from the temporal and spatial distortion in the transmitted laser pulses. From Eq. (7), the temporal transmittance at *t* is derived as:

Likewise, the transverse transmittance at $z=0$ can be written as:

From these, the transmitted temporal and spatial profiles through graphene are calculated for different intensities and plotted in Fig. 4(b)
and 4(d). The solid lines in Fig. 4(b) are derived from *τ*
_{1} = 7 fs along with the same parameters as used in our experiments. Similarly, the calculated spatial profiles are shown in Fig. 4(d). For comparison, the input temporal and spatial laser profiles are plotted in Fig. 4(a) and 4(c). In Fig. 4(b) the calculated maximum transmittance occur a few fs after time zero which is taken to be the center of the temporal profile. This asymmetry in the temporal profile arises due to the two competing processes during the accumulation of carriers in the VB and CB: photo absorption of incoming photons at the same energy (within the pulse duration) and the intraband c-c scattering (that leads to the redistribution of the carriers). This causes a delay in reaching the maximum transmittance. The narrowing of the temporal profile of the transmitted pulses occurs when the pump intensity is increased from 1 to 5 GW/cm^{2}. But this effect becomes less obvious at higher pump intensities (80 GW/cm^{2}). This is attributed to the saturation of the saturable absorption, which is dependent on the saturation depth of the materials. From Fig. 4(d), the narrowing of the spatial profiles shows a similar trend to that of the temporal profiles. Unlike the temporal case, the transmittances of the spatial profile always show symmetrical narrowing.

The transmitted laser pulse temporal shape is strongly dependent on the intraband carrier thermalization time. To clearly illustrate this dependence, the dashed lines in Fig. 4(b) were calculated using *τ*
_{1} = 100 fs and all other parameters remain the same. The narrowing of the temporal profile and the subsequent saturation of the saturable absorption occurs at much lower pump intensities compared to that with *τ*
_{1} = 7 fs. In light of the competing processes discussed earlier, the temporal transmittance profile is more asymmetrical. The transmittance also has a longer tail, which is caused by the slower intraband carrier relaxation.

The strong saturable absorption in atomic layer graphene is attributed to two main reasons: Firstly, the wavelength independent strong linear absorption (*πα* = 2.3%) of graphene provides a potential saturable absorption depth (i.e. maximum change in transmittance). This large linear absorption arises from the unique properties of graphene: i.e. two dimensional massless fermions and a conical band structure. Secondly, the excited states absorption in graphene is momentum forbidden and they require the assistance of phonons. The only photon coupling process for the excited state electrons is through stimulated emission (*ε*(*ћω*/2) → *ε*(-*ћω*/2)). The nonlinear optical properties of graphene and graphene oxide were previously investigated using picosecond and nanosecond lasers on small pieces of sample dispersed in a solution [16,17]. However, the high thermal conductivity, large linear absorption and small sample size together with the long laser pulses will inevitably generate solvent bubbles and micro-plasmas. In contrast to our findings, these earlier results were dominated by the nonlinear scattering.

It is also possible to control the saturation depth in graphene through varying the number of atomic layers. As the epitaxial grown layers on SiC are effectively decoupled, the light can be considered to be transmitting sequentially through different layers. Figure 5
shows the calculated transmission dependence on the incident pump intensity for different atomic layers at the focal point. It clearly shows that the saturation depth is nearly proportional to the number of layers and the saturation onset is as low as 0.1 GW/cm^{2}. However, due to the ultrafast intraband c-c dynamics, a pump intensity as high as 1000 GW/cm^{2} is needed to reach the maximum transmittance. For the graphene layers epitaxially grown on SiC substrate, the SiC nonlinear absorption signals will dominate in the Z-scans above 200 GW/cm^{2} at 1.55 eV. The damage threshold of graphene is determined to be higher than 300 GW/cm^{2}.

For applications as a saturable absorber, the saturation intensity (*I*
_{s}) is another crucial parameter [24]. The attenuation of the incident light through a single graphene layer can be described by:

*I*

_{in}is the input light intensity,

*I*

_{T}is the transmitted light intensity,

*α*

_{0}is the linear absorption coefficient of a single layer of graphene,

*I*

_{s}is the saturation intensity of a single layer of graphene. Considering that light sequentially passes through the different graphene layers, the

*z*position dependent transmittance is calculated from the ratio of the energy of the transmitted pulse to that of the incident pulse. These energies are obtained by integrating

*I*

_{T}and

*I*

_{in}(for a Gaussian pulse) over the temporal and spatial domains. Figure 6(a) shows a typical experimental data fitted with

*I*

_{s}as the only unknown parameter. Figure 6(b) shows the obtained saturation intensities vs. pump intensities. The saturation intensity was found to be ~4( ± 1) GW/cm

^{2}for a single layer of graphene and it is independent of the pump intensity.

## 4. Conclusion

The ultrafast saturable absorption properties of graphene is experimentally characterized and theoretically modeled in the femtosecond time regime. The saturable absorption properties of graphene are well-modeled with valence band depletion, conduction band filling and ultrafast intraband carrier thermalization. The ultrafast intraband carrier thermalization is dominated by intraband c-c scattering. With our method of *z*-scan measurements in conjunction with theoretical calculations, the scattering time is determined to be 8 ( ± 3) fs. Such ultrafast c-c dynamics is far beyond the time resolution of other ultrafast techniques with typical hundred fs laser pulses. In addition, our results show that the spatiotemporal profiles of an intense Gaussian pulse narrow upon transmission through graphene. This narrowing can be controlled either by tuning the incident light intensity or by varying the number of layers. Our findings reveal that graphene possesses great potential for applications as passive mode-lockers, optical pulse shapers or output couplers. Graphene, with all its fascinating properties, continues to offer us new insights into the field of nonlinear optics and their applications.

## Acknowledgements

This research is supported by a grant from the Academic Research Fund (AcRF) Tier 1 – RG 49/08 (M52110082) and a NTU start-up grant under Grant No. M58110068.

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