Splashing transients of 2D plasmons launched by swift electrons

See allHide authors and affiliations

Science Advances  27 Jan 2017:
Vol. 3, no. 1, e1601192
DOI: 10.1126/sciadv.1601192


Launching of plasmons by swift electrons has long been used in electron energy–loss spectroscopy (EELS) to investigate the plasmonic properties of ultrathin, or two-dimensional (2D), electron systems. However, the question of how a swift electron generates plasmons in space and time has never been answered. We address this issue by calculating and demonstrating the spatial-temporal dynamics of 2D plasmon generation in graphene. We predict a jet-like rise of excessive charge concentration that delays the generation of 2D plasmons in EELS, exhibiting an analog to the hydrodynamic Rayleigh jet in a splashing phenomenon before the launching of ripples. The photon radiation, analogous to the splashing sound, accompanies the plasmon emission and can be understood as being shaken off by the Rayleigh jet–like charge concentration. Considering this newly revealed process, we argue that previous estimates on the yields of graphene plasmons in EELS need to be reevaluated.

  • 2D plasmons
  • transition radiation
  • EELS
  • Reyleigh jet
  • splashing
  • formation zone
  • formation time
  • graphene


Since the first successful confirmation of surface plasmons (1, 2) on the platform of thin metal films, swift electrons have long been used to investigate plasmonic properties of ultrathin, or two-dimensional (2D), electron systems, including graphene plasmons recently (310). Electron energy–loss spectroscopy (EELS) (1, 3, 11), which uses swift electrons as a probe, has been an indispensable tool in studying 2D plasmons. On the other hand, despite the long history of studies of 2D plasmons (1, 2), the dynamic mechanism of how a swift electron launches 2D plasmons has never been clearly revealed.

This is because the impact of an electron will generate not only plasmons but also photons [the so called “transition radiation” (12, 13)], whose emission cannot be achieved at a single space-time point but demands a finite space-time region. Historically, the concepts of “formation time” and “formation zone” [that is, “it takes a relatively long time and, therefore, a long distance for an energetic electron to create a photon,” as retailed by Uggerhøj (14)] were first presented by Ter-Mikaelian in Landau’s seminar in 1952 (15). Landau strongly opposed these concepts at first (15), but soon realized their correctness and significance and further developed them in the Landau-Pomeranchuk-Migdal effect, which was experimentally confirmed 40 years later. The existence of formation time and formation zone reflects our ignorance about the exact moment and location at which a photon is generated. In the early days of the quantum uncertainty principle, Bohr already commented on the impossibility of describing the electron-photon interaction “without considering a finite space-time region” (16). Later, it was Ginzburg and colleagues (12, 13) who included the formation time and formation zone with mathematical form into the classical framework of transition radiation (established by Ginzburg and Frank in 1945) while still admitting that “comparatively little is known.”

Although the above space-time discussions in the context of photon emission have lasted for decades, similar discussions have never been conducted on the generation of plasmons in EELS experiments. This explains why the spatiotemporal process of 2D plasmon launching by a swift electron remains elusive after a long research history.

In this paper, we introduce the concepts of formation time and formation zone into plasmon generation in EELS. On the platform of a graphene monolayer, we show within the framework of classical electrodynamics the dynamical process of 2D plasmon launching by a swift electron affecting on the graphene monolayer (see movie S1 for this process). We link this dynamical process during the formation time of graphene plasmons to the deep-water hydrodynamic splashing phenomenon, in which a picosecond jet-like rise of excessive charge concentration is formed on graphene as an analog of the “Rayleigh jet” (also called “Worthington jet”) in hydrodynamic splashing (17, 18). In this newly revealed physical process, a significant part of electromagnetic energy has already been dissipated before graphene plasmons are generated. In view of this consideration, we show that previous estimates of graphene plasmon yields (36) from the electron energy–loss (EEL) spectra need to be reevaluated. Note that although we adopt graphene as the platform, our analysis is general in any 2D electron system. In addition, although the formal similarity of dispersion between hydrodynamic water waves and 2D electron systems (1923) [including graphene plasmons (24, 25)] has been investigated with some hydrodynamic wave–like phenomena predicted (2629), the analog to the splashing phenomenon has never been discussed.


Modeling of 2D plasmon launching by swift electrons

The model of calculation is schematically shown in Fig. 1. We consider a swift electron with charge q, moving with a velocity Embedded Image, where c is the speed of light in free space. Because the energy loss of the electron (coupled to plasmons and transition radiation) is much lower than the electron’s kinetic energy, the electron’s velocity is treated as constant (13). The space-time dependence of the current density due to the electron is classically described as Embedded Image, in which t = 0 when the electron goes through the origin. A graphene layer is located at the interface between medium 1 (z < 0) with permittivity ε1rε0 and medium 2 (z > 0) with permittivity ε2rε0, where ε0 is the permittivity of free space. To simplify the analysis, we set mediums 1 and 2 to be free space. As a typical 2D electron system, graphene can be characterized by two macroscopic variables (24): the deviation of the electron density from its average value Embedded Image and the associated current density Embedded Image, which depends on graphene’s surface conductivity σs. Here, we calculate graphene’s surface conductivity based on the Kubo formula (see section S2) (30, 31) and set the relaxation time to τ = 0.5 ps and the chemical potential in graphene to μc = 0.4 eV [well within experimental capabilities (32, 33)]. Because of the rotational symmetry of the system, all fields must be transverse magnetic and thus can be characterized by an electric field component Ez in the Embedded Image direction. By decomposing all the quantities into Fourier components in time and in the coordinates Embedded Image with corresponding wavevectors Embedded Image, we haveEmbedded Image(1)Embedded Image(2)By writing the fields due to the electron field as Embedded Image and the radiation fields in regions of z < 0 and z > 0 as Embedded Image and Embedded Image, we can get the total fields in regions of z < 0 and z > 0 as Embedded Image and Embedded Image, respectively. Derivation from matching boundary conditions at the graphene plane shows phase relations of Embedded Image and Embedded Image, where “∓” in the exponent corresponds to “1,2” in the superscript of Embedded Image and Embedded Image (see section S2).

Fig. 1 Schematic of 2D plasmons launching with a swift electron penetrating through a graphene monolayer.

Lf1 and Lf2 are the lengths of the formation zone in the region above and below the graphene layer, respectively.

Formation zone and formation time

Ginzburg estimated the length of the formation zone (denoted as “formation length” Lf) for photon emission in transition radiation based on the following considerations (13). Inside the formation zone, the total energy of the fields Embedded Image is proportional to Embedded Image. The length Lf describes a boundary at which the total energy becomes practically equal to the sum of the energy of the electron field [that is, Embedded Image] and the energy of the radiation field [that is, Embedded Image] meaning that the electron field and the radiation field are separated from each other. That is, the interference term Embedded Image must play a trivial role. Ginzburg thus set the phase difference of 2π between Embedded Image and Embedded Image to determine the length Lf. That is, Embedded Image, which givesEmbedded Image(3)where Lf1 and Lf2 correspond to the length of the formation zones in regions of z < 0 and z > 0, respectively (see Fig. 1). Apparently, the formation length depends not only on the frequency of emitted photons and the swift electron’s velocity but also on the emission angle of photons. As a numerical example, with the electron’s velocity v = 0.8c, to emit a photon at frequency 10 THz in the backward −Embedded Image direction Embedded Image, it takes the electron about Embedded Image ps to accomplish it. For photon emission in the forward +Embedded Image direction Embedded Image at the same frequency, it takes about Embedded Image ps. These time intervals of 0.06 and 0.5 ps are considered as formation times for the backward and forward photon emission at 10 THz.

Ginzburg’s estimation only applies to photon emission with the condition Embedded Image to satisfy the square root in Eq. 3. Yet, it is well known that surface plasmons have Embedded Image. Compared to the electron-photon interaction as analyzed by Ginzburg, in the interaction between the electron and surface plasmons, only the electron field has phase variation along the z axis, whereas the surface plasmons have zero phase variation. Therefore, along the line of Ginzburg’s thought, the phase difference of 2π between Embedded Image and Embedded Image should only come from Embedded Image, that is, Embedded Image. This givesEmbedded Image(4)Numerically, it means that it will take the electron about (Lf1 + Lf2)/v = 0.2 ps to launch a 2D plasmon at 10 THz. The value 0.2 ps is considered as the formation time for the 2D plasmon at 10 THz.

Transients of photon emission

It is interesting to see what happens during the formation time of 2D plasmons when the electron goes through the formation zone, as schematically illustrated in Fig. 1. The dynamical process of photon emission and 2D plasmon launching by a swift electron moving with v = 0.8c (or kinetic energy 340 keV), which can be conveniently realized in modern electron microscope systems (1, 34), is shown in movie S1. (The relatively large velocity considered in this simulation shows that our theoretical analysis is not limited to low electron speeds.) The bandwidth of calculation is from 0 to 20 THz, as justified in fig. S3. Figure 2 shows the temporal evolution of photon emission. When the incident electron moves close to the graphene interface (Fig. 2A), its evanescent field touches graphene, expelling the conduction electrons from the vicinity of the swift electron’s trajectory. Because of electromagnetic induction, the induced surface current in turn blocks the penetration of the evanescent electron field by accumulating fields on the upper side of graphene (Fig. 2, A and B). Immediately after the electron crosses the graphene (Fig. 2, B and C), the fields previously accumulated on the upper side have lost direct contact with the electron and thus are “shaken off” into the upper space. Meanwhile, the insufficient fields on the lower side of graphene need to recover their strength in the presence of the electron and thus “shake off” radiation into the lower space (Fig. 2, C and D). It can be seen that, at the central frequency (10 THz) of the calculation bandwidth, the formation time of 0.06 ps for the backward radiation is consistent with Fig. 2 (A and B) and that of 0.5 ps for the forward radiation is consistent with Fig. 2 (C and D).

Fig. 2 Time evolution of magnetic field Embedded Image when a swift electron perpendicularly penetrates through a graphene monolayer.

The green dashed line represents graphene. The electron is located (A) above graphene, (B) at graphene, and (C) below graphene.

Transients of 2D plasmon launching

Of greater interest is the charge motion on graphene itself. We plot the dynamics of the deviation of electron density from its average value Embedded Image on graphene during the penetration of the swift electron in Fig. 3. Similarities to the hydrodynamic splashing scenario caused by a little droplet falling on a 2D liquid surface are evident, as described below.

Fig. 3 Time evolution of the deviation of the electron density from its average value on graphene plane Embedded Image when a swift electron penetrates through a graphene monolayer.

The electron is located (A and B) above graphene, (C) at graphene, and (D to H) below graphene.

First, in hydrodynamics (17, 18), when a small droplet affects a calm, deep-water surface, a crater is formed first and water splashes to the side. As the water rushes back to fill the crater, a central jet column called the Rayleigh jet due to its instability (17), or the Worthington jet because Worthington performed extensive observations back in 1908 (17, 18), will rise above the initial water surface along the collapse axis. When it comes to charge motion on graphene, a “crater” of the density of conduction electron in graphene is first formed when the incident electron approaches the graphene layer (Fig. 3, A to C). Immediately after the penetration of the electron through the graphene layer, a rebound of the density of conduction electrons is formed with a central jet-like rise (Fig. 3, D and E), analogous to the hallmark of Rayleigh jet or Worthington jet in hydrodynamics. We observe, as in Fig. 3E, that the jet-like rise reaches its peak at about t = 0.15 ps. Other analogs of this hydrodynamic splashing jet have also been widely discussed, including those occurring during the meteor impact (17, 18) and during the interaction between the highly focused femtosecond laser pulses and a metal film surface (35).

Second, after the central jet-like rise falls down, ripples of 2D plasmons propagate outward as concentric circles, as shown in Fig. 3, F to H. The excited 2D plasmons, which cover a broad spectrum of frequencies, gradually spread into a sequence of plasmonic ripples where longer-wavelength plasmons stay at the outer periphery and shorter-wavelength plasmons stay closer to the inner boundary (Fig. 3H). This is because the dispersion of 2D plasmons (including graphene plasmons) is typically Embedded Image (24, 25), which is formally analogous to the dispersion of deep-water waves; this is reflected in the fact that longer wavelengths go out faster (see section S4), although they are formed later (for their longer formation times) than the shorter wavelengths.

Energy of generated photons and 2D plasmons

We plot in Fig. 4A the time evolution of total radiated photon energy by numerically monitoring the Poynting power going through an imaginary sphere with a large radius R centered at the origin and then shifting the time axis backward by R/c, where the photon radiation is analogous to the sound emitted from a hydrodynamic splash. The total radiated photon energy eventually saturates and approaches a value of 0.171 × 10−4 eV that we calculate analytically by letting t = ∞ (see the Supplementary Materials). It can be seen that most photon energy has been radiated out before t = 0.15 ps, which is the moment when the jet-like rise of charge reaches its maximum (Fig. 3E) because most photon energy is shaken off by the charge jet. We also plot the time evolution of “energy” of the induced fields without considering the interference fields of the swift electron. Note that the 2D plasmons have not been fully generated before their formation times, so this energy should be treated as a parameter related to the field strength Embedded Image of induced charges but not as the real energy. It can be seen that even before most photon energy is radiated out, the field strength of Embedded Image has already started to drop.

Fig. 4 Energy dissipation during the plasmonic formation time.

(A) Time evolution of emitted photon energy and the induced field energy [related to the induced field strength Embedded Image]. (B) Energy spectra of graphene plasmons by taking t = ∞ in the lossless case and by taking t = Lf2/v in the lossy case.

We calculate the real energy of generated graphene plasmons by checking the electromagnetic energy for each frequency component immediately after the time t = Lf2/v. For the calculation spectrum of 2D plasmons from 0 to 20 THz, the corresponding formation time (Lf1 + Lf2)/v varies from ∞ to 0.1 ps, whose duration is comparable to the propagation time (~0.5 ps) for graphene plasmons (see section S4). The energy loss during the formation time cannot be taken into account by simply resorting to the propagation time or propagation length of 2D plasmons that are widely used to characterize the propagation of graphene plasmons because this energy loss happens before the generation of 2D plasmons themselves.

Only in the ideal lossless situation can one equate the EEL spectrum to the energy spectrum of generated 2D plasmons (the energy of emitted photons generally occupies only <5% of the energy loss of the swift electron, and considerably less for lower electron velocities, and thus is negligible). We plot in Fig. 4B the spectrum of 2D plasmons in the ideal lossless situation by taking t = ∞, which exactly agrees with the EEL spectrum calculation (see sections S5 and S6 and fig. S4). We also plot in Fig. 4B the spectrum of 2D plasmons for the realistic lossy graphene (the relaxation time is finite) after formation time is taken into account by taking t = Lf2/v. The comparison between the lossless and lossy cases shows that a significant portion of energy (more than 25% total energy from 0 to 20 THz) has already been dissipated before 2D plasmons are generated. In addition, the losses in graphene, including those caused by defects, can be theoretically characterized by the relaxation time, where a smaller relaxation time indicates a larger loss. If more defects exist in the graphene sample, this will unavoidably degrade the relaxation time used in this work (0.5 ps), resulting in a larger loss in graphene, and it is thus expected that a larger portion of energy will be dissipated before 2D plasmons are generated.


Recent advances in electron microscopy now suggest a new way to observe the temporal dynamics of the plasmons, including its ultrafast and subwavelength features, by using photon-induced near-field electron microscopy (7, 36). This exciting possibility will allow one to visualize the plasmonic splashing-like effects, instead of inferring them indirectly through EELS or transition radiation measurements.

Because graphene is just one typical example of many different 2D electron gas systems (1923, 37, 38) that support 2D plasmons, our analysis could be applicable to any 2D electron system. Therefore, other 2D electron gas systems (1923), and particularly other 2D materials (37, 38), will likely further enrich the potential implementations of plasmonic splashing-like transients. However, we argue that graphene is particularly suitable for this purpose because of the flexible tunability of the chemical potential and the recent advances in the fabrication of graphene samples with large area, high quality, and the precise control of the layer number. In addition, it is reported that van der Waals materials can support different kinds of polaritons (38), such as phonon polaritons in a boron nitride slab (37, 38). We thus expect more polaritonic splashing-like transient to be revealed in van der Waals materials.

The above results demonstrate the transients of 2D plasmon generation in EELS experiment. An intermediate process between the impact of the swift electron and the formation of 2D plasmons is revealed as a result of the space-time limitation on plasmon generation. This process is found to be analogous to the hydrodynamic splashing phenomenon. Explicit calculation that takes into account the energy dissipation before 2D plasmons are generated has shown that previous estimates on the yields of graphene plasmons in EELS under the assumption of negligible loss need to be reevaluated.


Our rigorous analytical calculations are based on an extension of Ginzburg and Frank’s theory on transition radiation within the framework of macroscopic electrodynamics. This can give us an analytical expression of the radiated fields induced by swift electrons. From this, we can further analytically derive the spectrum of emitted photons; with the assumption of trivial losses in the calculated system, we can also analytically derive the EEL spectrum. Because the EEL spectrum is derived without the assumption of the electrostatic approximation, our analytical formula of the EEL spectrum is applicable to the cases with high electron kinetic energies. Furthermore, by choosing the appropriate Sommerfeld branch cut and using the Sommerfeld integration path, numerical calculation of the radiated fields at different times can be carried out. Therefore, the emitted photon energy, the induced field energy, and the energy spectrum of induced charges on lossy graphene at different times can be numerically obtained by applying these numerically calculated radiated fields.


Supplementary material for this article is available at

section S1. Figure caption of movie S1.

section S2. Photon emission from graphene affected by swift electrons.

section S3. Energy spectrum of induced charges on graphene.

section S4. Dispersion relation and propagation length/time of graphene plasmons.

section S5. Analytical EEL spectrum.

section S6. Comparison of EEL spectra between previous work and our result.

section S7. Total energy of emitted photons.

section S8. Numerical implementation with Sommerfeld integration.

fig. S1. Dispersion curve of TM graphene plasmons.

fig. S2. Propagation time of TM graphene plasmons as a function of frequency.

fig. S3. EEL spectrum when an electron normally incident on an ideal lossless graphene layer.

fig. S4. EEL spectra for an electron normally incident on graphene.

movie S1. Time evolution of 2D plasmons launched by swift electrons.

References (3952)

This is an open-access article distributed under the terms of the Creative Commons Attribution-NonCommercial license, which permits use, distribution, and reproduction in any medium, so long as the resultant use is not for commercial advantage and provided the original work is properly cited.


Acknowledgments: We thank L. Lu for helpful discussions. Funding: This work was sponsored by the National Natural Science Foundation of China (grant nos. 61625502, 61574127, 61601408, and 61550110245), the Zhejiang Natural Science Foundation (grant no. LY17F010008), the Postdoctoral Science Foundation of China (grant no. 2015M581930), the Top-Notch Young Talents Program of China, the Innovation Joint Research Center for Cyber-Physical-Society System, the Nanyang Technological University for Nanyang Assistant Professorship Start-Up Grant, the Singapore Ministry of Education (grant nos. MOE2015-T2-1-070 and MOE2011-T3-1-005), the U.S. Army Research Laboratory and the U.S. Army Research Office through the Institute for Soldier Nanotechnologies (contract no. W911NF-13-D-0001), the Massachusetts Institute of Technology S3TEC Energy Frontier Research Center of the Department of Energy (grant no. de-sc0001299), the QuantiXLie Center of Excellence, and the Chinese Scholarship Council (CSC 201506320075). Author contributions: All authors contributed extensively to this work. B.Z. conceived the idea. X.L. performed the main calculations. X.S., Z.Y., F.G., and Z.G. contributed to the numerical Sommerfeld integration and the analytical calculations on photon radiation. I.K. contributed to the EEL spectrum calculation. X.L., I.K., H.B., J.D.J., M.S., H.C., and B.Z. analyzed the data and discussed and interpreted the detailed results. I.K., H.C., and B.Z. supervised the project. All authors discussed, revised, and approved the manuscript. Competing interests: The authors declare that they have no competing interests. Data and materials availability: All data needed to evaluate the conclusions in the paper are present in the paper and/or the Supplementary Materials. Additional data related to this paper may be requested from the authors.

Stay Connected to Science Advances

Navigate This Article